Gaëtan Borot

Jérémie Bouttier

Bertrand Duplantier

Timothy Budd

Philippe Di

Clément Hongler

Jason Miller

NESTING STATISTICS IN THE O(n) LOOP MODEL ON RANDOM PLANAR MAPS

In the O(n) loop model on random planar maps, we study the depthin terms of the number of levels of nesting -of the loop configuration, by means of analytic combinatorics. We focus on the 'refined' generating series of pointed disks or cylinders, which keep track of the number of loops separating the marked point from the boundary (for disks), or the two boundaries (for cylinders). For the general O(n) loop model, we show that these generating series satisfy functional relations obtained by a modification of those satisfied by the unrefined generating series. In a more specific O(n) model where loops cross only triangles and have a bending energy, we explicitly compute the refined generating series. We analyse their non generic critical behavior in the dense and dilute phases, and obtain the large deviations function of the nesting distribution, which is expected to be universal. Using the framework of Liouville quantum gravity (LQG), we show that a rigorous functional KPZ relation can be applied to the multifractal spectrum of extreme nesting in the conformal loop ensemble (CLE κ ) in the Euclidean unit disk, as obtained by Miller, Watson and Wilson [120], or to its natural generalisation to the Riemann sphere. It allows us to recover the large deviations results obtained for the critical O(n) random planar map models. This offers, at the refined level of large deviations theory, a rigorous check of the fundamental fact that the universal scaling limits of random planar map models as weighted by partition functions of critical statistical models are given by LQG random surfaces decorated by independent CLEs.

Introduction

The enumeration of planar random maps, which are models for discretised surfaces, developed initially from the work of Tutte [START_REF] Tutte | A census of planar triangulations[END_REF][START_REF] Tutte | A census of planar maps[END_REF][START_REF] Tutte | On the enumeration of planar maps[END_REF]. The discovery of matrix model techniques [START_REF] Brézin | Planar diagrams[END_REF] and the development of bijective techniques based on coding by decorated trees [START_REF] Cori | Planar maps are well-labeled trees[END_REF][START_REF] Schaeffer | Conjugaison d'arbres et cartes combinatoires aléatoires[END_REF] led in the past thirty years to a wealth of results. An important motivation comes from the physics conjecture that the geometry of large random maps is universal, i.e., there should exist ensembles of random metric spaces depending on a small set of data (like the central charge and a symmetry group attached to the problem) which describe the continuum limit of random maps. Two-dimensional quantum gravity aims at the description of these random continuum objects and physical processes on them, and the universal theory which should underlie it is Liouville quantum gravity, possibly coupled to a conformal field theory [START_REF] Francesco | 2d gravity and random matrices[END_REF][START_REF] Ginsparg | Lectures on 2d gravity and 2d string theory[END_REF][START_REF] Knizhnik | Fractal structure of 2D-quantum gravity[END_REF][START_REF] Polyakov | Quantum geometry of bosonic strings[END_REF]. Understanding rigorously the emergent fractal geometry of such limit objects is nowadays a major problem in mathematical physics and in probability theory. Another important problem is to establish the convergence of discrete random planar maps towards such limit objects. Solving various problems of map enumeration is often instrumental in this program, as it provides useful probabilistic estimates.

As of now, the geometry of large random planar maps with faces of bounded degrees (e.g., quadrangulations) is fairly well understood, thanks to recent spectacular progress. In particular, their scaling limit is the so called Brownian map [START_REF] Gall | The topological structure of scaling limits of large planar maps[END_REF][START_REF] Gall | Uniqueness and universality of the Brownian map[END_REF][START_REF] Marckert | Limit of normalized random quadrangulations: the Brownian map[END_REF][START_REF] Miermont | The Brownian map is the scaling limit of uniform random plane quadrangulations[END_REF][START_REF] Miller | An axiomatic characterization of the Brownian map[END_REF], with its convergence in the Gromov-Hausdorff sense established by Le Gall and Miermont in Refs. [START_REF] Gall | Uniqueness and universality of the Brownian map[END_REF][START_REF] Miermont | The Brownian map is the scaling limit of uniform random plane quadrangulations[END_REF]. Another major progress is the recent construction by Miller and Sheffield, via the so called quantum Loewner evolution [START_REF] Miller | Quantum Loewner evolution[END_REF], of a metric structure for Liouville quantum gravity (at Liouville parameter γ = 8 3 ), and the proof that it is indeed equivalent to that of the Brownian planar map [START_REF] Miller | Liouville quantum gravity as a metric space and a scaling limit[END_REF][START_REF] Miller | Liouville quantum gravity and the Brownian map I: The QLE(8/3,0) metric[END_REF][START_REF] Miller | Liouville quantum gravity and the Brownian map II: geodesics and continuity of the embedding[END_REF][START_REF] Miller | Liouville quantum gravity and the Brownian map III: the conformal structure is determined[END_REF].

This universality class is often called in physics that of pure gravity. Recent progress generalised part of this understanding to other universality classes, those of planar maps containing faces whose degrees are drawn from a heavy tail distribution. In particular, the limiting object is the so-called α-stable map, which can be coded in terms of stable processes whose parameter α is related to the power law decay of the degree distribution and to the Hausdorff dimension of the random map [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF][START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF][START_REF] Gall | Scaling limits of random planar maps with large faces[END_REF].

The next class of interesting models concerns random maps equipped with a statistical physics model, like the Ising model [START_REF] Boulatov | The Ising model on a random planar lattice: the structure of the phase transition and the exact critical exponents[END_REF][START_REF] Kazakov | Ising model on a dynamical planar random lattice: Exact solution[END_REF], percolation [START_REF] Kazakov | Exactly solvable Potts models, bond-and tree-like percolation on dynamical (random) planar lattice[END_REF], the O(n) model [17, 18, 54, 55, 65-68, 74, 100, 103], the Q-Potts model [START_REF] Bonnet | The Potts-q random matrix model: loop equations, critical exponents, and rational case[END_REF][START_REF] Borot | Loop models on random maps via nested loops: case of domain symmetry breaking and application to the Potts model[END_REF][START_REF] Daul | Q-states Potts model on a random planar lattice[END_REF]146], or non intersecting random walks [START_REF] Duplantier | Random walks and quantum gravity in two dimensions[END_REF][START_REF] Duplantier | Conformal invariance and intersections of random walks[END_REF]. The O(n) model admits a famous representation in terms of loops [START_REF] Domany | Duality relations and equivalences for models with O(n) and cubic symmetry[END_REF][START_REF] Nienhuis | Coulomb gas formulation of two-dimensional phase transitions[END_REF] with n being the fugacity per loop. It is also well known, at least on fixed lattices [START_REF] Baxter | Equivalence of the Potts model or Whitney polynomial with an ice-type model[END_REF][START_REF] Nijs | Extended scaling relations for the magnetic critical exponents of the Potts model[END_REF][START_REF] Duplantier | Critical exponents of Manhattan Hamiltonian walks in two dimensions, from Potts and O(n) models[END_REF][START_REF] Fortuin | On the random-cluster model. I-introduction and relation to other models[END_REF][START_REF] Nienhuis | Coulomb gas formulation of two-dimensional phase transitions[END_REF][START_REF] Perk | Nonintersecting string model and graphical approach: equivalence with a Potts model[END_REF][START_REF] Truong | Structural properties of a Z(N 2 )-spin model and its equivalent Z(N )-vertex model[END_REF], that the critical Q-state Potts model, via its Fortuin-Kasteleyn (FK) cluster representation, can be reformulated as a fully packed loop model with a fugacity √ Q per loop; for planar random maps this equivalence is explained in detail as was repeatedly checked for a series of models [START_REF] Duplantier | Conformal fractal geometry & boundary quantum gravity[END_REF][START_REF] Duplantier | Conformal spectra of polymers on a random surface[END_REF][START_REF] Duplantier | Geometrical critical phenomena on a random surface of arbitrary genus[END_REF][START_REF] Kazakov | Ising model on a dynamical planar random lattice: Exact solution[END_REF][START_REF] Knizhnik | Fractal structure of 2D-quantum gravity[END_REF][START_REF] Kostov | O(n) vector model on a planar random lattice: spectrum of anomalous dimensions[END_REF]. In the framework of Liouville quantum gravity, the KPZ relations have now been mathematically proven for the Liouville measure defined as the (renormalised) exponential of the Gaussian free field (GFF) times a parameter γ ∈ [0, 2] [62], as well as in the context of Mandelbrot multiplicative cascades [START_REF] Barral | Critical Mandelbrot cascades[END_REF][START_REF] Benjamini | KPZ in one dimensional random geometry of multiplicative cascades[END_REF] and Gaussian multiplicative chaos [START_REF] Barral | Gaussian multiplicative chaos and KPZ duality[END_REF][START_REF] Duplantier | Renormalization of critical Gaussian multiplicative chaos and KPZ relation[END_REF][START_REF] Rhodes | KPZ formula for log-infinitely divisible multifractal random measures[END_REF].

It is widely believed that after a Riemann conformal map to a given planar domain, the correct conformal structure for the continuum limit of random planar maps weighted by the partition function of a critical statistical model is described by the theory of Liouville quantum gravity (LQG), coupled to the conformal field theory (CFT) representing the conformally invariant model at its critical point (see, e.g., the reviews [START_REF] Francesco | 2d gravity and random matrices[END_REF][START_REF] Ginsparg | Lectures on 2d gravity and 2d string theory[END_REF][START_REF] Nakayama | Liouville field theory: a decade after the revolution[END_REF] and [START_REF] Duplantier | Liouville quantum gravity, KPZ and Schramm-Loewner evolution[END_REF][START_REF] Gall | Random Geometry on the Sphere[END_REF]). In a more probabilistic setting, one expects the continuum limit after conformal embedding to be some form of Liouville random surface decorated by Schramm-Loewner evolution (SLE) paths.

There are now several senses in which random planar maps with statistical models have been rigorously proved to converge to LQG surfaces, as path-decorated metric spaces in the self-avoiding walk and percolation models cases [START_REF] Gwynne | Convergence of percolation on uniform quadrangulations with boundary to SLE 6 on 8/3-Liouville quantum gravity[END_REF][START_REF] Gwynne | Convergence of the self-avoiding walk on random quadrangulations to SLE 8/3 on 8/3-Liouville quantum gravity[END_REF][START_REF] Miller | Liouville quantum gravity as a metric space and a scaling limit[END_REF], as mated pairs of trees [START_REF] Gwynne | Joint scaling limit of a bipolar-oriented triangulation and its dual in the peanosphere sense[END_REF][START_REF] Gwynne | Active spanning trees with bending energy on planar maps and SLE-decorated Liouville quantum gravity for κ > 8[END_REF][START_REF] Kenyon | Bipolar orientations on planar maps and SLE 12[END_REF][START_REF] Li | Schnyder woods, SLE(16), and Liouville quantum gravity[END_REF][START_REF] Sheffield | Quantum gravity and inventory accumulation[END_REF], or as Tutte discrete embedding of so-called mated-CRT maps [START_REF] Gwynne | The Tutte embedding of the mated-CRT map converges to Liouville quantum gravity[END_REF], using results for the continuum mating of continuum random trees (CRT) [START_REF] Duplantier | Liouville quantum gravity as a mating of trees[END_REF][START_REF] Miller | Liouville quantum gravity spheres as matings of finite-diameter trees[END_REF]. This approach was recently extended to graph distances [START_REF] Gwynne | A mating-of-trees approach to graph distances in random planar maps[END_REF] and random walk [START_REF] Gwynne | Random walk on random planar maps: spectral dimension, resistance, and displacement[END_REF] on random planar maps.

The first instance was the proof by Sheffield [START_REF] Sheffield | Quantum gravity and inventory accumulation[END_REF] in the infinite volume case of the convergence of quadrangulations equipped with the FK clusters of a critical Potts model to LQG decorated by SLE, while the finite/sphere case was recently studied in [START_REF] Gwynne | Scaling limits for the critical Fortuin-Kasteleyn model on a random planar map I: cone times[END_REF][START_REF] Gwynne | Scaling limits for the critical Fortuin-Kasteleyn model on a random planar map III: finite volume case[END_REF][START_REF] Gwynne | Scaling limits for the critical Fortuin-Kasteleyn model on a random planar map II: local estimates and empty reduced word exponent[END_REF]. The convergence is here in the so-called peanosphere topology, obtained from the mating of trees approach [START_REF] Duplantier | Liouville quantum gravity as a mating of trees[END_REF][START_REF] Miller | Liouville quantum gravity spheres as matings of finite-diameter trees[END_REF] (see also [START_REF] Gwynne | Brownian motion correlation in the peanosphere for κ > 8[END_REF]).

In the case of the O(n) model, the configuration of critical loops after the Riemann conformal mapping is expected to be described in the continuous limit by the conformal loop ensemble CLE κ [START_REF] Sheffield | Exploration trees and conformal loop ensembles[END_REF][START_REF] Sheffield | Conformal loop ensembles: the Markovian characterization and the loop-soup construction[END_REF]. It depends on the continuous index κ ∈ ( 8 3 , 8) of the associated Schramm-Loewner evolution (SLE κ ), with the correspondence n = 2 cos π 1 -4 κ for n ∈ (0, 2] [51, [START_REF] Duplantier | Conformal fractal geometry & boundary quantum gravity[END_REF][START_REF] Kager | A guide to stochastic Löwner evolution and its applications[END_REF][START_REF] Sheffield | Quantum gravity and inventory accumulation[END_REF]. In Liouville quantum gravity, the CLE κ is coupled to an independent GFF, which both govern the random measure with Liouville parameter γ = min √ κ, 4 √ κ , and the conformal welding of SLE κ curves according to the LQGboundary measure [START_REF] Duplantier | Liouville quantum gravity, KPZ and Schramm-Loewner evolution[END_REF][START_REF] Duplantier | Liouville quantum gravity as a mating of trees[END_REF][START_REF] Duplantier | Schramm-Loewner evolution and Liouville quantum gravity[END_REF][START_REF] Miller | Liouville quantum gravity spheres as matings of finite-diameter trees[END_REF][START_REF] Sheffield | Conformal weldings of random surfaces: SLE and the quantum gravity zipper[END_REF]; see also [START_REF] Astala | Random conformal weldings[END_REF]).

Yet, except for the pure gravity n = 0, γ 2 = 8 3 case, little is known on the metric properties of large random maps weighted by an O(n) model, even from a physical point of view. In this work, we shall rigorously investigate the nesting properties of loops in those maps. From the point of view of 2d quantum gravity, it is a necessary, albeit perhaps modest, step towards a more complete understanding of the geometry of these large random maps. For instance, one should first determine the typical 'depth' (i.e., the number of loops crossed) on a random map before trying to determine how deep geodesics are penetrating the nested loop configuration. While this last question seems at present to be out of reach, its answer is expected to be related to the value of the almost sure Hausdorff dimension of large random maps with an O(n) model, a question which is under active debate (see, e.g., Refs. [START_REF] Ambjørn | The toroidal Hausdorff dimension of 2d Euclidean quantum gravity[END_REF][START_REF] Ambjørn | Geodesic distances in Liouville quantum gravity[END_REF][START_REF] Ding | Upper bounds on Liouville first passage percolation and Watabiki's prediction[END_REF][START_REF] Duplantier | Geodesic duality and the Hausdorff dimension of two-dimensional quantum gravity[END_REF][START_REF] Gwynne | A mating-of-trees approach to graph distances in random planar maps[END_REF]).

An early study of the depth via a transfer matrix approach can be found in the work by Kostov [START_REF] Kostov | Strings with discrete target space[END_REF][START_REF] Kostov | Loop space hamiltonian for c = 1 open strings[END_REF]. Our approach is based on analytic combinatorics, and mainly relies on the substitution approach developed in [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF][START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF], and uses transfer matrices as an intermediate step. For instance, we compute generating series of cylinders (planar maps with two boundary faces) weighted by s P , where P is the number of loops separating the two boundaries. This novel type of results has a combinatorial interest per se; we find that the new s variable appears in a remarkably simple way in the generating series. While the present article is restricted to the case of planar maps, the tools that we present are applied in Ref. [START_REF] Borot | Nesting statistics in the O(n) loop model on random maps of arbitrary topologies[END_REF] to investigate the topology of nesting in maps of arbitrary genus, number of boundaries and marked points.

We also relate the asymptotics of our results in the critical scaling limit of large number of loops and large volume, to extreme nesting in CLE κ in a bounded planar domain in C, as obtained by Miller, Watson and Wilson in Ref. [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF], who built on earlier works [START_REF] Cardy | [END_REF][START_REF] Cardy | Exact results for the universal area distribution of clusters in percolation, Ising, and Potts models[END_REF][START_REF] Dubédat | For κ = 6[END_REF][START_REF] Kenyon | Conformal radii of loop models[END_REF][START_REF] Schramm | Conformal radii for conformal loop ensembles[END_REF]. The large deviations functions, obtained here for nesting on random planar maps, are rigorously shown to be identical to some transforms, in Liouville quantum gravity, of the Euclidean large deviations functions for CLE κ in the disk, as obtained in Ref. [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF], which we also generalise to the Riemann sphere. These transforms represent subtle extensions of the KPZ relation. By matching continuous sets of critical exponents, i.e., multifractal spectra, our results strongly support the conjecture that CLE observed in Liouville quantum gravity describes the scaling limit of the loop ensemble on large maps carrying a critical O(n) model.

Notations. If F and G are non zero and depend on some parameter ε → 0,

• F ≍ G means that ln F ∼ ln G;

• F . ≍ G means that F = e O(1) G; • F . ∼ G means there exists C > 0 independent of ε such that F ∼ CG.

If F is a formal series in some parameter u, [u m ] F is the coefficient of u m in F .

General definitions, reminders and main results

2.1. The O(n) loop model on random maps. We start by reminding the definition of the model, following the presentation of Refs. [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF][START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF].

Maps and loop configurations.

A map is a finite connected graph (possibly with loops and multiple edges) drawn on a closed orientable compact surface, in such a way that the edges do not cross and that the connected components of the complement of the graph (called faces) are simply connected. Maps differing by an orientation-preserving homeomorphism of their underlying surfaces are identified, so that there are countably many maps. The map is planar if the underlying surface is topologically a sphere. The degree of a vertex or a face is its number of incident edges (counted with multiplicity).

To each map we may associate its dual map which, roughly speaking, is obtained by exchanging the roles of vertices and faces. For m ≥ 1, a map with m boundaries is a map with m distinguished faces, labeled from 1 to m. By convention all the boundary faces are rooted, that is to say for each boundary face f we pick an oriented edge (called a root) having f on its right. The perimeter of a boundary is the degree of the corresponding face. Non boundary faces are called inner faces. A triangulation with m boundaries (resp. a quadrangulation with m boundaries) is a map with m boundaries such that each inner face has degree 3 (resp. 4).

Figure 1. A planar triangulation with a boundary of perimeter 8 (with root in red, the distinguished face being the outer face), endowed with a loop configuration (drawn in green).

Given a map, a loop is an undirected simple closed path on the dual map (i.e., it covers edges and vertices of the dual map, and hence visits faces and crosses edges of the original map). This is not to be confused with the graph-theoretical notion of loop (an edge incident twice to the same vertex), which plays no role here. A loop configuration is a collection of disjoint loops, and may be viewed alternatively as a collection of crossed edges such that every face of the map is incident to either 0 or 2 crossed edges. When considering maps with boundaries, we assume that the boundary faces are not visited by loops. Finally, a configuration of the O(n) loop model on random maps is a map endowed with a loop configuration, see Figure 1 for an example.

Remark 2.1. In the original formulation in Refs. [START_REF] Eynard | Exact solution of the O(n) model on a random lattice[END_REF][START_REF] Eynard | More on the exact solution of the O(n) model on a random lattice and an investigation of the case |n| > 2[END_REF][START_REF] Gaudin | O(n) on a fluctuating lattice. Some exact results[END_REF][START_REF] Kostov | O(n) vector model on a planar random lattice: spectrum of anomalous dimensions[END_REF][START_REF] Kostov | Multicritical phases of the O(n) model on a random lattice[END_REF], the loops cover vertices and edges the map itself. Our motivation for drawing them on the dual map is that it makes our combinatorial decompositions easier to visualise.

2.1.2. Statistical weights and partition functions. Colloquially speaking, the O(n) loop model is a statistical ensemble of configurations in which n plays the role of a fugacity per loop. In addition to this "nonlocal" parameter, we need also some "local" parameters, controlling in particular the size of the maps and of the loops. Precise instances of the model can be defined in various ways.

The simplest instance is the O(n) loop model on random triangulations [START_REF] Eynard | Exact solution of the O(n) model on a random lattice[END_REF][START_REF] Eynard | More on the exact solution of the O(n) model on a random lattice and an investigation of the case |n| > 2[END_REF][START_REF] Gaudin | O(n) on a fluctuating lattice. Some exact results[END_REF][START_REF] Kostov | O(n) vector model on a planar random lattice: spectrum of anomalous dimensions[END_REF][START_REF] Kostov | Multicritical phases of the O(n) model on a random lattice[END_REF]: here we require the underlying map to be a triangulation, possibly with boundaries. There are two local parameters g and h, which are the weights per inner face (triangle) which is, respectively, not visited and visited by a loop. The Boltzmann weight attached to a configuration C is thus w(C) = n L g T 1 h T 2 , with L the number of loops of C, T 1 its number of unvisited triangles and T 2 its number of visited triangles. A slight generalisation of this model is the bending energy model [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF], where we incorporate in the Boltzmann weight w(C) an extra factor α B , where B is the number of pairs of successive loop turns in the same direction, see Figure 2. Another variant is the O(n) loop model on random quadrangulations considered in [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF] (and its "rigid" specialisation). Finally, a fairly general model encompassing all the above, and amenable to a combinatorial decomposition, is described in [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF]Section 2.2]. We now define the partition function. Fixing an integer m ≥ 1, we consider the ensemble of allowed configurations where the underlying map is planar and has m boundaries of respective perimeters ℓ 1 , ℓ 2 , . . . , ℓ m ≥ 1 (called perimeters). We will mainly be interested in m = 1 (disks) and m = 2 (cylinders). The corresponding partition function is then the sum of the Boltzmann weights w(C) of all such configurations. We find convenient to add an auxiliary weight u per vertex, and define the partition function as (2.1)

F (m) ℓ 1 ,...,ℓm = δ m,1 δ ℓ 1 ,0 u + C u |V (C)| w(C),
where the sum runs over all desired configurations C, and |V (C)| denotes the number of vertices of the underlying map of C, also called volume. By convention, the partition function for m = 1 includes an extra term δ ℓ 1 ,0 u, which means that we consider the map consisting of a single vertex on a sphere to be a planar map with one boundary of perimeter zero. We also introduce the shorthand notation (2.2)

F ℓ ≡ F (1)
ℓ . 2.2. Phase diagram and critical points. When we choose the parameters to be real positive numbers such that the sum (2.1) converges, we say that the model is well defined (it induces a probability distribution over the set of configurations). Under mild assumptions on the model (e.g., the face degrees are bounded), this is the case for u small, and there exists a critical value u c above which the model ceases to be well defined: (2.3) u c = sup{u ≥ 0 : F (m) ℓ 1 ,...,ℓm < ∞}.

It is not difficult to check that u c does not depend on m and ℓ 1 , ℓ 2 , . . . , ℓ m ≥ 1. If u c = 1 (resp. u c > 1, u c < 1), we say that the model is at a critical (resp. subcritical, supercritical ) point. At a critical point, the partition function has a singularity at u = 1, and the nature (universality class) of this singularity is characterised by some critical exponents, to be discussed below. For n ∈ (0, 2), three different universality classes of critical points may be obtained in the O(n) loop model on random triangulations [START_REF] Kostov | O(n) vector model on a planar random lattice: spectrum of anomalous dimensions[END_REF], which we call generic, dilute and dense.

The generic universality class is that of "pure gravity", also obtained in models of maps without loops. The location of these points in the (g, h) plane forms the phase diagram of the model, displayed qualitatively on Figure 3, and established in [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF] -see also the earlier works [START_REF] Eynard | Exact solution of the O(n) model on a random lattice[END_REF][START_REF] Eynard | More on the exact solution of the O(n) model on a random lattice and an investigation of the case |n| > 2[END_REF][START_REF] Gaudin | O(n) on a fluctuating lattice. Some exact results[END_REF][START_REF] Kostov | O(n) vector model on a planar random lattice: spectrum of anomalous dimensions[END_REF][START_REF] Kostov | Multicritical phases of the O(n) model on a random lattice[END_REF]. For the bending energy model, the phase diagram is similar for α not too large, but as α grows the line of non generic critical points shrinks and vanishes eventually [START_REF] Borot | Loop models on random maps via nested loops: case of domain symmetry breaking and application to the Potts model[END_REF]Section 5.5]. The same universality classes, and a similar phase diagram, is also obtained for the rigid O(n) loop model on quadrangulations [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF], and is expected for more general loop models, where g and h should be thought as a fugacity per empty and visited faces, respectively. 2.3. Critical exponents. We now discuss some exponents that characterise the different universality classes of critical points of the O(n) loop model. Some of them are well known while others are introduced here for the purposes of the study of nesting (for completeness all definitions are given below). In the case of the dilute and dense universality classes, the known exponents are rational functions of the parameter:

(2.4) b = 1 π arccos n 2 ,
which decreases from 1 2 to 0 as n increases from 0 to 2. Let us mention that b is closely related to the so-called coupling constant g appearing in the Coulomb gas description of exponent subcrit. generic dilute dense n = 0 Perc. Ising 3-Potts KT b b b Before entering into definitions, we summarise the exponents on Table 1. An entry • indicates that the exponent is unknown. At the time of writing, there is no consensus about the value of the Hausdorff dimension d H in the physics literature, although a socalled Watabiki formula has been proposed (see e.g., [START_REF] Ambjørn | The toroidal Hausdorff dimension of 2d Euclidean quantum gravity[END_REF][START_REF] Ambjørn | Geodesic distances in Liouville quantum gravity[END_REF][START_REF] Bowick | The Hausdorff dimension of surfaces in two-dimensional gravity coupled to Ising minimal matter[END_REF][START_REF] Duplantier | Geodesic duality and the Hausdorff dimension of two-dimensional quantum gravity[END_REF] and references therein) and critically analysed in view of recent mathematical results [START_REF] Ding | Upper bounds on Liouville first passage percolation and Watabiki's prediction[END_REF][START_REF] Gwynne | A mating-of-trees approach to graph distances in random planar maps[END_REF]. All other exponents can be derived rigorously in the O(n) model on triangulations, as well as the model with bending energy, and are expected to be universal. We actually reprove these results in the course of the article -the only new statement concerns ν -for the dense and dilute phases of the model with bending energy. 2.3.1. Volume exponent. The singularity of the partition function in the vicinity of a critical point is captured in the so-called string susceptibility exponent γ str :

1 2 1 3 1 4 1 6 γ str -1 2 -b -b 1-b -1 -1 Table 1.
(2.5)

F ℓ | sing . ∼ (1 -u) 1-γstr , u → 1,
where ℓ is fixed, and F ℓ | sing denotes the leading singular part in the asymptotic expansion of F ℓ around u = 1. As u is coupled to the volume, the generating series of maps with fixed volume V behaves as:

(2.6) [u V ] F ℓ . ∼ V γstr-2 , V → ∞.
provided a delta-analyticity condition can be checked. In the context of the O(n) loop model, γ str may take the generic value -1 2 , already observed in models of maps without loops (n = 0) ; the dilute value -b ; and the dense value -b 1-b . In all cases we consider, γ str is comprised between -1 and 0. Let us recall the celebrated KPZ relation [START_REF] Knizhnik | Fractal structure of 2D-quantum gravity[END_REF] (2.7)

γ str = c -1 -(1 -c)(25 -c) 12 ,
linking the string susceptibility exponent to the central charge c of conformal field theory. For completeness, we also indicate in Table 1 the value of the κ parameter for the corresponding conformal loop ensemble (see Section 2.6).

The parameter c ∈ [1, 2) defined by:

(2.8) c := -γ str b

will play an important role in this paper (note that it has nothing to do with c).

Perimeter exponent.

Another exponent is obtained as we keep u = 1 fixed but take one boundary to be of large perimeter. Clearly, this requires F ℓ to be finite for all ℓ, hence the model to be either subcritical or critical, since γ str ∈ (-1, 0). We have the asymptotic behavior:

(2.9)

F ℓ . ∼ γ ℓ + ℓ a , ℓ → ∞,
where γ + is a non universal constant, and a is a universal exponent comprised between [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF] is the map formed by the vertices and edges which are exterior to all the loops, see Figure 4.

In Corollary 6.8, we will combine known properties of the generating series of disks in the model with bending energy to show that the probability that a vertex chosen at random uniformly in a disk of volume V and finite perimeter belongs to the gasket behaves as (2.10)

P • ∈ gasket V . ∼ V -ν , V → ∞ , with ν = c( 1 2 -b)
, modulo the check of a delta-analyticity condition. Relying on the work of Le Gall and Miermont [START_REF] Gall | Scaling limits of random planar maps with large faces[END_REF], we showed in [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF] that the almost sure fractal dimension of the gasket when V → ∞, denoted d gasket

H

, is equal to 3 -2b in the dense phase, 3 + 2b in the dilute phase. This exponent can also be extracted from Kostov [101, Section 4.2] -where g is the Coulomb gas coupling constant g mentioned above. This contrasts with the well known value d H = 4 for the fractal dimension of disks at the generic critical point. We can only expect d H > d gasket H . Ref. [START_REF] Duplantier | Geodesic duality and the Hausdorff dimension of two-dimensional quantum gravity[END_REF] relates it to the value of yet another critical exponent, which expresses how deep geodesics enter in the nested configuration of loops.

2.4.

Main results on random maps. This paper is concerned with the statistical properties of nesting between loops. The situation is simpler in the planar case since every loop is contractible, and divides the underlying surface into two components. The nesting structure of large maps of arbitrary topology is analysed in the subsequent work [START_REF] Borot | Nesting statistics in the O(n) loop model on random maps of arbitrary topologies[END_REF].

In the general O(n) loop model, the generating series of disks and cylinders have been characterised in [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF][START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF][START_REF] Borot | Abstract loop equations, topological recursion, and applications[END_REF], and explicitly computed in the model with bending energy in [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF], building on the previous works [START_REF] Borot | Enumeration of maps with self avoiding loops and the O(n) model on random lattices of all topologies[END_REF][START_REF] Eynard | Exact solution of the O(n) model on a random lattice[END_REF][START_REF] Eynard | More on the exact solution of the O(n) model on a random lattice and an investigation of the case |n| > 2[END_REF]. This characterisation is a linear functional relation which depends explicitly on n, accompanied by a nonlinear consistency relation depending implicitly on n. We remind the steps leading to this characterisation in Sections 3-4. In particular, we review in Section 3 the nested loop approach developed in [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF], which allows enumerating maps with loop configurations in terms of generating series of usual maps. We then derive in Section 4 the functional relations for maps with loops as direct consequences of the well known functional relations for generating series of usual maps. The key to our results is the derivation in Section 4.4 of an analogous characterisation for refined generating series of pointed disks (resp. cylinders), in which the loops which separate the origin (resp. the second boundary) and the (first) boundary face are counted with an extra weight s each. We find that the characterisation of the generating series is only modified by replacing n with ns in the linear functional relation, while keeping n in the consistency relation. Subsequently, in the model with bending energy, we can compute explicitly the refined generating series, in Section 5. We analyse in Section 6 the behavior of those generating series at a non generic critical point which pertains to the O(n) model. In the process, we rederive the phase diagram of the model with bending energy. More precisely, we perform an analysis of singularity in the canonical ensemble where the Boltzmann weight u coupled to the volume tends to its critical value, which is equal to 1 when suitably normalised. In order to convert it to large volume asymptotics, we establish in Appendices I.2 and J a property of delta-analyticity of the generating series with respect to u, which partially relies on the explicit solution (see Theorem 5.3) for the generating series of disks. One of our main result is then Theorem 6.10 in the text, restated below. Theorem 2.2. Fix (g, h, α) and n ∈ (0, 2) such that the model with bending energy achieves a non generic critical point for the vertex weight u = 1. In the ensemble of random pointed disks of volume V and perimeter L, the distribution of the number P of separating loops between the marked point and the boundary face behaves when V → ∞ as:

P P = c ln V π p V , L = ℓ . ≍ (ln V ) -1 2 V -c π J(p) , P P = c ln V 2π p V , L = ⌊V c 2 ℓ⌋ . ≍ (ln V ) -1 2 V -c 2π J(p) ,
where

J(p) = p ln 2 n p 1 + p 2 + arccot(p) -arccos n 2 .
In the above estimates, ℓ and p are bounded and bounded away from 0 as V → ∞.

We expect this result to be universal among all O(n) loop models at non generic critical points. The explicit, non universal finite prefactors in those asymptotics are given in the more precise Theorem 6.10. We establish a similar result in Section 7 and Theorem 7.1 for the number of loops separating the boundaries in cylinders. Note that our derivation of these theorems relies on the results of [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF], some of which were justified using numerical evidence rather than formal arguments. See Remark 5.4 below.

The large deviations function has the following properties (see Figure 5):

• J(p) ≥ 0 for positive p, and achieves its minimum value 0 at p opt = n √ 4-n 2 . • J(p) is strictly convex, and J ′′ (p) = 1 p(p 2 +1) . • J(p) has a slope ln(2/n) when p → ∞.

• When p → 0, we have J(p) = arcsin n 2 + p ln 2p n + O(p). In Section 6.3, we prove a central limit theorem for fluctuations P near its typical value. It is consistent with the Gaussian behavior of the large deviations function around its minimum p opt . Proposition 2.3. In pointed disks as above, the number of separating loops between the marked point and the boundary face behaves almost surely like cpopt jπ ln V , with Gaussian fluctuations of order O( √ ln V ):

P -cpopt jπ ln V √ ln V -→ N (0, σ 2 ), p opt = n √ 4 -n 2 , σ 2 = 2 3-j nc π(4 -n 2 ) 3 2 . with j = 1 if we keep L finite, or j = 2 if we scale L = ⌊ℓ V c 2 ⌋ for a finite positive ℓ.
Establishing the critical behavior of the generating series and the phase diagram requires analyzing special functions related to the Jacobi theta functions and elliptic functions in the trigonometric limit. The aformentioned variable q is the elliptic nome. The lengthy computations with these special functions are postponed to Appendices to ease the reading. In Section 8, we generalise these results to a model where loops are weighted by independent, identically distributed random variables. Lastly, Section 9, the content of which is briefly described below, uses a different perspective, and re-derives the above results on random maps from the Liouville quantum gravity approach. The latter is applied to similar earlier results obtained in Ref. [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF] for a CLE κ in the unit disk.

2.5.

Relation with other works. We now mention some closely related works, which appeared after the initial version of this paper was posted on the arXiv.

Chen, Curien and Maillard [START_REF] Chen | The perimeter cascade in critical Boltzmann quadrangulations decorated by an O(n) loop model[END_REF] proposed an alternative study of the nesting, and proved the convergence of the nesting tree (see Section 3.2) labeled by loop perimeters in rigid O(n) loop model on random quadrangulations, to an explicit multiplicative cascade. This rigid O(n) model is a variant of the one studied in the present article, for which an analogous explicit analysis can be carried out -the seeds of the computation are in [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF] -and lead to the same Theorem 2.2 and Proposition 2.3. Ref [START_REF] Chen | The perimeter cascade in critical Boltzmann quadrangulations decorated by an O(n) loop model[END_REF] has proposed a heuristic argument confirming the result of Theorem 2.2 from the properties of the offspring distribution of the cascade.

A detailed study of the rigid O(n) loop model on random bipartite maps was performed by Budd (with some input by Chen) in a series of works. Budd's first observation [START_REF] Budd | On a connection between planar map combinatorics and random walks. Talk at the workshop[END_REF] was an unexpected connection between planar maps and lattice walks on the slit plane. An extension of his construction relates walks on Z 2 with a controlled winding angle around the origin to the rigid O(n) loop model. This led to new results [START_REF] Budd | Winding of simple walks on the square lattice[END_REF] on the counting of simple diagonal walks on Z 2 with a prescribed winding angle, hinging on the explicit diagonalisation of certain transfer matrices acting on a ℓ 2 -space which are closely related to the transfer matrices considered in the present article. Finally, the paper [START_REF] Budd | The peeling process on random planar maps coupled to an O(n) loop model (with an appendix by L. Chen[END_REF] extends to loop-decorated maps the peeling process of (undecorated) Boltzmann maps introduced in [START_REF] Budd | The peeling process of infinite Boltzmann planar maps[END_REF]. This approach brings many results:

• a formal justification of the phase diagram of the rigid model, see also [START_REF] Chen | Random Planar Maps coupled to Spin Systems[END_REF]ter II] and Remark 5.4 below, • a characterisation of the scaling limit of the perimeter process, which implies in turn the convergence of a certain rescaled first passage percolation distance, • exact and asymptotic results on the number of separating loops in a pointed rooted map, which are consistent with our own results (see Appendix I), and also include the case n = 2.

2.6.

Comparison with CLE properties. It is strongly believed that, if the random disks were embedded conformally to the unit disk D, the loop configuration would be described in the thermodynamic V → ∞ limit by the conformal loop ensemble in presence of Liouville quantum gravity. On a regular planar lattice, the critical O(n)-model is expected to converge in the continuum limit to the universality class of the SLE κ /CLE κ , for [START_REF] Barral | Gaussian multiplicative chaos and KPZ duality[END_REF], dense phase and the same is expected to hold at a non generic critical point in the dilute or dense phase on a random planar map. Although both conjectures are not yet mathematically fully established, we may try to relate the large deviations properties of nesting, as derived in the critical regime in the O(n) loop model on a random planar map, to the corresponding nesting properties of CLE κ , in order to support both conjectures altogether.

(2.11) n = 2 cos π 1 -4 κ n ∈ (0, 2] κ ∈ ( 8 3 , 4], dilute phase κ ∈ [4,
Using the so-called Coulomb gas method for critical O(n) and Potts models, Cardy and Ziff provided the first prediction, numerically verified, for the expected number of loops surrounding a given point in a finite domain [START_REF] Cardy | Exact results for the universal area distribution of clusters in percolation, Ising, and Potts models[END_REF]. Elaborating on this work and on Refs. [START_REF] Cardy | [END_REF][START_REF] Dubédat | For κ = 6[END_REF][START_REF] Kenyon | Conformal radii of loop models[END_REF][START_REF] Schramm | Conformal radii for conformal loop ensembles[END_REF], Miller, Watson and Wilson [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF] (see also [START_REF] Miller | The conformal loop ensemble nesting field[END_REF]) were able to derive the almost sure multifractal dimension spectrum of extreme nesting in the conformal loop ensemble. Let Γ be a CLE κ in D. For each point z ∈ D, let N z (ε) be the number of loops of Γ which surround the ball B(z, ε) centered at z and of radius ε > 0. For ν > 0, define

Φ ν = Φ ν (Γ) := z ∈ D : lim ε→0 N z (ε) ln(1/ε) = ν .
The almost-sure Hausdorff dimension of this set is given in terms of the distribution of conformal radii of outermost loops in CLE κ . More precisely, let U be the connected component containing the origin in the complement D \ L of the largest loop L of Γ surrounding the origin in D, and CR(0, U) its conformal radius from 0. The cumulant generating function of T :=ln(CR(0, U)) was computed independently in unpublished works [START_REF] Cardy | [END_REF][START_REF] Dubédat | For κ = 6[END_REF][START_REF] Kenyon | Conformal radii of loop models[END_REF], and rigorously confirmed in Ref. [START_REF] Schramm | Conformal radii for conformal loop ensembles[END_REF]. It is given by

(2.12) Λ κ (λ) := ln E e λT = ln     -cos( 4π κ ) cos π 1 -4 κ 2 + 8λ κ     , for λ ∈ (-∞, 1 -2 κ -3κ 32 ). The symmetric Legendre-Fenchel transform, Λ * κ : R → R + of Λ κ is defined by (2.13) Λ ⋆ κ (x) := sup λ∈R (λx -Λ κ (λ)) .
The authors of [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF] then define

(2.14) γ κ (ν) := νΛ ⋆ κ (1/ν), if ν > 0 1 -2 κ -3κ 32 if ν = 0,
which is right-continuous at 0. Then, for κ ∈ ( 8 3 , 8), the Hausdorff dimension of the set

Φ ν is almost surely [120, Theorem 1.1], dim H Φ ν = max(0, 2 -γ κ (ν)).
As a Lemma for this result, the authors of Ref. [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF] estimate, for ε → 0, the asymptotic nesting probability around point z,

(2.15) P(N z (ε) ≈ ν ln(1/ε) | ε) ≍ ε γκ(ν) ,
where the sign ≈ stands for a growth of the form (ν +o(1)) ln(1/ε), and where ≍ means an asymptotic equivalence of logarithms. In Section 9, we consider the unit disk in Liouville quantum gravity (LQG), i.e., we equip it with a random measure, formally written here as µ γ = e γh d 2 z, where γ ∈ [0, 2] and h is an instance of a GFF on D, d 2 z being the Lebesgue measure. The random measure µ γ is called the Liouville quantum gravity measure. We define accordingly δ := B(z,ε) µ γ as the (random) quantum area of the ball B(z, ε). In this setting, the KPZ formula, which relates a Euclidean conformal weight x to its LQG counterpart ∆ [START_REF] Duplantier | Liouville quantum gravity and KPZ[END_REF], reads

(2.16) x = U γ (∆) := γ 2 4 ∆ 2 + 1 - γ 2 4 ∆.
Studying extreme nesting in LQG then consists in looking for the distribution of loops of a CLE κ around the same ball B(z, ε), the latter being now conditioned to have a given quantum measure δ, and to measure this nesting in terms of the logarithmic variable ln(1/δ), instead of ln(1/ε). We thus look for the probability, (2.17)

P Q (N z ≈ p ln(1/δ) | δ) , p ∈ R + ,
which is the analogue of the left-hand side of (2.15) in Liouville quantum gravity, and which we may call the quantum nesting probability. By taking into account the distribution of the Euclidean radius ε for a given δ [START_REF] Duplantier | Duality and KPZ in Liouville quantum gravity[END_REF][START_REF] Duplantier | Liouville quantum gravity and KPZ[END_REF], we obtain two main results, a first general one deriving via the KPZ relation the large deviations in nesting of a CLE κ in LQG from those in the Euclidean disk D, as derived in Ref. [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF], and a second one identifying these Liouville quantum gravity results to those obtained here for the critical O(n) model on a random map.

Theorem 2.4. In Liouville quantum gravity, the cumulant generating function Λ κ (2.12) with κ ∈ ( 8 3 , 8), is transformed into the quantum one, (2.18)

Λ Q κ := Λ κ • 2U γ ,
where Λ κ is given by (2.12) and U γ is the KPZ function (2.16), with γ = min

√ κ, 4 √ κ . The Legendre-Fenchel transform, Λ Q⋆ κ : R → R + of Λ Q κ is defined by Λ Q⋆ κ (x) := sup λ∈R λx -Λ Q κ (λ) .
The quantum nesting distribution (2.17) in the disk is then, when δ → 0,

P Q N z ≈ p ln(1/δ) | δ ≍ δ Θ(p) , Θ(p) =      pΛ Q⋆ κ 1 p , if p > 0 3 4 -2 κ if p = 0 and κ ∈ ( 8 3 , 4]
Λ Q κ (λ) = Λ κ • 2U γ (λ) = ln   cos π(1 -4 κ ) cos π 2λ c + 1 -4 κ   , c = max{1, κ 4 }, λ ∈ 1 2 -2 κ , 3 4 -2 κ for κ ∈ 8 3 , 4 ; λ ∈ 1 2 -κ 8 , 1 2 -κ 16 for κ ∈ [4, 8).
Remark 2.6. Θ(p) is right-continuous at p = 0.

Remark 2.7. Theorem 2.4 shows that the KPZ relation can directly act on an arbitrary continuum variable, here the conjugate variable in the cumulant generating function (2.12) for the CLE κ log-conformal radius. This seems the first occurrence of such a role for the KPZ relation, which usually concerns scaling dimensions.

Remark 2.8. As the derivation in Section 9 will show, the map Λ κ → Λ Q κ in (2.18) to go from Euclidean geometry to Liouville quantum gravity is fairly general: the composition of Λ by the KPZ function U γ would hold for any large deviations problem, the large deviations function being the Legendre-Fenchel transform of a certain generating function Λ.

Theorem 2.9. The quantum nesting probability of a CLE κ in a proper simply connected domain D ⊊ C, for the number N z of loops surrounding a ball centered at z and conditioned to have a given Liouville quantum area δ, has the large deviations form,

P Q N z ≈ cp 2π ln(1/δ) δ ≍ δ c 2π J(p) , δ → 0,
where c and J are the same as in Theorem 2.2.

A complementary result concerns the case of the Riemann sphere. The extreme nestings of CLE for this geometry is written in Theorem 9.8 and seems to be new. After coupling to LQG, we obtain Theorem 2.10. On the Riemann sphere C, the large deviations function Θ which governs the quantum nesting probability,

P C Q N ≈ p ln(1/δ) | δ ≍ δ Θ(p) , δ → 0,
is related to the similar function Θ for the disk topology, as obtained in Theorem 2.4, by

Θ(2p) = 2Θ(p).
From Theorem 2.9, we get explicitly,

P C Q N ≈ cp π ln(1/δ) δ ≍ δ c π J(p) , δ → 0,
where c and J are as in Theorem (2.2).

Remark 2.11. The reader will have noticed the perfect matching of the LQG results for CLE κ in Theorems 2.4, 2.9 and 2.10 with the main Theorem 2.2 for the O(n) model on a random planar map, with the proviso that the first ones are local versions (i.e., in the δ → 0 limit), while the latter one gives a global version (i.e., in the V → ∞ limit).

3. First combinatorial results on planar maps 3.1. Reminder on the nested loop approach. We remind that F ℓ is the partition function for a loop model on a planar map with a boundary of perimeter ℓ. The nested loop approach describes it in terms of the generating series F p = F p (g 1 , g 2 , . . .) of usual maps (i.e., without a loop configuration) which are planar, have a rooted boundary of perimeter p, and counted with a Boltzmann weight g k per inner face of degree k (k ≥ 1) and an auxiliary weight u per vertex. To alleviate notations, the dependence on u is left implicit in most expressions. By convention, we assume that boundaries are rooted. We then have the fundamental relation [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF] (3.1)

F ℓ = F ℓ (G 1 , G 2 , . . .),
where the G k 's satisfy the fixed point condition

(3.2) G k = g k + ℓ ′ ≥0 A k,ℓ ′ F ℓ ′ (G 1 , G 2 , . . .) = g k + ℓ ′ ≥0 A k,ℓ ′ F ℓ ′ ,
where A k,ℓ is the generating series of sequences of faces visited by a loop, which are glued together so as to form an annulus, in which the outer boundary is rooted and has perimeter k, and the inner boundary is unrooted and has perimeter ℓ. Compared to the notations of [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF], we decide to include in A k,ℓ the weight n for the loop crossing all faces of the annulus. We call G k the renormalised face weights.

Throughout the text, unless it is specified in the paragraph headline that we are working with usual maps, the occurrence of F will always refer to F(G 1 , G 2 , . . .).

3.2.

The nesting graphs. In this paragraph, we introduce a notion of nesting graph attached to a configuration C of the O(n) model. Although this level of generality is not necessary for this article (see the discussion at the end of this paragraph), we include it to put our study in a broader context.

Let us cut the underlying surface along every loop, which splits it into several connected components c 1 , . . . , c N . Let T be the graph on the vertex set {c 1 , . . . , c N } where there is an edge between c i and c j if and only if they have a common boundary, i.e., they touch each other along a loop (thus the edges of T correspond to the loops of C).

If the map is planar, T is a tree called the nesting tree of C, see Figure 6. Each loop crosses a sequence of faces which form an annulus. This annulus has an outer and inner boundary, and we can record their perimeter on the half edges of T . As a result, T is a rooted tree whose half edges carry non negative integers. If the map has a boundary face, we can root T on the vertex corresponding to the connected component containing the boundary face. Then, for any vertex v ∈ T , there is a notion of parent vertex (the one incident to v and closer to the root) and children vertices (all other incident vertices). We denote ℓ(v) the perimeter attached to the half-edge arriving to v from the parent vertex. In this way, we can convert T to a tree T ′ where each vertex v carries the non negative integer ℓ(v).

The nesting tree is closely related to the gasket decomposition introduced in [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF][START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF]. Consider the canonical ensemble of disks in the O(n) model such that vertices receive a Boltzmann weight u, and the probability law it induces on the tree T '. The probability that a vertex v with perimeter ℓ has m children with perimeters {ℓ 1 , . . . , ℓ m } is:

P ℓ→ℓ 1 ,...,ℓm = 1 m! k 1 ,...,km≥0 m i=1 A k i ,ℓ i F ℓ i ∂ g k 1 • • • ∂ g km F ℓ (g 1 , g 2 , . . .) F ℓ .
We see that T ′ forms a Galton-Watson tree with infinitely many types. For the rigid O(n) model on planar quadrangulation of a disk [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF], the situation is a bit simpler as the inner and outer perimeters of the annuli carrying the loops coincide. We therefore obtain a random tree with one integer label for each vertex, whose convergence at criticality was studied in [START_REF] Chen | The perimeter cascade in critical Boltzmann quadrangulations decorated by an O(n) loop model[END_REF] (see Section 2.5).

If one decides to consider a map M with a given finite set of marked elements -e.g., boundary faces or marked points -, one can define the reduced nesting tree (T red , p) by: (i) For each mark in M , belonging to a connected component c i , putting a mark on the corresponding vertex of T ; (ii) erasing all vertices in T which correspond to connected components which, in the complement of all loops and of the marked elements in M , are homeomorphic to disks ; this step should be iterated until all such vertices have disappeared ; (iii) replacing any maximal simple path of the form v 0v 1 -• • •v p with p ≥ 2 where (v i ) p i=1 represent connected components homeomorphic to cylinders, by a single edge v 0 p v p carrying a length p. By convention, edges which are not obtained in this way carry a length p = 1. The outcome is a tree, in which vertices may carry the marks that belonged to the corresponding connected components, and whose edges carry positive integers p. By construction, given a finite set of marked elements, one can only obtain finitely many inequivalent T red .

In the subsequent article [START_REF] Borot | Nesting statistics in the O(n) loop model on random maps of arbitrary topologies[END_REF], the first-named author and Garcia-Failde analyse the probability that a given topology of nesting tree is realised, conditioned on the lengths of the arms, as well as the generalisation to non simply connected maps. In the present article, we focus on the case of two marks: either a marked point and a boundary face, or two boundary faces. Then, the reduced nesting graph is either the graph with a single vertex (containing the two marked elements) and no edge, or the graph with two vertices (each of them containing a marked element) connected by an arm of length P ≥ 0. Our goal consists in determining the distribution of P , which is the number of loops separating the two marked elements in the map (the pruning consisted in forgetting all information about the loops which were not separating). Yet, the tools we shall develop are important steps in the more general analysis of [START_REF] Borot | Nesting statistics in the O(n) loop model on random maps of arbitrary topologies[END_REF].

Maps with two boundaries. We denote F

(2) ℓ 1 ,ℓ 2 the partition function for a loop model on a random planar map with 2 labeled boundaries of respective perimeters ℓ 1 , ℓ 2 , and similarly F

(2)

ℓ 1 ,ℓ 2 ≡ F (2)
ℓ 1 ,ℓ 2 (g 1 , g 2 , . . .) for the partition function of usual maps. Such maps can be obtained from disks by marking an extra face and rooting it at an edge. At the level of partition functions, this amounts to:

(3.3) F (2) ℓ 1 ,ℓ 2 = ℓ 2 ∂ ∂g ℓ 2 F ℓ 1 , F (2)
ℓ 1 ,ℓ 2 = ℓ 2 ∂ ∂g ℓ 2 F ℓ 1 .
Differentiating the fixed point relation (3.1), we can relate F

ℓ 1 ,ℓ 2 to partition functions of usual maps:

(3.4) F (2) ℓ 1 ,ℓ 2 = F (2) ℓ 1 ,ℓ 2 + k≥1 ℓ≥0 F (2) ℓ 1 ,k R k,ℓ F (2) ℓ,ℓ 2 ,
where we have introduced the generating series R k,ℓ = A k,ℓ /k, which now enumerate annuli whose outer and inner boundaries are both unrooted. In this equation, the evaluation of the generating series of usual maps at G k given by (3.2) is implicit.

3.4. Separating loops and transfer matrix. We say that a loop in a map M with 2 boundaries is separating if after its removal, each connected component contains one boundary. The combinatorial interpretation of (3.4) is transparent : the first term counts cylinders where no loop separates the two boundaries, while the second term counts cylinders with at least one separating loop (see Figure 7). With this remark, we can address a refined enumeration problem. We denote by F

ℓ 1 ,ℓ 2 [s] the partition function of cylinders carrying a loop model, with an extra weight s per loop separating the two boundaries. Obviously, the configurations without separating loops

• • • F (2) F (2) s sR F (2) F (2) F (2)
sR sR sR are enumerated by F

(2)

ℓ 1 ,ℓ 2 .
If a configuration has at least one separating loop, let us cut along the first separating loop, and remove it. It decomposes the cylinder into : a cylinder without separating loops, that is adjacent to the first boundary ; the annulus that carried the first separating loop ; a cylinder with one separating loop less, which is adjacent to the second boundary. We therefore obtain the identity :

(3.5) F (2)
ℓ 1 ,ℓ 2 [s] = F (2)
ℓ 1 ,ℓ 2 + s k≥1 ℓ≥0 F (2)
ℓ 1 ,k R k,ℓ F (2)
ℓ,ℓ 2 [s].

We retrieve (3.4) when s = 1, i.e., when separating and non separating loops have the same weight. We remind for the last time that F's should be evaluated at the renormalised face weights G k . Although it is not essential and will rarely be used in the body of this article, we point out that these relations can be rewritten concisely with matrix notations. Let F (2) s (resp. R) be the semi-infinite matrices with entries F

(2)

ℓ 1 ,ℓ 2 [s] (resp. R ℓ 1 ,ℓ 2 )
with row and column indices ℓ 1 , ℓ 2 ≥ 0, with the convention that R 0,ℓ 2 = 0. It allows the repackaging of (3.5) as:

(3.6) F (2) s = F (2) + s F (2) RF (2)
s . Therefore: 2) .

(3.7) F (2) s = 1 1 -s F (2) R F (
Then, Γ s = (1 -s F (2) R) -
Z • = u ∂ ∂u Z.
We refer to the marked point as the origin of the map. Let us apply this identity to disks with loops. We have to differentiate (3.1) and remember that the renormalised face weights depend implicitly on u:

(3.9)

F • ℓ = F • ℓ + k≥1 ℓ ′ ≥1 F (2) ℓ,k R k,ℓ ′ F • ℓ ′ .
Obviously, the first term enumerates disks where the boundary and the origin are not separated by a loop. Let us introduce a refined partition function F • ℓ [s] that includes a Boltzmann weight s per separating loop between the origin and the boundary. Cutting along the first (if any) separating loop starting from the boundary and repeating the argument of § 3.4, we find:

(3.10) F • ℓ [s] = F • ℓ + s k≥1 ℓ ′ ≥0 F (2) ℓ,k R k,ℓ ′ F • ℓ ′ [s].
If we introduce the semi-infinite line vectors

F • s (resp. F • s ) whose entries are F • ℓ [s] (resp. F • ℓ [s]
) for ℓ ≥ 0, (3.10) can be written in matrix form:

(3.11) F • s = F • + s F (2) RF • s .
The solution reads:

(3.12)

F • s = 1 1 -s F (2) R F • = Γ s F • ,
involving again the transfer matrix.

Functional relations

4.1. More notations: boundary perimeters. It is customary to introduce generating series for the perimeter of a boundary. Here, we will abandon the matrix notations of § 3.4 unless explicitly mentioned, and rather introduce:

(4.1) F(x) = ℓ≥0 F ℓ x ℓ+1 , F (x) = ℓ≥0 F ℓ x ℓ+1 ,
which enumerate disks with loops (resp. usual disks) with a weight x -(ℓ+1) associated to a boundary of perimeter ℓ, and similarly the generating series of pointed disks (4.2)

F • (x) = ℓ≥0 F • ℓ x ℓ+1 , F • (x) = ℓ≥0 F • ℓ x ℓ+1
and the generating series of pointed disks in which a weight s P is included when the boundary and the marked point are separated by P loops:

(4.3) F • s (x) = ℓ≥0 F • ℓ [s] x ℓ+1
Likewise, for the generating series of cylinders, we introduce:

F (2) (x 1 , x 2 ) = ℓ 1 ,ℓ 2 ≥1 F (2) ℓ 1 ,ℓ 2 x ℓ 1 +1 1 x ℓ 2 +1 2 , F (2) s (x 1 , x 2 ) = ℓ 1 ,ℓ 2 ≥1 F (2) ℓ 1 ,ℓ 2 [s] x ℓ 1 +1 1 x ℓ 2 +1 2 , F (2) (x 1 , x 2 ) = ℓ 1 ,ℓ 2 ≥1 F (2) ℓ 1 ,ℓ 2 x ℓ 1 +1 1 x ℓ 2 +1 2 , (4.4)
etc. We will also find convenient to introduce generating series of annuli1 :

R(x, z) = k+ℓ≥1 R k,ℓ x k z ℓ , A(x, z) = k≥1 ℓ≥0 A k,ℓ x k-1 z ℓ = ∂ x R(x, z). (4.5) 4.2.
Reminder on usual maps. The properties of the generating series of usual disks F (x) have been extensively studied. We now review the results of [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF]. We say that a sequence of nonnegative weights (u, g 1 , g 2 , . . .) is admissible if for any ℓ ≥ 0, we have F • ℓ < ∞ ; by extension, we say that a sequence of real-valued weights (u, g 1 , g 2 , . . .) k≥1 is admissible if (|u|, |g 1 |, |g 2 |, . . .) is admissible. Then, F (x) satisfies the one-cut lemma and a functional relation coming from Tutte's combinatorial decomposition of rooted maps: Proposition 4.1. If (u, g 1 , g 2 , . . .) is admissible, then the formal series F (x) is the Laurent series expansion at x = ∞ of a holomorphic function in a maximal domain of the form C \ γ, where γ = [γ -, γ + ] is a segment of the real line depending on the vertex and the face weights. Its endpoints are given by γ ± = s ± 2 √ r where r and s are the unique formal series in the variables u and (g k ) k≥1 such that:

C(γ) dx 2iπ x -k≥1 g k x k-1 σ(x) = 0, -2u + C(γ) dx 2iπ x x -k≥1 g k x k-1 σ(x) = 0. (4.6)
where σ(x) = √ x 2 -2sx + s 2 -4r and C(γ) is a contour surrounding (and close enough to) γ in the positive direction. Besides, the endpoints satisfy |γ -| ≤ γ + , with equality iff g k = 0 for all odd k's.

Remark 4.2. The relations (4.6) are equivalent to [18, Equation 6.22] after simple algebraic manipulations. In fact, r and s may be interpreted combinatorially as certain series of pointed rooted maps, see e.g. [START_REF] Bouttier | Planar maps and continued fractions[END_REF]. In particular, we have (4.7)

F • 1 = u s, F • 2 = u (s 2 + 2r).
From now on, we shall use the same notation for the formal series and the holomorphic function.

Proposition 4.3. F (x) behaves like u x + O( 1 x 2 ) when x → ∞, like O √ x -γ ± when x → γ ± ,
and its boundary values on the cut satisfy the functional relation:

(4.8) ∀x ∈ γ, F (x + i0) + F (x -i0) = x - k≥1 g k x k-1
where γ := (γ -, γ + ). If γ -and γ + are given, there is a unique holomorphic function F (x) on C \ γ satisfying these properties.

Although (4.8) arises as a consequence of Tutte's equation and analytical continuation, it has not received a direct combinatorial interpretation yet.

With Proposition 4.1 in hand, the analysis of Tutte's equation for generating series of maps with several boundaries, and their analytical continuation, has been performed in a more general setting in [START_REF] Borot | Formal multidimensional integrals, stuffed maps, and topological recursion[END_REF][START_REF] Borot | Abstract loop equations, topological recursion, and applications[END_REF]. The outcome for usual cylinders (see also [START_REF] Borot | Abstract loop equations, topological recursion, and applications[END_REF][START_REF] Eynard | Counting surfaces[END_REF]) is the following: Proposition 4.4. If (g k ) k≥1 is admissible, the formal series F (2) (x, y) is the Laurent series expansion of a holomorphic function in (C \ γ) 2 when x, y → ∞, where γ is as in Proposition 4.1. We have the functional relation, for x ∈ γ and y ∈ C \ γ:

F (2) (x + i0, y) + F (2) (x -i0, y) = - 1 (x -y) 2 .
It is subjected to the growth condition

F (2) (x, y) ∈ O((x -γ ± ) - 1
2 ) when x → γ + for fixed y ∈ C \ γ, and a similar condition when x and y are exchanged.

4.3.

Reminder on maps with loops. The relation (3.1) between disks with loops and usual disks allows carrying those results to the loop model. We say that a sequence of face weights (g k ) k≥1 and annuli weights (A k,l ) k,l≥0 is admissible if the sequence of renormalised face weights (G k ) k≥1 given by (3.2) is admissible as it is meant for usual maps. We say it is subcritical if the annuli generating series A(x, z) is holomorphic in a neighborhood of γ ×γ, where γ is the segment determined by (4.6) for the renormalised face weights. Being strictly admissible is equivalent to being admissible and not in the non generic critical phase in the terminology of [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF]. In the remaining of Section 4 and 5, we always assume strict admissibility.

In particular, F(x) satisfies the one-cut property (Proposition 4.1) on this segment γ, which now depends on face weights (g k ) k and annuli weights (A k,l ) k,l . And, its boundary values on the cut satisfy the functional relation: Proposition 4.5. For any x ∈ γ, (4.9)

F(x + i0) + F(x -i0) + C(γ) dz 2iπ A(x, z) F(z) = x - k≥1 g k x k-1 .
With Proposition 4.1 in hand, the analysis of Tutte's equation for the partition functions of maps having several boundaries in the loop model, and their analytical continuation, has been performed in [START_REF] Borot | Formal multidimensional integrals, stuffed maps, and topological recursion[END_REF][START_REF] Borot | Abstract loop equations, topological recursion, and applications[END_REF]. In particular, one can derive a functional relation for F (2) (x 1 , x 2 ), which matches the one formally obtained by marking a face in Proposition 4.5 while considering the contour C(γ) independent of the face weights.

Proposition 4.6. The formal series F (2) (x, y) is the Laurent series expansion of a holomorphic function in (C \ γ) 2 when x, y → ∞, with γ as in Proposition 4.5. Besides, it satisfies the functional relation, for x ∈ γ and y ∈ C \ γ:

(4.10) F (2) (x + i0, y) + F (2) (x -i0, y) + C(γ) dz 2iπ A(x, z) F (2) (z, y) = - 1 (x -y) 2 .
It is subjected to the growth condition

F (2) (x, y) ∈ O (x -γ ± ) -1 2
when x → γ ± and y ∈ C \ γ, and a similar condition when x and y are exchanged.

By similar arguments for the differentiation of (4.9) with respect to the vertex weight u, one can derive for the generating series of pointed rooted disks a linear functional equation. This equation is in fact homogeneous because the right-hand side in (4.9) does not depend on u, which leads to Proposition 4.7. For any x ∈ γ, (4.11)

F • (x + i0) + F • (x -i0) + C(γ) dz 2iπ A(x, z) F • (z) = 0.
It is subjected to the growth conditions s (x, y) is the Laurent expansion of a holomorphic function in (C \ γ) 2 when x, y → ∞, and γ is the segment already appearing in Proposition 4.5 and is independent of s. For any x ∈ γ and y ∈ C \ γ, we have:

F • (x) = u x + O( 1 x 2 ) when x → ∞ and F • (x) ∈ O (x -γ ± ) -1 2 when x → γ ± .
(4.12) F (2) s (x + i0, y) + F (2) s (x -i0, y) + s C(γ) dz 2iπ A(x, z) F (2) s (z, y) = - 1 (x -y) 2 .
It is subjected to the growth condition

F (2) s (x, y) ∈ O((x -γ ± ) -1
2 ) when x → γ + for fixed y ∈ C \ γ, and a similar one when x and y are exchanged. Proposition 4.9. At least for |s| < 1 and for s = 1, the formal series

F • s (x) is the Laurent expansion of a holomorphic function in (C \ γ). It has the growth properties F • s (x) = u x + O( 1 x 2 ) when x → ∞, and F • s (x) ∈ O (x -γ ± ) -1 2 when x → γ ± .
Besides, for any x ∈ γ, we have:

(4.13) F • s (x + i0) + F • s (x -i0) + s C(γ) dz 2iπ A(x, z) F • s (z) = 0.
Proof. Let us denote F

[P ] , the generating series of cylinders with exactly P separating loops (discarding the power of s), and F

[-1] ≡ 0 by convention. In particular (4.14)

F (2) s = P ≥0 F (2)
[P ] s P

We first claim that for any P ≥ 0, F

[P ] (x, y) defines a holomorphic function in (C \ γ) 2 , and satisfies the functional relation: for any x ∈ γ and y ∈ C \ γ,

F (2) [P ] (x + i0, y) + F (2) [P ] (x -i0, y) = - δ P,0 (x -y) 2 + C(γ) dz 1 2iπ F (2) (x, z 1 ) C(γ) dz 2 2iπ A(z 1 , z 2 ) F (2)
[P -1] (z 2 , y)

(4.15)
The assumption of strict admissibility guarantees that A(ξ, η) -and thus its ξ-antiderivative R(ξ, η) -is holomorphic in a neighborhood of γ × γ, ensuring that the contour integrals in (4.15) are well defined. Let us momentarily accept the claim.

Since

F (2) (x, y) = F (2)
s=1 (x, y), by dominated convergence we deduce that F

s (x, y) is an analytic function of s -uniformly for x, y ∈ C \ γ -with radius of convergence at least 1. Then, we can sum over P ≥ 0 the functional relation (4.15) multiplied by s P : the result is the announced (4.12), valid in the whole domain of analyticity of F

2) s (x, y)| ≤ F (2),|| (|x|, |y|), we deduce that F (2)
s (x, y) also satisfies the growth condition. The claim is established by induction on P . Since F

[0] = F (2) , the claim follows by application of Proposition 4.4 for usual cylinders with renormalised face weights, i.e., vanishing annuli weights in the functional relation (4.10). We however emphasise that the cut γ is determined by Proposition 4.5, thus depends on annuli weights via the renormalised face weights.

Assume the statement holds for some P ≥ 0. We know from the combinatorial relation (3.6) that: (4. [START_REF] Borot | Formal multidimensional integrals, stuffed maps, and topological recursion[END_REF]) F

(2)

[P +1] = F (2) RF (2) [P ]
with the matrix notations of § 3.4. The analytic properties of F (2) and of F

[P ] -as known from the induction hypothesis -allows the rewriting: (4.17) F

(2)

[P +1] (x, y) = C(γ) dz 1 2iπ F (2) (x, z 1 ) C(γ) dz 2 2iπ R(z 1 , z 2 ) F (2)
[P ] (z 2 , y).

The expression on the right-hand side emphasises that the left-hand side, though initially defined as a formal Laurent series in x and y, can actually be analytically continued to (C \ γ) 2 . Besides, for x ∈ γ and y ∈ C \ γ, we can compute the combination:

F (2) [P +1] (x + i0, y) + F (2) [P +1] (x -i0, y) = C(γ) dz 1 2iπ F (2) (x + i0, z 1 ) + F (2) (x -i0, z 1 ) C(γ) dz 2 2iπ R(z 1 , z 2 ) F (2)
[P ] (z 2 , y)

= - C(γ) dz 1 2iπ 1 (x -z 1 ) 2 C(γ) dz 2 2iπ R(z 1 , z 2 ) F (2)
[P ] (z 2 , y)

= - C(γ) dz 2 2iπ ∂ x R(x, z 2 ) F (2)
[P ] (z 2 , y).

and we recognise A(x, z 2 ) = ∂ x R(x, z 2 ). Hence the statement is valid for F

[P +1] and we conclude by induction. We thus have established the functional equation in Proposition 4.8.

The proof of Proposition 4.9 is similar, except that we use F • [0] = F • for initialisation, and later, the combinatorial relation (3.11) instead of (3.6). □ 4.5. Depth of a vertex. We now consider the depth P of a vertex chosen at random in a disk configuration of the loop model. P is by definition the number of loops that separate it from the boundary. This quantity gives an idea about how nested maps in the loop model are. Equivalently, P is the depth of the origin in an ensemble of pointed disk configurations. We can study this ensemble in the microcanonical approach -i.e., fixing the volume equal to V and the perimeter equal to L -or in the canonical approachrandomising the volume V with a weight u V and the perimeter with a weight x -(L+1) .

In the canonical approach, the generating function of the depth distribution can be expressed in terms of the refined generating series of § 3.5:

(4.18) E[s P ] = F • s (x) F • (x) .
In the microcanonical approach, the probability that, in an ensemble of pointed disks of volume V and perimeter L, the depth takes the value P reads:

P P V , L = [u V • x -(L+1) • s P ] F • s (x) [u V • x -(L+1) ] F • (x)
.

Computations in the loop model with bending energy

We shall focus on the class of loop models on triangulations with bending energy (see § 2.1.2) studied in [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF], for which the computations can be explicitly carried out. The annuli generating series in this model are:

R(x, z) = n ln 1 1 -αh(x + z) -(1 -α 2 )h 2 xz , A(x, z) = n ς(z) -x = n ς ′ (x) z -ς(x) + ς ′′ (x) 2ς ′ (x) , (5.1)
where:

(5.2)

ς(x) = 1 -αhx αh + (1 -α 2 )h 2 x
is a rational involution. In terms of the loop model, h is the weight per triangle crossed by a loop, α is the bending energy, and we assume they are both non negative. Note that, for α = 1, we have ς(x) = 1 hx, so ς ′′ (x) = 0. In general:

ς ′′ (x) 2ς ′ (x) = - 1 x + α (1-α 2 )h = - 1 x -ς(∞)
.

If we assume ς(γ) ∩ γ = ∅ and f is a holomorphic function in C \ γ such that f (x) ∼ c f /x when x → ∞, we can evaluate the contour integral:

(5.3)

C(γ) dz 2iπ A(x, z) f (z) = -nς ′ (x) f (ς(x)) + nc f ς ′′ (x) 2ς ′ (x) .
5.1. Preliminaries. Technically, the fact that A(x, z) is a rational function with a single pole allows for an explicit solution of the model, and the loop model with bending energy provides a combinatorial realisation of such a situation. We review the solution of the functional equations for strictly admissible weights (see Section 4), which amounts to requiring ς(γ) ∩ γ = ∅ or equivalently

γ + < γ * + := 1 h(α + 1)
The techniques to solve these functional equations have already been developed in [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF] slightly generalising [START_REF] Borot | Quelques problèmes de géométrie énumérative, de matrices aléatoires, d'intégrabilité, étudiés via la géometrie des surfaces de Riemann[END_REF][START_REF] Borot | Enumeration of maps with self avoiding loops and the O(n) model on random lattices of all topologies[END_REF][START_REF] Eynard | More on the exact solution of the O(n) model on a random lattice and an investigation of the case |n| > 2[END_REF], and we refer to these works for more details. In the next Section 6, we will study the non-generic critical weight by taking the limit γ + → γ * + in these solutions.

The key to the solution is the use of an elliptic parametrisation x = x(v). It depends on a parameter τ = iT which is completely determined by the data of γ ± and ς(γ ± ). The domain C \ γ ∪ ς(γ) will be the image via v → x(v) of the rectangle (Figure 8)

(5.4) R := v ∈ C, Re v ∈ -1 2 , 1 2 , Im v ∈ (0, T ) , with values: (5.5) x(τ ) = x(-τ ) = γ + , x τ + 1 2 = x -τ + 1 2 = γ -, x(0) = ς(γ + ), x 1 2 = x -1 2 = ς(γ -). We let (5.6) R = v ∈ C, Re v ∈ -1 2 , 1 2 , Im v ∈ [0, T ]
. and say that x is in the physical sheet when v(x) ∈ R. For x in the physical sheet, we have v(ς(x)) = τv(x). We call v ∞ the point corresponding to x = ∞ in the physical sheet. With our assumptions, the involution ς is decreasing and we have γ + < γ * + < ς(γ + ). Therefore, the point ∞ can be to the right of ς(γ + ) and to the left of ς(γ -), or to the right of ς(γ -) and to the left of

γ -, that is v ∞ ∈ 0, 1 2 ∪ 1 2 , 1 2 + τ At least when we have ς -1 (∞) / ∈ (-γ * + , γ * + ), that is when α > 1 2
, we must be in the second situation:

(5.7) v ∞ = 1 2 + τ w ∞ , w ∞ ∈ (0, 1).
When α = 1, by symmetry we must have w ∞ = 1 2 . Remark 5.1. For simplicity, we will assume in the remaining of the text that (5.7) is satisfied unless explicitly mentioned otherwise, i.e. that α is not too small; the main conclusions of our study are not affected when v ∞ belongs to τ, 1 2 +τ , but some intermediate steps of analysis of the critical regime are a bit different. The function v → x(v) is analytically continued for v ∈ C by the relations:

0 γ + ς(γ + ) γ - ς(γ -) τ = iT 1 2 + τ 1 2 γ - ς(γ -) -1 2 + τ -1 2 ∞ 1 2 + τ w ∞
(5.8) x(-v) = x(v + 1) = x(v + 2τ ) = x(v).
This parametrisation allows the conversion [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF][START_REF] Eynard | More on the exact solution of the O(n) model on a random lattice and an investigation of the case |n| > 2[END_REF] of the functional equation:

(5.9)

∀x ∈ γ, f (x + i0) + f (x -i0) -n ς ′ (x) f (ς(x)) = 0
for an analytic function f (x) in C \ γ, into the functional equation:

(5.10) ∀v ∈ C, f (v + 2τ ) + f (v) -n f (v + τ ) = 0, f (v) = f (v + 1) = -f (-v),
for the analytic continuation of the function

f (v) = f (x(v))x ′ (v).
The second condition in (5.10) enforces the continuity of f (x) on R \ γ. We set:

(5.11) b = arccos(n/2) π .
The new parameter b ranges from 1 to 0 when n ranges from -2 to 2, and b = 1 2 corresponds to n = 0. We emphasise the following uniqueness property which we will use repeatedly. It can be traced back to [START_REF] Eynard | More on the exact solution of the O(n) model on a random lattice and an investigation of the case |n| > 2[END_REF] but we reproduce the argument for completeness.

Lemma 5.2. If n ∈ (-2, 2), there is at most one solution f (v) to the equation ∀v ∈ C, f (v + 2τ ) + f (v) -nf (v + τ ) = 0, f (v) = f (v + 1)
which is an entire function of v.

Proof. If f is a solution, the functions

f ± (v) = f (v) -e ±iπb f (v + τ ) 1 -e ±iπb satisfy f ± (v + 1) = f ± (v) = e ∓iπb f (v + τ ) for v ∈ C.
Since b is real-valued, f + and f -must be bounded entire functions, so must be constant by Liouville's theorem. The pseudo-periodicity condition in the τ direction then implies f ± = 0 hence f = 0. □ Solutions of the first two equations of (5.10) with prescribed divergent part at prescribed points in R can be built from a fundamental solution Υ b , defined uniquely by the properties:

(5.12)

Υ b (v + 1) = Υ b (v), Υ b (v + τ ) = e iπb Υ b (v), Υ b (v) ∼ v→0 1 v .
Its expression and main properties are reminded in Appendix D. In combination with Lemma 5.2 this provides an effective way to solve the functional equations.

Remark. We will encounter the linear equation with non zero right-hand side given by a rational function g(x):

(5.13)

f (x + i0) + f (x -i0) -n ς ′ (x) f (ς(x)) = g(x).
It is enough to find a particular solution in the class of rational functions and subtract it from f (x) to obtain a function f hom (x) satisfying (5.13) with vanishing right-hand side. This can be achieved for n ̸ = ±2 by:

(5.14)

f hom (x) = f (x) - 1 4 -n 2 2g(x) + nς ′ (x)g(ς(x)) . 5.2.
Disk and cylinder generating series. We now review the results of [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF] for the generating series of disks F(x) for subcritical weights. Let G(v) be the analytic continuation of (5.15)

x

′ (v)F(x(v)) - ∂ ∂v 2V(x(v)) + nV(ς(x(v))) 4 -n 2 - nu ln ς ′ (x(v)) 2(2 + n) , where V(x) = x 2 2 -k≥1 g k x k
k collects the weights of empty faces. In the model we study, empty faces are triangles counted with weight g each, so V(x) = x 2 2 -g x 3 3 . However, there is no difficulty in including Boltzmann weights for empty faces of higher (bounded) degree as far as the solution of the linear equation is concerned, so we shall keep the notation V(x). Note that the last term in (5.15) is absent if α = 1. Let us introduce (g k ) k≥1 as the coefficients of expansion:

(5.16) ∂ ∂v - 2V(x(v)) 4 -n 2 + 2u ln x(v) 2 + n = k≥0 gk (v -v ∞ ) k+1 + O(1), v → v ∞
Their expressions for the model where all faces are triangles are recorded in Appendix C.

Theorem 5.3 (Disks [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF]). We have:

G(v) = k≥0 1 2 gk k! ∂ k ∂v k ∞ Υ b (v + v ∞ ) + Υ b (v -v ∞ ) -Υ b (-v + v ∞ ) -Υ b (-v -v ∞ ) .
The endpoints γ ± are determined by the two conditions:

(5.17) G(τ + ε) = 0, ε = 0, 1 2 , which follow from the finiteness of the generating series F(x) at x = γ ± .

If α = 1, the 4 terms expression can be reduced to 2 terms using τv ∞ = v ∞ mod Z and the pseudo-periodicity of the special function Υ b .

Remark 5.4. We refer to the original paper for the derivation of Theorem 5.3. In all rigor, the conditions (5.17) may yield several solutions for the cut endpoints γ ± , and the correct choice corresponds to the solution which leads to a series F with positive coefficients. The original paper used numerical evidence as a justification. For the rigid case [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF], a formal justification was later provided in [START_REF] Budd | The peeling process on random planar maps coupled to an O(n) loop model (with an appendix by L. Chen[END_REF] via two theorems, due to Timothy Budd and Linxiao Chen respectively, see also [37, Chapter II]. Here we consider the bending energy model, to which these theorems do not apply directly. In Appendix H, we prove the analogue of Budd's theorem for the bending energy model, for n ∈ (0, 2). To keep a bound on the size of this paper, we do not prove the analogue of Chen's theorem, but we believe that there should be no unsurpassable obstacle in generalising his approach. Such an argument is also necessary to justify completely the phase diagram of the model.

Remarkably, the generating series of pointed disks and of cylinders have very simple expressions.

Proposition 5.5 (Pointed disks). Define G • (v) as the analytic continuation of:

(5.18) x ′ (v)F • (x(v)) + ∂ ∂v nu ln[ς ′ (x(v))] 2(2 + n) .
(for α = 1 the last term is absent). We have:

(5.19) G • (v) = u 2 + n -Υ b (v + v ∞ ) -Υ b (v -v ∞ ) + Υ b (-v + v ∞ ) + Υ b (-v -v ∞ ) .
Proof. The strategy is similar to [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF]. In the functional equation of Proposition 4.7, we can evaluate the contour integral using (5.3) and F • (x) ∼ u x when x → ∞. Thus:

(5.20) ∀x ∈ γ, F • (x + i0) + F • (x -i0) -nς ′ (x) F • (ς(x)) = nu x -ς(∞) .
We can find a rational function of x which is a particular solution to (5.20), and subtract it from F • (x) to obtain a solution of the linear equation with vanishing right-hand side. This is the origin of the second term in (5.18). The construction reviewed in § 5.1 then implies that G • (v) satisfies the functional relation:

(5.21) G • (v + 2τ ) + G • (v) -nG • (v + τ ) = 0, G • (v) = G • (v + 1) = -G • (-v).
G • (v) inherits the singularities of (5.18). If α ̸ = 1, we have a simple pole in the fundamental domain at:

(5. [START_REF] Borot | Nesting statistics in the O(n) loop model on random maps of arbitrary topologies[END_REF])

Res v=v∞ dv G • (v) = -2u 2 + n , Res v=(τ -v∞) dv G • (v) = -nu 2 + n .
(5.19) provides the (unique by Lemma 5.2) solution to this problem. When α = 1, we have ς(∞) = ∞, and

v ∞ = 1+τ 2 , therefore v ∞ = τ -v ∞ mod 1.
Then, we have a unique simple pole in the fundamental domain:

Res v=v∞ dv G • (v) = -u.
In this case, we find:

G • (v) = u 1 + e -iπb -Υ b (v -v ∞ ) + Υ b (-v -v ∞ ) .
Using the properties of Υ b under translation, this is still equal to the right-hand side of (5.19). In other words, formula (5.19)

is well behaved when v ∞ → (τ -v ∞ ). □ Proposition 5.6 (Cylinders). Define G (2) (v 1 , v 2 )
as the analytic continuation of:

(5.23)

x ′ (v 1 )x ′ (v 2 )F (2) (x(v 1 ), x(v 2 )) + ∂ ∂v 1 ∂ ∂v 2 2 ln x(v 1 ) -x(v 2 ) + n ln ς(x(v 1 )) -x(v 2 ) 4 -n 2 .
We have:

(5.24) G (2) (v 1 , v 2 ) = 1 4 -n 2 Υ ′ b (v 1 + v 2 ) -Υ ′ b (v 1 -v 2 ) -Υ ′ b (-v 1 + v 2 ) + Υ ′ b (-v 1 -v 2 ) .
Proof. This result is proved in [20, Section 3.4] for α = 1, but its proof actually holds when ς is any rational involution. We include it for completeness. The fact that ς is an involution implies that G (2) (v 1 , v 2 ) is a symmetric function of v 1 and v 2 , as:

dx 1 dx 2 (x 1 -x 2 ) 2 = dς(x 1 )dς(x 2 ) (ς(x 1 ) -ς(x 2 )) 2 .
It must satisfy: (5.25), and no other singularities. Equation (5.24) provides the (unique by Lemma 5.2) solution to this problem. □ 5.3. Refinement: separating loops. We have explained in § 4.4 that the functional equation satisfied by refined generating series, with a weight s per separating loop, only differs from the unrefined case by keeping the same cut γ, but replacing n → ns in the linear functional equations. Thus defining:

G (2) (v 1 , v 2 ) + G (2) (v 1 + 2τ, v 2 ) -nG (2) (v 1 + τ, v 2 ) = 0, G (2) (v 1 , v 2 ) = G (2) (v 1 + 1, v 2 ) = -G (2) (-v 1 , v 2 ). (5.25) It has a double pole at v 1 = v 2 so that G (2) (v 1 , v 2 ) = 2 4-n 2 1 (v 1 -v 2 ) 2 + O(1), double poles at v 1 = v 2 + (Z ⊕ τ Z) ensuing from
(5.26) b(s) = arccos(ns/2) π ,
we immediately find:

Corollary 5.7 (Refined pointed disks). Let G • s (v) be the analytic continuation of:

(5.27) x ′ (v)F • s (x(v)) + ∂ ∂v ns ln[ς ′ (x(v))] 2(2 + ns) .
We have:

(5.28) G • s (v) = u 2 + ns -Υ b(s) (v+v ∞ )-Υ b(s) (v-v ∞ )+Υ b(s) (-v+v ∞ )+Υ b(s) (-v-v ∞ ) . □ Corollary 5.8 (Refined cylinders). Let G (2)
s (v 1 , v 2 ) be the analytic continuation of:

x ′ (v 1 )x ′ (v 2 )F (2) s (x(v 1 ), x(v 2 )) + ∂ ∂v 1 ∂ ∂v 2 2 ln x(v 1 ) -x(v 2 ) + ns ln ς(x(v 1 )) -x(v 2 ) 4 -n 2 s 2 .
We have:

(5.29) G (2) s (v 1 , v 2 ) = 1 4 -n 2 s 2 Υ ′ b(s) (v 1 + v 2 ) -Υ ′ b(s) (v 1 -v 2 ) -Υ ′ b(s) (-v 1 + v 2 ) + Υ ′ b(s) (-v 1 -v 2 ) . □ 6.

Depth of a vertex in disks

We now study the asymptotic behavior of the distribution of the depth P of the origin of a pointed disk, in loop model with bending energy. While the algebraic results that we have obtained in the previous sections are valid for nonpositive weights, we will in the rest of the paper assume that

n ∈ (0, 2), b ∈ 0, 1 2 , g, α ≥ 0, h > 0
unless specified otherwise.

6.1. Phase diagram and the volume exponent. The phase diagram of the model with bending energy is Theorem 6.1 below, and was established in [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF]. We review its derivation, and push further the computations of [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF] to derive (Corollary 6.6 below) the well known exponent γ str appearing in the asymptotic number of pointed rooted disks of fixed, large volume V , and justify delta-analyticity statements that are used for the asymptotic analysis. We remind that the model depends on the weight g per empty triangle, h per triangle crossed by a loop, and the bending energy α, and the weight u per vertex is set to 1 unless mentioned otherwise. A non generic critical point occurs when γ + approaches the fixed point of the involution:

(6.1) γ * + = ς(γ * + ) = 1 h(α + 1)
.

In this limit, the two cuts γ and ς(γ) merge at γ * + , and one can justify on the basis of combinatorial arguments [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF]Section 6]

that γ -→ γ * -with: |γ * -| < |γ * + | and ς(γ * -) ̸ = γ * -.
In terms of the parametrisation x(v), it amounts to letting T → 0, and this is conveniently measured in terms of the parameter:

q = e -π
T → 0. To analyse the non generic critical regime, we first need to derive the asymptotic behavior of the parametrisation x(v) and the special function Υ b (v). This is performed respectively in Appendix B and D. The phase diagram and the volume exponent can then be obtained after a tedious algebra, which is summarised in Appendix E. Theorems 6.1-6.2 and a large part of the calculations done in Appendix appeared in [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF]. Here, we push these calculations further to present some consequences on generating series of pointed disks/gaskets (Corollaries 6.7-6.8 below), and we add a detailed description of the analytic properties with respect to u. It is then possible to apply transfer theorems, i.e. extracting asymptotic behavior of coefficients of the generating series from the analysis of their singularities. Theorem 6.1. [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF] Assume α = 1, and introduce the parameter:

ρ := 1 -2hγ * -= 1 - γ * - γ * + .
There is a non generic critical line, parametrised by ρ ∈ (ρ min , ρ max ]:

g h = 4(ρb √ 2 + n - √ 2 -n) -ρ 2 (1 -b 2 ) √ 2 -n + 4ρb √ 2 + n -2 √ 2 -n h 2 = ρ 2 b 24 √ 4 -n 2 ρ 2 b(1 -b 2 ) √ 2 + n -4ρ √ 2 -n + 6b √ 2 + n -ρ 2 (1 -b 2 ) √ 2 -n + 4ρb √ 2 + n -2 √ 2 -n .
It realises the dense phase of the model. The endpoint

ρ max = 1 b 2 -n 2 + n
corresponds to the fully packed model g = 0, with the critical value h =

1 2 √ 2 √
2+n . The endpoint

ρ min = √ 6 + n - √ 2 -n (1 -b) √ 2 +
n is a non generic critical point realising the dilute phase, and it has coordinates:

g h = 1 + 2 -n 6 + n , h 2 = b(2 -b) 3(1 -b 2 )(2 + n) 1 - 1 4 (2 -n)(6 + n) .
The fact that the non generic critical line ends at ρ max < 2 is in agreement with |γ * -| < |γ * -|. Remark 6.2. In [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF], it is proved that there exists α c (n) > 1 such that, in the model with bending energy α < α c (n), the qualitative conclusions of the previous theorem still hold, with a more complicated parametrisation of the critical line given in Appendix E. For α = α c (n), only a non generic critical point in the dilute phase exists, and for α > α c (n), non generic critical points do not exist. Theorem 6.3. Assume (g, h) are chosen such that the model has a non generic critical point for vertex weight u = 1. When u < 1 tends to 1, we have:

q ∼ 1 -u ∆ c .
with the universal exponent:

c = 1 1-b dense 1 dilute .
The non universal constant reads, for α = 1:

∆ = 6(n+2) b ρ 2 (1-b) 2 √ 2+n+2ρ(1-b) √ 2-n-2 √ 2+n ρ 2 b(1-b 2 ) √ 2+n-4ρ(1-b 2 ) √ 2-n+6b √ 2+n dense 24 b(1-b)(2-b)
dilute .

For α ̸ = 1, its expression is much more involved, but all the ingredients to obtain it are in Appendix E.

We in fact obtain a stronger information in the Appendices.

Lemma 6.4. u → q is delta-analytic.

This statement has two parts: delta-analyticity locally around u = 1, which is justified in Lemma E.3; and analytic continuation across the unit circle away from u = 1, which is justified in Theorem I.3 for the rigid loop model, and more generally in Theorem J.1 for the bending energy model. 6.2. Singular behavior of refined generating series. We would like to study the asymptotic behavior of the weighted count of:

(i) pointed disks with fixed volume V and fixed depth P , in such a way that V, P → ∞. (ii) cylinders with fixed volume V , with two boundaries separated by P loops, in such a way that V, P → ∞.

This information can be extracted from the canonical ensemble where a map with a boundary of perimeter L i is weighted by x -(L i +1) , each separating loop is counted with a weight s, and each vertex with a weight u. The generating series of interest are respectively F • s (x) for (i), and F

s (x 1 , x 2 ) for (ii). To retrieve the generating series of maps with fixed, large V and P , we must first obtain scaling asymptotics for these generating series when u → 1.

As for fixing boundary perimeters, two regimes can be addressed. Either we want L i to diverge, in which case we should derive the previous asymptotics when x approached the singularity γ + → γ * + , since the other endpoint |γ * -| < |γ * + | is subdominant. Or, we want to keep L i finite. In that case, we can work in the canonical ensemble by choosing x away from [γ -, γ + ]. We will actually consider the canonical ensemble with a control parameter w i such that x i = x 1 2 + τ w i , and derive asymptotics for w i in some compact region containing [0, 1). The asymptotic count of maps with fixed, finite boundary perimeter L i can then be retrieved by a contour integration around w i = w * ∞ . In a nutshell, we will set x = x(v i ) with v i = ε i + τ w i and ε i = 0 to study a i-th boundary of large perimeter, and ε i = 1 2 to study finite boundaries. The scaling behavior of F • s (x) in the regime of large boundaries is established in Appendix F. Theorem 6.5. Let (g, h) be a non generic critical point at u = 1. F • s (x) is an analytic family of meromorphic functions of x, parametrised by u, s where u belongs to a deltadomain centered at 1 and s to the strip |Re s| <2 n . Besides, if Re b(s) ∈ 0, 1 2 , when u → 1, in the two regimes x → γ + and x fixed away from the cut, we have respectively 2

F • s (x)| sing = q b(s)-1 2 1 -q b(s) Φ b(s) x -γ + q 1 2 + O(q b(s)
2 ),

F • s (x)| sing = Ψ b(s) (x) + q b(s) 1 -q b(s) Ψb(s) (x) + O(q). (6.2)
The error in the first line of (6.2) is uniform for ξ = q -1 2 (xγ + ) in any fixed compact, and compatible3 with differentiation. For the expression of the scaling functions, we refer to (F.5)-(F.6) and (F.7)-(F.8) in the Appendix. Corollary 6.6. Assume (g, h) are chosen such that the model has a non generic critical point for vertex weight u = 1. The number of pointed rooted planar maps of volume V → ∞ behaves like:

[u V • x -4 ] F • (x) ∼ A ∆ bc [-Γ(-bc)] V 1+bc .
for some positive constant A > 0 given in Appendix, (F.11)-(F.12). Therefore, the critical exponent mentioned in (2.6) is γ str = -bc.

Corollary 6.7. Assume (g, h) are chosen such that the model has a non generic critical point for vertex weight u = 1. The number of rooted maps of volume V → ∞ with a marked point in the gasket behaves as:

[u V • x -4 ] F • in gasket (x) ∼ A gasket ∆ c 2 [-Γ(-c 2 )] V 1+ c 2 .
for a non universal constant A gasket > 0 given in Appendix, (F.14)-(F.15).

We can deduce the behavior when V → ∞ of the probability that in a pointed rooted disk of volume V , the origin belongs to the gasket: Corollary 6.8. Assume (g, h) are chosen such that the model has a non generic critical point for vertex weight u = 1. When V → ∞:

P • in gasket V, L = 3 ∼ A gasket A Γ(-bc) Γ(-c 2 ) 1 ∆ c( 1 2 -b) V c( 1 2 -b
) . 6.3. Central limit theorem for the depth. We are going to prove the following result. Theorem 6.9. Let (g, h) be a non generic critical point at u = 1. Consider an ensemble of refined pointed disks of volume V , boundary perimeter L. Let P the random variable giving the depth, i.e. the number of loops separating the origin from the boundary. When L is chosen independent of V , we have as V → ∞ the convergence in law

P -cpopt π ln V √ ln V → N (0, σ 2 ), p opt = n √ 4 -n 2 , σ 2 = 4nc π(4 -n 2 ) 3 2
. which is uniform for L > 0 bounded. When L = ⌊ℓV c/2 ⌋ and V → ∞ while ℓ is bounded and bounded away from 0, we have

P -cpopt 2π ln V √ ln V → N (0, σ 2 ), σ 2 = 2nc π(4 -n 2 ) 3 2 .
Proof. We first treat the case of L being a fixed integer. By Lévy's continuity, it is sufficient to prove that for t ∈ R

(6.3) lim V →∞ ϕ V (t) = exp σ 2 t 2 2 , ϕ V (t) = E exp it P -cpopt 2π √ ln V V, L .
The characteristic function can be computed by

ϕ V (t) = exp -itcp opt √ ln V x L dx 2iπ du 2iπ u V +1 F • exp(it/ √ ln V ) (x) x L dx 2iπ du 2iπ u V +1 F • (x)
, where the contours in x surrounds ∞ and the contours in u initially surrounds u = 0. We first look at the numerator. For fixed x in a u-independent neighborhood of ∞, we first use Theorem 6.5, in particular the second line in (6.2), with a fixed s in a small enough neighboorhood of 1. The term Ψ b(s) (x) can be discarded as it does not contribute to the integral in u. The second term in

F • s (x)| sing is (6.4) q b(s) 1 -q b(s) Ψ b(s) (x) ∼ 1 -u ∆ cb(s) Ψ b(s) (x)
uniformly for s and x in their respective domains mentioned above. Computing the contour integral in x therefore preserves the error, and by transfer theorem (here we rely on Lemma E.3), the u → 1 asymptotics yields the V → ∞ asymptotics

dx x L 2iπ du 2iπ u V +1 F • s (x) ∼ dx x L 2iπ Ψb(s) (x) ∆ cb(s) [-Γ(b(s)c)] V 1+cb(s) ,
again uniformly in s. We can therefore compute the integral over x and substitute s = s V (t) := it √ ln V . Doing the same for the denominator -this amounts to set s = 1 -we get

ϕ V (t) ∼ exp -itcp opt √ ln V dx x L 2iπ Ψb(s V (t)) (x) dx x L 2iπ Ψb (x) ∆ c(b-b(s V (t))) -Γ(-bc) -Γ(-b(s V (t))c) V c(b-b(s V (t))) .
Since s V (t) → 1, the prefactors disappear in the limit and expanding V c(b-b(s V (t))) up to o(1) we find

ϕ V (t) ∼ exp it √ ln V cn π √ 4 -n 2 -cp opt + 2cnt 2 π(4 -n 2 ) 3 2
.

The value of p opt = n √ 4-n 2 exactly cancels the divergent term, and we obtain (6.3) with variance (6.5)

σ 2 = 4cn π(4 -n 2 ) 3 2
.

When L = ⌊ℓV c/2 ⌋, we have L = ℓV c/2 + o(V c/2 ). We now move the contour in x to surround [γ -, γ + ] at distance q 1 2 , hence depending on u, so that it can be converted into a u-independent contour L in the variable w such that q -1 2 (x

-γ + ) = x * 0 (w) + O(q 1
2 ). A difficulty is that now

x L = γ + + q 1 2 x * 1 2 (w) + O(q)
L with q → 0 and L → ∞. It is however possible to repeat the proof of the transfer theorem [69, Theorem IV.3] and show that we only need the asymptotic of the integrand when u → 1 at scale 1u = O(V -1 ). In this case we have q 1) and thus we can use

1 2 V c 2 = O(
x L ∼ γ L + exp -ℓx * 1 2 (w)[(1 -u)V /∆] c 2 + o(1) .
The rest of the analysis is similar to the previous case, with factor q b(s) replaced by q b(s)-1 2

. Omitting the details, we arrive to

ϕ V (t) ∼ exp it √ ln V cn π √ 4 -n 2 -cp opt + 2cnt 2 π(4 -n 2 ) 3 2
, and this gives the central limit theorem with mean and variance divided by 2 compared to the previous case. □ 6.4. Large deviations for the depth: main result. The central limit theorem directly came from the analysis of the singularity F • s . We now refine it to obtain large deviations for the depth. Theorem 6.10. Let (g, h) be a non generic critical point at u = 1. Consider the random ensemble of refined disks of volume V , boundary perimeter L. When V → ∞ and ℓ remains fixed positive, the probability that the origin is separated from the boundary by P loops behaves like:

P P = c ln V π p V, L = ℓ . ≍ 1 √ ln V V c π J(p) , (6.6
)

P P = c ln V 2π p V, L = ⌊ℓV c 2 ⌋ . ≍ 1 √ ln V V c 2π J(p) .
(6.7)

These estimates are uniform for p bounded and bounded away from 0. The large deviations function reads: From a macroscopic point of view, a pointed disk with a finite boundary looks like a sphere with two marked points, while a pointed disk with large boundary looks like a disk. We observe that in the regime where P .

J(p) = sup

≍ ln

V P 2P V, L = ℓ . ≍ P P V, L = ℓV c 2 2
Intuitively, this means that the nesting of loops in a sphere can be described by cutting the sphere in two independent halves (which are disks). In Section 9.4 and in particular Corollary 9.9, we will find an analog property for CLE.

The remaining of this section is devoted to the proof of these results. The probability that the origin of a pointed disk is separated from the boundary by P loops reads:

P[P | V, L] = P(V, L; P ) P(V, L)
and we need to analyse, when V → ∞, and L and P in various regimes, the behavior of the integrals:

P(V, L, P ) = du 2iπ u V +1 x L dx 2iπ ds 2iπs P +1 F • s (x), P(V, L) = du 2iπ u V +1 x L dx 2iπ F • (x). (6.9)
The contours for u and s are initially small circles around 0, and the contour for x surrounds the union of the cuts [γ -, γ + ] for the corresponding u's.

6.5. Proof of Theorem 6.10 for finite perimeters. When L is finite, we can keep the contour integral over x away from the cut. So, we need to use (6.2). The first term disappears when integrating over u, and remains: (6.10)

F • s (x)| sing = - q b(s) Ψb(s) (x) 1 -q b(s) + O(q),
where the error in (6.10) is uniform for x in any compact away from the cut for s in the strip |Re s| < 2 n away from its boundaries. The first term does not depend on u, therefore it does not contribute to the contour integral and can be discarded. Since q ∼ 1-u ∆ c when u → 1 and is delta-analytic, we find directly by transfer theorems:

(6.11) P(V, L) ∼ C([γ * -,γ * + ]) x L dx 2iπ Ψb (x) 1 [-Γ(-bc)]∆ bc 1 V 1+bc .
Due to the aforementioned uniformity of the estimates with respect to x and s, we also have (6.12)

P(V, L, P ) ∼ C([γ * -,γ * + ]) ds 2iπ s P +1 x L dx 2iπ Ψb(s) (x) [-Γ(-b(s)c)]∆ b(s)c 1 V 1+b(s)c .
where the contour in s initially surrounds 0 and must remain away from the boundaries of the strip |Re s| < 2 n . Through the analysis the x-contour surrounding [γ * -, γ * + ] will be fixed independent of s. We are going to apply the saddle point method to analyse the behavior of the s-contour integral when P → ∞. The integral to compute is The location of the critical point suggests to take a fixed value of p > 0 and set

P(V, L, P ) := C([γ * -,γ * + ]) dx x L 2iπ ds 2iπs Ψb(s) (x) e S (s) Γ(-b(s)c)∆ b(s)c V 1+bc
P := cp ln V π
We also define pV as the function of (p, V ) such that (6.17)

P = cp ln V π , It is such that (6.18) p -p ∈ O 1 ln V Step 1. Let ϵ > 0 small so that ρ(p) := n 2 |s(p) + iϵ| < 1. Then for V large enough, |s(p) + iϵ| < 2
n . We deform the s-contour to a contour C defined as follows. It is the union of the vertical segment C + 1 from s(p)iϵ to s(p) + iϵ, followed by the counterclockwise arc of circle C + 2 in the upper-half plane joining s(p) + iϵ to -s(p) + iϵ, followed by the vertical segment C - 1 from -s(p) + iϵ to -s(p)iϵ, followed by the counterclockwise arc of circle C - 2 in the lower-half plane joining -s(p)iϵ to s(p)iϵ. We claim that there exists a choice of ϵ and of constant η > 0 depending on p but independent of V , such that for any

s ∈ C ± 2 (6.19) R(s) := Re S (s) -S (s(p)) < -η ln V Since s → R(s)
is even and its first term is independent of s ∈ C ± 2 by definition of the contour, it is sufficient to prove the existence of η > 0 such that R(s(p) ± iϵ) < -η ln V and that t → R ρ(p)e ±iπt is a decreasing function of t ∈ [0, 1 2 ]. The first point follows for ϵ small enough independently of V from the computation of the second derivative in (6. [START_REF] Borot | Formal multidimensional integrals, stuffed maps, and topological recursion[END_REF]), and we can choose η depending on p and not on V because pp ∈ O 1 ln V . To justify the second point, we compute

dR dt = ∓ c ln V π 2ρ(p) n Im 1 e ∓2iπt -ρ 2 (p)
where we use the standard determination of the square root. This quantity is nonnegative if and only if ∓Im e ∓2iπtρ 2 (p) = sin(2πt) ≥ 0, which indeed holds for t ∈ [0, 1 2 ]. We note that there exists a constant M (p) > 0 such that for x ∈ C([γ * -, γ * + ]) and s ∈ C, we have for V large enough

Ψb(s) (x) Γ(-b(s)c)∆ b(s)c ≤ M (p)
Together with (6. [START_REF] Borot | Loop models on random maps via nested loops: case of domain symmetry breaking and application to the Potts model[END_REF]) and (6.18) we deduce the existence of a constant M ′ (L, p) > 0 such that for V large enough (6.20)

C([γ * -,γ * + ]) dx x L 2iπ C + 2 ∪C - 2 ds 2iπs Ψb(s) (x) e S (s) Γ(-b(s)c)∆ b(s)c V ≤ 1 V 1+bc+ cJ(p) π M ′ (L, p) V η
Step 2. By parity in s, the contributions of C ± 1 to the P (V, L, P ) are equal. To study the contribution of C + 1 , the order of magnitude ln V of the Hessian in (6.16) suggests to perform the change of variables

s = s(p) + is √ ln V
Since s(p) corresponds to the critical point of S , we obtain by Taylor approximation at order 2

S (s) = - cJ(p) π - c π n 2 (1 + p 2 ) 2 8p s2 + O 1 √ ln V
and the error is uniform when

s ∈ C + 1 , that is |s| ≤ ϵ √ ln V . Besides, there exists a constant M (ϵ) > 0 such that for any x ∈ C([γ * -, γ * + ]) and s ∈ C + 1 , Ψb(s) (x) Γ(-b(s)c)∆ b(s)c ≤ M (ϵ)
and we have the convergence when

V → ∞, poinwise in s ∈ R Ψb(s) (x) Γ(-b(s)c)∆ b(s)c -→ Ψb(p) (x) Γ(-b(p)c)∆ b(p)c Dominated convergence then implies C([γ * -,γ * + ]) dx x L 2iπ C + 1 ds 2iπs Ψb(s) (x) e S (s) Γ(-b(s)c)∆ b(s)c V 1+bc ∼ C([γ * -,γ * + ]) dx x L 2iπ Ψb(p) (x) Γ(-b(p)c)∆ b(p)c • 1 √ ln V V 1+bc+ cJ( p) π R ds e -c π n 2 (1+p 2 ) 2 8p
s2

The effect of replacing p by p in the argument of J only results in changing the overall constant by a quantity that may now depend on V (since p depend on V ) but remains bounded and bounded away from 0. The prefactors bounded and bounded away from zero become irrelevant when we write

C([γ * -,γ * + ]) dx x L 2iπ C + 1 ∪C - 1 ds 2iπs . ≍ 1 √ ln V V 1+bc+J(p)
where we recall that F .

≍ G means that ln F = ln G + O(1). In comparison to this, the contribution of C + 2 ∪ C - 2 is negligible due to (6.20), hence

P (V, L, P ) . ≍ 1 √ ln V V 1+bc+ cJ(p) π
Taking the ratio with (6.11) cancels V 1+bc and leads to the desired estimate

P P = cp ln V π L . ≍ (ln V ) -1 2 V -cJ(p) π 6.6.
Proof of Theorem 6.10 for large perimeters. Now, we study (with less details) the case where the (x * , s * )-coordinates of the critical point are such that ξ * =

x * -γ * + (q * ) 1/2 has a limit, and s * has a limit away from 2/n. We can then use (6.2): (6.21)

F • s (x)| sing ∼ q b(s) 2 -1 2 1 -q b(s) Φ b(s) x -γ + q 1/2 .
We need to analyse the critical points of:

S 2 (u, x, s) = -V ln u -P ln s + L ln x + c 2 (b(s) -1) ln 1 -u ∆ + ln Φ b(s) x -γ * + [(1 -u)/∆] c 2 .
Compared to (6.21), we have replaced γ + by γ * + , as it only differ by O(q). The equation

∂ u S 2 = 0 gives: V ∼ -c 2 1 -u * b(s * ) -1 + ξ * (ln Φ b(s * ) ) ′ (ξ * ) , while the equation ∂ x S 2 = 0 gives: L γ * + ∼ - ∆ 1 -u * c 2 (ln Φ b(s * ) ) ′ (ξ * ). It is then necessary that L . ≍ V c 2 . The equation ∂ s S 2 = 0 gives: P s * ∼ nc ln(1 -u * ) 2π 4 -n 2 (s * ) 2 .
If we set P = c ln V 2π p, we obtain s * ∼ s(p) with the function introduced in (6.14). Notice the factor of 1 2 compared to (6.17) in the previous section, due to the occurrence of q b(s) 2

here and q b(s) there in the scaling limits of F • s (x). We also evaluate:

∂ 2 s S 2 (u * , x * , s(p))
.

≍ ln V.

Therefore, let us now assume:

L = ℓ V c 2 , P = cp ln V 2π
for a fixed positive ℓ. The previous discussion suggests the change of variable to compute P(V, L):

u = 1 - ũ V , x = γ * + + x V c 2
.

We then find:

du u V +1 dx x L F • s (x) ∼ dũ dx V 1+ cb 2 Φ b x (ũ/∆) c 2 e ũ+ℓx/γ * + u ∆ c 2 (b-1)
, where the convergence to the limit function in the right-hand side is uniform for (ũ, x) in any compact away from R 2 ≤0 . The contours can be deformed to steepest descent contours C 2 (see Figures 9 and10), and we can conclude as before by dominated convergence:

(6.22) P(V, L) ∼ C C dũ dx (2iπ) 2 e ũ+ℓx/γ * + ũ ∆ c 2 (b-1) Φ b x (ũ/∆) c 2 V -1-cb 2 .
Likewise, in order to compute P(V, L, P ), we make the change of variable:

u = 1 - ũ V , s = s(p) + s √ ln V , x = γ * + + x V c 2 .
We then find:

du u V +1 ds s P +1 dx x L F • s (x) ∼ dũ dx ds (γ * + ) L s(p) V 1+ c 2 b(p)+ c p 2π ln s(p) √ ln V Φ b(s) x (ũ/∆) c 2 e ũ+ℓx/γ * + ũ ∆ c 2 (b(s)-1) exp cn 2 (p 2 + 1) 2 16π p s2 ,
where the convergence to the limit function in the right-hand side is uniform for s, x, ũ in any compact with ũ away from 0. We deform the contours to steepest descent contours C 2 in the variables (x, u), and iR in the variable |s| ≪ √ ln V . By properties of steepest descent contours, we can apply dominated convergence and find:

P(V, L, P ) ∼ C C dx dũ (2iπ) 2 e ũ+ℓx/γ * + ũ ∆ c 2 (b(s)-1) Φ b(s) x (ũ/∆) c 2 × (ln V ) -1/2 V -1-c 2 b(p)-c p 2π ln s(p)
cp(p 2 + 1) .

Separating loops in cylinders

Let us consider the probability that, in a random ensemble of planar maps of volume V , two boundaries of given perimeter L 1 and L 2 are separated by P loops:

P[P | V, L 1 , L 2 ] = du 2iπ u V +1 x L 1 1 dx 1 2iπ x L 2 2 dx 2 2iπ ds 2iπ s P +1 F (2) s (x 1 , x 2 ) du 2iπ u V +1 x L 1 1 dx 1 2iπ x L 2 2 dx 2 2iπ F (2) (x 1 , x 2 )
.

The analog of Theorem 6.5 for the behavior of F

(2) s is derived in Appendix G, and it features singularities of the type4 q b(s)/j with j = 1 for x 1 and x 2 both close to or both away from γ * + , and j = 2 for x 1 close to γ * + and x 2 close to ∞. In that regard, the origin in pointed disks behaves as a boundary face whose perimeter is kept finite in a cylinder.

As the type of singularities encountered in the asymptotic analysis is identical, the result can be directly derived from Sections 6.5-6.6: Theorem 7.1. Let (g, h) be a non generic critical point at u = 1. Let ℓ 1 , ℓ 2 , p > 0. When V → ∞, we have

P P = c ln V π p V, L 1 = ℓ 1 , L 2 = ℓ 2 . ≍ 1 √ ln V V c π J(p) , P P = c ln V 2π p V, L 1 = ℓ 1 , L 2 = ⌊ℓ 2 V c 2 ⌋ . ≍ 1 √ ln V V c 2π J(p)
, where the large deviations function J(p) is the same as in (6.8). □

In the regime where the two boundaries of the cylinder have perimeter of order V c 2 , the nesting distribution behaves differently and is not analysed here. 8. Weighting loops by i.i.d. random variables 8.1. Definition and main result. Following [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF], we introduce a model of random maps with weighted loop configurations ; we describe it for pointed disks, but it will be clear that our reasoning extends to the cylinder topology. Let ξ be a random variable, with distribution µ, for which we assume that the cumulant function,

Λ µ (λ) := ln E[e λξ ],
exists for λ in a neighborhood of 0. Given a map with a self-avoiding loop configuration, let (ξ l ) l∈L be a sequence of i.i.d. random variables distributed like ξ, indexed by the set L of loops. Let L sep ⊆ L be the set of loops separating the boundary from the marked point. We would like the describe the joint distribution of the depth P = |L sep | and of the sum Ξ = l∈Lsep ξ l .

Recall from the proof of Proposition 4.9 that F • [P ] (x) is the generating series of pointed disks with exactly P separating loops. Our problem is solved by introducing the generating series F • s,λ (x), as the µ-expectation value of the generating series of pointed disks, whose usual weight in the loop model is multiplied by l∈Lsep s e λξ l . By construction, we have:

F • s,λ (x) = P ≥0 (se Λµ(λ) ) P F • [P ] (x) = F • s exp(Λµ(λ)) (x).
In the ensemble of pointed disks with volume V and perimeter L, the joint distribution we look for reads:

P(P, Ξ|V, L) = P(V, L; P, Ξ) P(V, L)
with a new numerator -compare with (6.9):

P(V, L; P, Ξ) = du 2iπu V +1 dx x L 2iπ ds 2iπ s P +1 dλ e -λΞ 2iπ F • s,λ (x).
Theorem 8.1. Let (g, h) be a non generic critical point at u = 1. Let5 ℓ, p, q > 0. When V → ∞, we have

P P = c ln V π p and Ξ = c ln V π q V, L = ℓ . ≍ 1 (ln V ) V c π J(p,q) , (8.1)
P P = c ln V 2π p and Ξ = c ln V 2π q V, L = ⌊V c 2 ℓ⌋ . ≍ 1 (ln V ) V c 2π J(p,q) . (8.2)
The bivariate large deviations function reads:

J(p, q) = J(p) + qλ ′ -Λ µ (λ ′ ),
in terms of J(p) defined in (6.8), and λ ′ is the function of (p, q) which is the unique solution to

q p = ∂Λ µ (λ ′ ) ∂λ ′ .
It is remarkable that the bivariate large deviations function is a sum of two terms, one being the usual n-dependent large deviations function for depth J(p), the other being µ-dependent but n-independent.

8.1.1. Bernoulli weights. For instance, if µ is the distribution of a signed Bernoulli random variable,

µ[ξ = -1] = µ[ξ = 1] = 1 2 , we have Λ µ (λ) = ln cosh(λ),
λ ′ = arctanh(q/p) = 1 2 ln p + q pq , and J(p, q) = J(p) + p + q 2 ln(p + q) + pq 2 ln(pq)p ln p.

Note that, as ξ ≤ 1, we have Ξ = l∈Lsep ξ l ≤ P , so we must have q ≤ p.

Gaussian weights.

If ξ is a centered Gaussian variable with variance σ 2 , we have:

Λ µ (λ) = σ 2 λ 2 2 , λ ′ = q pσ 2
and therefore:

J(p, q) = J(p) + q 2 2σ 2 p 2 .
8.2. Proof of Theorem 8.1. We give some details of the proof in the case of finite perimeters, as the modifications necessary in the case of large perimeters, L = ⌊V c 2 ℓ⌋, are parallel to the changes of Section 6.5 detailed in Section 6.6. As the strategy is similar to Section 6.5, we leave the details of the analysis to the reader. To analyse P(V, L; P, Ξ), we should study the critical points of:

S 1 (x, u, s, λ) = S 1 (x, u, se Λµ(λ) ) -λΞ = -V ln u -P ln s + cb(se Λµ(λ) ) + ln 1 -u ∆ -ln 1 - 1 -u ∆ cb(s exp(Λµ(λ)))
+ ln Ψb(s exp(Λµ(λ))) (x) -λΞ

(8.3)
Let (s * , λ * ) be the location of the critical point of S1 , and assume that s * has a limit away from 2 n , and λ * has a finite limit when V → ∞. Using the scalings6

P = c ln V π p, Ξ = c ln V π q,
we find that the equation ∂ s S1 = 0 yields in the limit V → ∞:

(8.4) ne Λµ(λ * ) 4 -(ns * e Λµ(λ * ) ) 2 = p s * ,
and the equation ∂ λ S1 = 0 yields likewise:

(8.5) ne Λµ(λ * ) Λ ′ µ (λ * ) 4 -(ns * e Λµ(λ * ) ) 2 = q s * ,
while the equation ∂ u S1 = 0 yields:

V ∼ -cb(s * e Λµ(λ * ) ) 1u * . Let us define λ ′ as a function of (p, q) in such a way that:

(8.6) ∂Λ µ ∂λ ′ = q p .
As ∂Λ ∂λ ′ (0) = E[ξ] and ∂ 2 Λµ ∂λ ′2 (0) = Var[ξ] > 0, λ ′ is defined at least for q p in the neighborhood of the value E[ξ], corresponding to λ ′ in a neighborhood of 0. We assume that q p belongs to the (maximal) domain of definition of λ ′ . Combining (8.4) and (8.5), we find that the saddle λ * is located at λ ′ , and:

s * e Λµ(λ ′ ) = s(p), b(s * e Λ(λ ′ ) ) = b(p),
in terms of the functions s and b defined in (6.14)-(6.15). We compute the Hessian matrix of S1 with respect to the variables (s, λ), and evaluated at the saddle point (s * , λ ′ ). At leading order in V ,

S1 = c ln V π Σ(s, λ) + o(ln V ), with Σ(s, λ) = πb(se Λµ(λ) ) -p ln s,
where the error o(ln V ) is stable under differentiation. After a tedious, but straightforward computation, we find:

H := ∂ 2 s Σ ∂ λ ∂ s Σ ⋆ ∂ 2 λ Σ s=s * λ=λ ′ = n 2 (p 2 +1) 2 4 exp(2Λ µ (λ ′ )) n(1+p 2 ) 3/2 2 ∂Λµ ∂λ ′ e Λµ(λ ′ ) ⋆ p ∂ 2 Λµ ∂λ ′2 + (p 2 + 1)( ∂Λµ ∂λ ′ 2 , (8.7)
where the lower corner of the matrix is deduced by symmetry. We also need to compute

det H = n 2 (p 2 + 1) 2 4 ∂ 2 Λ µ ∂λ ′2 e 2Λµ(λ ′ )
. Now, if we introduce the change of variables:

u = 1 - ũ V , s = e -Λµ(λ ′ ) s(p) + s √ ln V , λ = λ ′ + λ √ ln V , we obtain du u V +1 ds s P +1 dλ e -λΞ ∼ - dũ d λ V ln V Ψb(s exp(Λµ(λ ′ )) (x) s(p) exp(-Λ µ (λ ′ )) e ũ ũ ∆V cb(p) × V -c π (p ln s(p)-pΛµ(λ ′ )+qλ ′ ) exp c π (s, λ) • H • (s, λ) T .
We can perform the Gaussian integration in s and λ, while the remaining integration on ũ and x result in a prefactor already appearing in Section 6.5. The result is:

P V, L; P = cp ln V π ; Ξ = cq ln V π ∼ π Γ(-cb(p)) n 2 cp (p 2 + 1) ∂ 2 Λµ ∂λ ′2 C x L dx 2iπ Ψb(p) (x) ∆ cb(p) × V -1-cb(p)+ c π (-ln s(p)+Λµ(λ ′ )-qλ ′ ) (ln V ) -1 .
We obtain the final result (8.1) by dividing by P(V, L) given in (6.11), and replacing p with p such that P = cp ln V π ⌋, which only affect a O(1) term after taking logarithms. The proof of (8.2) is similar. □

Comparison with nesting in CLE via KPZ

In this section, we compare the large deviations of loop nesting at criticality in the O(n) model on a random planar map, as derived in the first sections of this work, with the large deviations of loop nesting in the so-called conformal loop ensemble in the plane. 9.1. Nesting in the conformal loop ensemble. The conformal loop ensemble CLE κ for κ ∈ (8/3, 8) is the canonical conformally invariant measure on countably infinite collections of non crossing loops in a simply connected domain D ⊂ C [START_REF] Sheffield | Exploration trees and conformal loop ensembles[END_REF][START_REF] Sheffield | Conformal loop ensembles: the Markovian characterization and the loop-soup construction[END_REF]. It is the analogue for loops of the celebrated Schramm-Loewner evolution SLE κ , the canonical conformally invariant measure on non crossing paths [START_REF] Schramm | Scaling limits of loop-erased random walks and uniform spanning trees[END_REF] in the plane, depending on the real positive parameter κ, an invention which is on par with Wiener's 1923 mathematical construction of continuous Brownian motion. It gives the universal continuous scaling limit of 2d critical curves; of particular physical interest are the loop-erased random walk (κ = 2) [START_REF] Lawler | Conformal invariance of planar loop-erased random walks and uniform spanning trees[END_REF], the self-avoiding walk (κ = 8

3 ), the Ising model interface (κ = 3 or 16 3 ) [START_REF] Chelkak | Universality in the 2D Ising model and conformal invariance of fermionic observables[END_REF][START_REF] Smirnov | Conformal invariance in random cluster models. I. Holomorphic fermions in the Ising model[END_REF], the GFF contour lines (κ = 4) [START_REF] Schramm | Contour lines of the two-dimensional discrete Gaussian free field[END_REF], and the percolation interface (κ = 6) [START_REF] Smirnov | Critical percolation in the plane: conformal invariance, Cardy's formula, scaling limits[END_REF]. Critical phenomena in the plane were earlier well known to be related to conformal field theory [START_REF] Belavin | Infinite conformal symmetry in two-dimensional quantum field theory[END_REF], a discovery anticipated in the so-called Coulomb gas approach to critical 2d statistical models (see, e.g., [START_REF] Nijs | Extended scaling relations for the magnetic critical exponents of the Potts model[END_REF][START_REF] Nienhuis | Exact critical point and critical exponents of O(n) models in two dimensions[END_REF]), and now including SLE [START_REF] Bauer | Conformal field theories of stochastic Loewner evolutions[END_REF][START_REF] Friedrich | Conformal restriction, highest weight representations and SLE[END_REF][START_REF] Kang | Gaussian free field and conformal field theory[END_REF].

In the same way as SLE κ is proven or expected to be the scaling limit of a single interface in 2d critical discrete models, CLE κ should be the limiting process of the collection of closed interfaces in such models. In particular, the critical O(n)-model on a regular planar lattice is expected to converge in the continuum limit to the universality class of the SLE κ /CLE κ , for

(9.1) n = 2 cos π 1 -4/κ , n ∈ [0, 2], κ ∈ ( 8 3 , 4] in dilute phase κ ∈ (4, 8) in dense phase.
In [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF] (see also [START_REF] Miller | The conformal loop ensemble nesting field[END_REF]), Miller, Watson and Wilson were able to derive the almost sure multifractal dimension spectrum of extreme nesting in the conformal loop ensemble. Fix a simply connected proper domain D ⊂ C and let Γ be a configuration of CLE κ . For each point z ∈ D, let N z (ε) be the number of loops of Γ which surround the ball B(z, ε) centered at z and of radius ε > 0. For ν > 0, define the random set (9.2)

Φ ν = Φ ν (Γ) := z ∈ D : lim ε→0 N z (ε) ln(1/ε) = ν .
This Hausdorff dimension of this set is almost surely equal to a constant, which is expressed in terms of the distribution of the conformal radius of the gasket of the origin in a CLE κ in the unit disk D. More precisely, the conformal radius CR(z, U) of a simply connected proper domain U ⊂ C is defined to be |φ ′ (0)|, where φ is the conformal map D → U which sends 0 to z. For a configuration Γ of CLE κ in D, let then U Γ be the connected component containing the origin in the complement D \ L of the largest loop L of Γ surrounding the origin in D, i.e. the interior of the outmost such loop. A formula for the cumulant generating function oflog(CR(0, U Γ )) was proposed in [START_REF] Cardy | [END_REF][START_REF] Cardy | Exact results for the universal area distribution of clusters in percolation, Ising, and Potts models[END_REF][START_REF] Dubédat | For κ = 6[END_REF][START_REF] Kenyon | Conformal radii of loop models[END_REF] and established in Ref. [START_REF] Schramm | Conformal radii for conformal loop ensembles[END_REF] (9.3)

Λ κ (λ) := ln E CR(0, U Γ ) -λ = ln    cos π(1 -4 κ ) cos π 1 -4 κ 2 + 8λ κ    , λ ∈ -∞, 1 -2 κ -3κ 32 .
The Legendre-Fenchel symmetric transform, Λ ⋆ κ : R → R + of Λ κ is defined by (9.4)

Λ ⋆ κ (x) := sup λ∈R (λx -Λ κ (λ)) .
It yields the continuous function on R + [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF],

(9.5) γ κ (ν) := νΛ ⋆ κ (1/ν) if ν > 0, 1 -2 κ -3κ 32 if ν = 0.
For κ ∈ (8/3, 8), the Hausdorff dimension of the set Φ ν is almost surely given by [120, Theorem 1.1],

(9.6) dim H Φ ν = max(0, 2 -γ κ (ν)),
with Φ ν being a.s. empty if γ κ (ν) > 2. Note that the Legendre-Fenchel transform equations above can be recast for γ κ (ν), ν > 0, as, (9.7)

γ κ (ν) ν = λ ν -Λ κ (λ), 1 ν = ∂Λ κ (λ) ∂λ ,
from which we immediately get,

(9.8) λ = ∂ ∂(1/ν) γ κ (ν) ν = γ κ (ν) -ν ∂ ∂ν γ κ (ν).
9.2. Liouville quantum gravity. Polyakov [START_REF] Polyakov | Quantum geometry of bosonic strings[END_REF] suggested in 1981 that the summation over random Riemannian metrics involved in a continuum theory of random surfaces could be represented canonically by the now celebrated Liouville theory of quantum gravity (see [START_REF] Duplantier | Liouville quantum gravity and KPZ[END_REF][START_REF] Francesco | 2d gravity and random matrices[END_REF][START_REF] Ginsparg | Lectures on 2d gravity and 2d string theory[END_REF][START_REF] Nakayama | Liouville field theory: a decade after the revolution[END_REF] and references therein). It is widely believed or proven in certain cases to provide, after a Riemann conformal map to a given planar domain, the correct conformal structure for the continuum limit of random planar maps, possibly weighted by the partition functions of various statistical models (see, e.g., the ICM reviews [START_REF] Duplantier | Liouville quantum gravity, KPZ and Schramm-Loewner evolution[END_REF][START_REF] Gall | Random Geometry on the Sphere[END_REF][START_REF] Miller | Liouville quantum gravity as a metric space and a scaling limit[END_REF]). In the case of usual random planar maps with faces of bounded degrees, the universal metric structure is that of the Brownian map [START_REF] Gall | Uniqueness and universality of the Brownian map[END_REF][START_REF] Miermont | The Brownian map is the scaling limit of uniform random plane quadrangulations[END_REF], which has been recently identified with that directly constructed from Liouville quantum gravity (LQG) [START_REF] Miller | An axiomatic characterization of the Brownian map[END_REF][START_REF] Miller | Liouville quantum gravity and the Brownian map I: The QLE(8/3,0) metric[END_REF][START_REF] Miller | Liouville quantum gravity and the Brownian map II: geodesics and continuity of the embedding[END_REF][START_REF] Miller | Liouville quantum gravity and the Brownian map III: the conformal structure is determined[END_REF]. Note also that different mathematical approaches to LQG exist [START_REF] David | Liouville quantum gravity on the Riemann sphere[END_REF][START_REF] Duplantier | Liouville quantum gravity as a mating of trees[END_REF][START_REF] Duplantier | Liouville quantum gravity and KPZ[END_REF][START_REF] Miller | Liouville quantum gravity spheres as matings of finite-diameter trees[END_REF], whose equivalence has been recently established [START_REF] Aru | Two perspectives of the 2d unit area quantum sphere and their equivalence[END_REF].

As mentioned in the introduction, Section 1, several models of random planar maps with critical statistical models have now been rigorously proven to converge to LQG surfaces, as path-decorated metric spaces [START_REF] Gwynne | Convergence of percolation on uniform quadrangulations with boundary to SLE 6 on 8/3-Liouville quantum gravity[END_REF][START_REF] Gwynne | Convergence of the self-avoiding walk on random quadrangulations to SLE 8/3 on 8/3-Liouville quantum gravity[END_REF], as mated pairs of trees [79-81, 86, 87, 96, 109, 138] in the so-called peanosphere topology of Refs. [START_REF] Duplantier | Liouville quantum gravity as a mating of trees[END_REF][START_REF] Miller | Liouville quantum gravity spheres as matings of finite-diameter trees[END_REF], or as Tutte embedding of mated-CRT maps [START_REF] Gwynne | The Tutte embedding of the mated-CRT map converges to Liouville quantum gravity[END_REF].

Here, in order to compare the asymptotic findings of previous sections to a direct LQG approach, we focus on the measure aspects associated with Liouville quantum gravity. 9.2.1. Liouville quantum measure [START_REF] Duplantier | Liouville quantum gravity and KPZ[END_REF]. Consider a simply connected domain D ⊂ C as the parameter domain of the random surface, and h an instance of the massless Gaussian free field (GFF), a random distribution on D, associated with the Dirichlet energy,

(h, h) ∇ := 1 2π D [∇h(z)] 2 d 2 z,
and whose two point correlations are given by the Green's function on D with Dirichlet zero boundary conditions [START_REF] Sheffield | Gaussian free fields for mathematicians[END_REF]. (Critical) Liouville quantum gravity consists in changing the Lebesgue area measure d 2 z on D to the quantum area measure, formally written as µ γ (d 2 z) := e γh(z) d 2 z, where γ is a real parameter. The GFF h is a random distribution, not a function, but the random measure µ γ can be constructed, for γ ∈ [0, 2], as the limit of regularised quantities, as follows.

Given an instance h of the GFF on D, for each z ∈ D, let h ε (z) denote the mean value of h on the circle of radius ε centered at z -where h(z) is defined to be zero for z ∈ C \ D [START_REF] Sheffield | Gaussian free fields for mathematicians[END_REF]. One then has E e γhε(z) = e γ 2 Var[hε(z)]/2 = [CR(z, D)/ε] γ 2 /2 , where CR(z, D) the conformal radius of D viewed from z. This strongly suggests considering the limit, (9.9)

µ γ (d 2 z) := lim ε→0 ε γ 2 /2 e γhε(z) d 2 z,
and one can indeed show that for γ ∈ [0, 2) this (weak) limit exists and is non degenerate, and is singular with respect to Lebesgue measure [START_REF] Duplantier | Liouville quantum gravity and KPZ[END_REF]. This mathematically defines Liouville quantum gravity, in a way reminiscent of so-called Wick normal ordering in quantum field theory -see also [START_REF] Høegh-Krohn | A general class of quantum fields without cut-offs in two space-time dimensions[END_REF] for earlier work on the so-called Høegh-Krohn model, and Kahane's general study of the so-called Gaussian multiplicative chaos [START_REF] Kahane | Sur le chaos multiplicatif[END_REF].

The critical case, γ = 2, requires additional care, and it is shown in [START_REF] Duplantier | Critical Gaussian multiplicative chaos: of the derivative martingale[END_REF][START_REF] Duplantier | Renormalization of critical Gaussian multiplicative chaos and KPZ relation[END_REF] (see also [START_REF] Aru | Critical Liouville measure as a limit of subcritical measures[END_REF]) that the weak limit, (9.10)

µ γ=2 (d 2 z) := lim ε→0 ln(1/ε) ε 2 e 2hε(z) d 2 z,
exists and is almost surely non atomic. µ γ (D) will be called the quantum area of D.

Remark 9.1. The Liouville quantum action is usually written as S(h) = 1 2 (h, h) ∇ +b µ γ (D), where the "(bulk) cosmological constant", b ≥ 0, weights the partition function according to the quantum area of the random surface. The corresponding Boltzmann statistical weight, exp[-S(h)], should be integrated over with a "flat" uniform functional measure Dh on h -which makes sense a priori for finite-dimensional approximations to h. The full Liouville quantum measure can then be constructed from the GFF one (see, e.g., [START_REF] David | Liouville quantum gravity on the Riemann sphere[END_REF]), and for our purpose of studying the CLE κ nesting properties, which are local ones, it will suffice to consider this measure for b = 0, i.e., in the GFF case. 9.2.2. Canonical coupling of LQG to SLE. Various values of γ are expected to describe weighting the random map by the partition function of a critical statistical physical model defined on that map (e.g., an Ising model, an O(n) or a Potts model). The correspondence can be obtained by first considering conformal welding in Liouville quantum gravity [START_REF] Duplantier | Liouville quantum gravity as a mating of trees[END_REF][START_REF] Duplantier | Schramm-Loewner evolution and Liouville quantum gravity[END_REF][START_REF] Sheffield | Conformal weldings of random surfaces: SLE and the quantum gravity zipper[END_REF][START_REF] Sheffield | Quantum gravity and inventory accumulation[END_REF] (see also [START_REF] Astala | Random conformal weldings[END_REF]). It turns out that pieces of Liouville quantum gravity surfaces of parameter γ ∈ [0, 2) can be conformally welded together to produce as random seams SLE κ curves, with the rigorous result, (9.11)

γ = √ κ if κ < 4 4 √ κ if κ > 4.
Together with (9.1), this provides us with the (γ, κ, n) correspondence that we sought after for the O(n) model. 9.2.3. KPZ formula. By the usual conformal invariance Ansatz in physics, it is natural to expect that if one conditions on the random map to be infinite, maps it into the plane, and then samples the loops or clusters in critical models, their law in the scaling limit will be independent of the random measure. This independence in turn leads to the Knizhnik, Polyakov, and Zamolodchikov (KPZ) formula [START_REF] Knizhnik | Fractal structure of 2D-quantum gravity[END_REF] -see also Refs. [START_REF] David | Conformal field theories coupled to 2-D gravity in the conformal gauge[END_REF][START_REF] Distler | Conformal field theory and 2D quantum gravity[END_REF] which is a relationship between (half) scaling dimensions (i.e., conformal weights x) of fields defined using Euclidean geometry and analogous dimensions (∆) defined via the Liouville quantum gravity measure µ γ , (9.12)

x = U γ (∆) := γ 2 4 ∆ 2 + 1 - γ 2 4 ∆.
The inverse of the relation (9.12) that is positive is given by (9.13)

∆ = U -1 γ (x) := 1 γ 4x + a 2 γ -a γ , a γ := 2 γ - γ 2 ≥ 0.
A mathematical proof of the KPZ relation, based on the stochastic properties of the GFF, first appeared in [START_REF] Duplantier | Liouville quantum gravity and KPZ[END_REF]; it was then also proved for multiplicative cascades [START_REF] Benjamini | KPZ in one dimensional random geometry of multiplicative cascades[END_REF] and in the framework of Gaussian multiplicative chaos [START_REF] Duplantier | Renormalization of critical Gaussian multiplicative chaos and KPZ relation[END_REF][START_REF] Rhodes | KPZ formula for log-infinitely divisible multifractal random measures[END_REF]. The KPZ formula holds for any fractal structure sampled independently of the GFF, and measured with the random measure µ γ , and for any 0 ≤ γ ≤ 2. For z fixed, a given quantum area δ, hence a given logarithmic coordinate A, corresponds through (9.14) to a random Euclidean radius ε, and the corresponding random value T A of t in (9.15) can be seen as a stopping time of some Brownian process [START_REF] Duplantier | Duality and KPZ in Liouville quantum gravity[END_REF][START_REF] Duplantier | Liouville quantum gravity and KPZ[END_REF]. The probability density of T A , such that P(t | A)dt := P T A ∈ [t, t + dt] , is obtained as a by-product of the KPZ analysis in [START_REF] Duplantier | Duality and KPZ in Liouville quantum gravity[END_REF][START_REF] Duplantier | Liouville quantum gravity and KPZ[END_REF]:

(9.16) P(t | A) = A √ 2πt 3 exp - (A -a γ t) 2 2t ;
it characterises, in logarithmic coordinates, the distribution of the Euclidean radius ε of a ball of given quantum area δ. For a GFF in a domain D with, say, Dirichlet boundary conditions, this local form is valid for a ball B(z, ε) far away from ∂D, i.e., for ε much smaller than the conformal radius C(z, D), or, equivalently, than the Euclidean distance between z and the boundary ∂D, since theorem. Note that we can rewrite it as (9.17)

P(t ′ A | A) = A -1/2 √ 2πt ′3 exp - A 2t ′ (1 -a γ t ′ ) 2 .
In the regime δ → 0, we have A → +∞, so the distribution (9.17) becomes localised at a γ t ′ = 1, thus t = A/a γ . This gives the typical scaling of the quantum area of balls in γ-Liouville quantum gravity, δ ≍ ε γaγ = ε 2-γ 2 /2 [START_REF] Hu | Thick points of the Gaussian free field[END_REF]. The large deviations from this typical value, associated with (9.17), will be the key in comparing the extreme nesting of CLE κ in the plane, as seen with the Euclidean (Lebesgue) measure, or with the Liouville quantum measure µ γ . 9.3. Nesting of CLE κ in Liouville quantum gravity. 9.3.1. Definition. One ingredient in the proof of (9.6) in Ref. [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF] is the following onepoint estimate [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF]Lemma 3.2]. For z ∈ D, define

N z (ε) := N z (ε) ln(1/ε) . Then (9.18) lim ε→0 ln P N z (ε) ∈ [ν -ω -(ε), ν + ω + (ε)] ln ε = γ κ (ν) for ν > 0,
for z ∈ D satisfying a ≤ CR(z, D) ≤ b, with 0 < a ≤ b, and for all ω ± (ε) decreasing to 0 sufficiently slowly. A similar result holds for ν = 0. We shall rewrite the above result, for ε → 0, in the more compact way, (9.19)

P N z ≈ ν ln(1/ε) ε ≍ ε γκ(ν) ,
where the sign ≈ stands for a scaling of the form (ν + o(1)) ln(1/ε). We also recall that the ≍ sign means an asymptotic equivalence of logarithms, i.e., a form ε γκ(ν)+o (1) on the r.h.s. Recalling definition (9.15), this is also for t → +∞, (9.20) P N z ≈ νt t ≍ e -γκ(ν)t . To define an analog of this nesting probability in LQG, instead of conditioning on the Euclidean radius ε -equivalently, on t -we condition on the quantum area δ (9.14) of the ball B(z, ε) -equivalently, on A (9.15). The number of loops N z surrounding the ball B(z, ε) stays the same. This conditional probability is then given by the convolution, (9.21)

P Q (N z | A) := ∞ 0 dt P(N z | t) P(t | A),
where P(t | A) is as in (9.16)-(9.17). We call it the quantum nesting probability.

Saddle point computation.

For large A, if we let N z scale as N z ≈ γpA, with p ∈ R + , we may also set N z ≈ νt, where ν is now defined as

(9.22) ν = ν(t) = γpA t ,
where p and A are considered as parameters. Note that expressions (9.20) and (9.17) for the two probability distributions appearing in the integrand in (9.21) are large deviations forms for t and A both large and in a finite ratio. Such is the case in (9.22), which yields (9.23)

P Q (N z ≈ γpA | A) ≍ ∞ 0 dt A √ 2πt 3 exp - (A -a γ t) 2 2t -γ κ (ν)t ,
where for A → +∞ the integral over t is consistently evaluated by a saddle point method.

We thus look for the extremum of (9.24)

E(t) := 1 2t (A -a γ t) 2 + γ κ (ν)t,
along trajectories at constant value of νt = γpA, and for fixed p and A. We then have

t ∂γ κ ∂t (ν) = -ν ∂γ κ ∂ν (ν),
and using (9.8), (9.25)

∂ ∂t γ κ (ν)t = γ κ (ν) -ν ∂γ κ ∂ν (ν) = λ.
This in turn gives (9.26)

∂E ∂t = λ - 1 2 A t 2 -a 2 γ ,
and a saddle point value t * of t at (9.27)

A t * := u = u(λ) := 2λ + a 2 γ .
which is implicitly a function of p. Note that from (9.8) again,

∂λ ∂t = -ν ∂ ∂ν γ κ (ν) -ν ∂γ κ ∂ν = ν 2 ∂ 2 γ κ ∂ν 2 > 0 so that ∂ 2 E ∂t 2 = ∂λ ∂t + A 2 t 3 > 0.
And the saddle point lies, as expected, at the minimum E * of E(t), (9.28)

E * := E(t * ) = A (u -a γ ) 2 2u + γ κ (ν) u ,
where, owing to definition (9.22) and to (9.27), ν is hereafter understood as the saddle point value,

(9.29) ν = ν(t * ) = γp A t * = γp u(λ).
Owing to (9.7)-(9.27) and (9.29), we have

(9.30) γ κ (ν) u = λ -νΛ κ (λ) u = u 2 -a 2 γ 2u -γpΛ κ (λ),
so that we finally get the simple form, (9.31)

E * A = u(λ) -a γ -γp Λ κ (λ).
Notice that (9.7), (9.27) and (9.29) also imply (9.32) We have just computed:

1 γp = u ν = u(λ) ∂Λ κ (λ) ∂λ = ∂Λ κ (λ) ∂u(λ) .
(9.33) Θ(p) = U -1 γ ( λ 2 ) -p Λ κ (λ)
, where λ is the function of p determined by (9.32), and where the inverse KPZ relation (9.13) precisely yields, (9.34)

U -1 γ λ 2 = u(λ) -a γ γ .
Note also that 1 p as in (9.32) is the derivative of Λ κ with respect to (9.34). Thus, setting λ ′ := U -1 γ ( λ 2 ), we get the Legendre-Fenchel transform equations:

(9.35) Θ(p) = λ ′ -p (Λ κ • 2U γ )(λ ′ ), 1 p = ∂(Λ κ • 2U γ )(λ ′ ) ∂λ ′ .
Comparing this result to the Legendre-Fenchel equations (9.7) in the Euclidean case, we get Theorem 9.2. In presence of γ-Liouville quantum gravity, the generating function Λ κ (9.3) is transformed into

(9.36) Λ Q κ := Λ κ • 2U γ
, where U γ is the KPZ function (9.12), with γ given by (9.11). The nesting distribution around a ball of given quantum area δ (9.23) is then given asymptotically for A = γ -1 ln(1/δ) → +∞, by

P Q N z ≈ γpA A ≍ e -γΘ(p)A = δ Θ(p) with Θ(p) = λ -pΛ Q κ (λ)
and λ is determined as a function of p by:

1 p = ∂Λ Q κ (λ) ∂λ .
Remark 9.3. The occurrence of a factor 2 in the composition law (9.36) is simply due to a different choice of scale when measuring large deviations, i.e., that of a quantum area δ in the quantum case, as opposed to that of a radius ε in the Euclidean one. This is seen in particular in the κ → 0 limit, where U γ simply becomes the identity function.

Remark 9.4. Theorem 9.2 shows that the KPZ relation, or its inverse as in (9.33), can directly act on an arbitrary continuum variable, here the conjugate variable in the cumulant generating function (9.3) for the CLE κ log-conformal radius. To our knowledge, this is the first occurrence of such a role for the KPZ relation, which usually concerns scaling dimensions.

Remark 9.5. The derivation above does not depend on the precise form of the large deviations function. Moreover, as shown in Refs. [START_REF] Duplantier | Duality and KPZ in Liouville quantum gravity[END_REF][START_REF] Duplantier | Liouville quantum gravity and KPZ[END_REF], the KPZ relation holds in full generality for any (fractal) random system in the plane and in Liouville quantum gravity, provided that the sampling of the random system is independent of that of the Gaussian free field defining LQG. Therefore, the map

Λ → Λ Q = Λ • 2U γ , from
Λ κ (λ) = ln cos π 1 -4 κ cos v , v = v(λ) := 2π √ κ √ κ 2 - 2 √ κ 2 + 2λ for λ ∈ (-∞, 1 -2 κ -3κ 32
), and to notice that (9.27) and (9.11) give

u(λ) = √ κ 2π v(λ).
Equations (9.32) and (9.33) then take the compact form, (9.38)

Θ(p) = Θ = c 2π (v -a ′ -p ′ Λ κ ), 1 p ′ = ∂Λ κ (v) ∂v ,
where we used the notations

c := √ κ γ , p := c 2π p ′ , a γ = 2 γ - γ 2 := √ κ 2π a ′ .
Because of (9.11), we find as parameters,

p ′ = cot v, Θ = c 2π v -(cot v) ln n 2 cos v -arccos(n/2) . One has p ′ ∈ R + for v ∈ [0, π 2 ), so that cos v = p ′ p ′2 + 1 ≥ 0, which finally yields (9.41) Θ(p) = c 2π J(p ′ ), J(p ′ ) := arccot(p ′ ) + p ′ ln 2 n p ′ 1 + p ′2 -arccos n 2 .
Note that the p = c 2π p ′ substitution above simply gives γpA = c 2π p ′ ln(1/δ). Theorem 9.2 then yields Theorem 9.6. The quantum nesting probability for CLE κ loops, with κ ∈ (8/3, 8) in a simply connected proper domain D ⊂ C, surrounding a ball centered at z with given quantum area δ, behaves as

P Q N z ≈ c 2π p ln(1/δ) δ ≍ δ c 2π J(p) , δ → 0,
where the large deviations function J is as in (9.41) and Theorem 2.2, and where c and n are given in (9.39) as functions of κ.

Remark 9.7. We see that this result perfectly matches the second large deviations result in Theorem 2.2 for nesting in the O(n) loop model on a random map with the topology of a pointed disk: one simply replaces 1 δ here with the large volume V of the map there. Indeed, one may assign elementary area 1 V to each face in the dual map, so that the dual map has in total unit area; then, the marked point corresponds in the dual to a face of elementary area 1 V , and its depth P = c 2π p ln V is the number of loops separating this face from the boundary of the disk.

It is interesting to compare the classical and quantum cases for nesting in CLE κ . In the classical case [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF], the parametric equations of the Legendre-Fenchel transform (9.7) are

ν = κ (2π) 2 v cot v γ κ (ν) = κ (2π) 2 v 2 2 -(v cot v) ln n 2 cos v - 1 2 (arccos(n/2)) 2
for v ∈ [0, π/2), and

ν = κ (2π) 2 w coth w γ κ (ν) = κ (2π) 2 - w 2 2 -(w coth w) ln n 2 cosh w - 1 2 (arccos(n/2)) 2
for v = iw with w ∈ R >0 . These parametric equations cannot be easily solved, whereas the quantum parametric equations (9.40), though similar, are simpler and explicitly solvable. Note also that in the classical case, the parameter λ is in the range λ ∈ (-∞, λ max ], with the values λ max = 1 -2 κ -3κ 32 corresponding to ν → 0 or equivalently v → π 2 , while λ → -∞ corresponds to ν → +∞ or v = iw with w → ∞. We observe more precisely that (9.42)

γ κ (ν) ∼ (2π) 2 κ ν 2 2 , ν → +∞.
In the quantum case (9.40), v is restricted to v ∈ [0, π 2 ), and λ spans a finite interval only, λ ∈ [λ min , λ max ], where λ min = 1 -2 κ -κ 8 is the point at which the square root in v(λ) vanishes, corresponding to p ′ → +∞. And this results in λ

′ = U -1 γ λ 2 spanning [ 1 2 -2 κ , 3 4 -2 κ ] if 8 3 < κ ≤ 4, and [ 1 2 -κ 8 , 1 2 -κ 16 ] if 4 ≤ κ < 8.
9.4. Sphere topology. Conformal loop ensembles can also be defined on the Riemann sphere C [START_REF] Kemppainen | The nested simple conformal loop ensembles in the Riemann sphere[END_REF][START_REF] Miller | The conformal loop ensemble nesting field[END_REF]. In particular, for any κ ∈ (8/3, 4], the law of the simple nested CLE κ in the full plane has been shown to be invariant under the inversion z → 1 z (and therefore under any Möbius transformation of the Riemann sphere) [START_REF] Kemppainen | The nested simple conformal loop ensembles in the Riemann sphere[END_REF]Theorem 1]. In this section, we connect the nesting statistics of CLE κ in C with the nesting statistics in the O(n) loop model on large random planar maps with the topology of the doubly punctured sphere.

We first discuss the properties of CLE κ ( C). Let us pick two points (punctures), z 1 , z 2 , on the sphere, which we may take to be (z 1 , z 2 ) = (0, ∞) using a suitable Möbius transformation. Consider the two balls B(z i , ε i ), i = 1, 2, centered at these points. In stereographic projection, the connected domain C \ (B(z 1 , ε 1 ) ∪ B(z 2 , ε 2 )) corresponds to the annulus

A(ε -1 2 , ε 1 ) := ε -1 2 D \ B(z 1 , ε 1
). Consider then in the whole CLE κ ( C) on the Riemann sphere, the loops which can be contracted to each one of the two punctures on Ĉ, i.e., those loops which in projection belong to the above annulus. By scale invariance, their number can depend only the product ε 1 ε 2 , and we write it as N (ε 1 ε 2 ). The nesting probability on the Riemann sphere is then defined as,

P C N (ε 1 ε 2 ) ≈ ν ln(1/ε 1 ε 2 ) | ε 1 , ε 2 ,
where we recall that ≈ is a short-hand notation for the event

N (ε 1 ε 2 ) ln(1/ε 1 ε 2 ) ∈ [ν -ω -, ν + ω + ]
for ω ± = ω ± (ε 1 ε 2 ) decreasing to 0 sufficiently slowly with the ε i 's (see Equation (9.18)). 9.4.1. Approximation to full-plane CLE and nesting estimates. Following Ref.

[119, Appendix A], about the rapid convergence of CLE on a large disk to full-plane CLE, we can take as a large disk, (εε 2 ) -1 D, with 0 < ε < 1, which contains the annulus A(ε -1 2 , ε 1 ) above. Using scale invariance, we may simply consider events in D and in the annulus A(ε, εε 1 ε 2 ) (see Figure 11), and by choosing ε small enough, approximate to any desired precision the probability of any event concerning a ball of radius ε in the ensemble CLE κ ( C) (with probability law denoted by P C ) by the probability of the same event in the ensemble CLE κ on the unit disk (with probability law simply denoted by P). Ref. [START_REF] Miller | The conformal loop ensemble nesting field[END_REF]Theorem A1] indeed states that with probability exponentially close to 1 in ln(1/ε) there exists a conformal map from whole-plane CLE κ ( C), restricted to the interior of its smallest loop containing B(0, ε), to CLE κ (D) similarly restricted to its smallest loop containing B(0, ε), and whose distorsion is exponentially close to 1.

As before, let N 0 (ε) be the number of loops surrounding the ball B(0, ε) in D, and let N ∩ (ε) be the number of loops surrounding the origin and intersecting ∂B(0, ε). We seek for an estimation of the law of the number of loops in the annulus B(0, ε) \ B(0, ερ),

(9.43) N (ερ) := N 0 (ερ) -N 0 (ε) -N ∩ (ε), ρ := ε 1 ε 2 ,
as illustrated in Figure 11. From Ref. [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF]Corollary 3.5], we know that N ∩ (ε) < c 0 ln(1/ε) for some constant c 0 > 0, except with probability exponentially small in ln(1/ε), since it is stochastically dominated by twice a geometric random variable with parameter p(κ) > 0 which depends only on κ.

From Ref. [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF]Lemma 3.2], and the convexity of γ κ (ν), we know that there exists η(ε) → 0, such that, (9.44)

P N 0 (ε) > ν ln(1/ε) ≤ ε γκ(ν)-η(ε) , ερ ε 1 Figure 11.
The whole set of loops in the unit disk D is counted by N 0 (ερ), with ρ = ε 1 ε 2 . The set of loops contained in the inner annulus, as counted by N (ερ) (resp. the set of intersecting loops, as counted by N ∩ (ε)) appears in red (resp. blue).

uniformly in ν ≥ ν 0 , with ν 0 fixed but strictly larger than the point at which γ κ (ν) reaches its minimum 0. We thus have in particular, (9.45)

P N 0 (ε) ≤ ν 0 ln(1/ε) ≥ 1 2 ,
for ε small enough. Besides, we also know from [120, Lemma 3.2] that there exists ω(ε), with ω(ε) → 0 as ε → 0, such that, (9.46) (ερ) γκ(ν)+η(ερ) ≤ P N 0 (ερ)ν ln(ερ) -1 ≤ ω(ερ) ln(ερ) -1 ≤ (ερ) γκ(ν)-η(ερ) .

Using these estimates will allow us shortly to show the existence of functions ω ± and η of ε and ρ, with ω ± (ε, ρ), η(ε, ρ) → 0 when ρ → 0, such that,

(9.47) (ερ) γκ(ν)+η(ε,ρ) ≤ P N (ερ) ln(1/ερ) ∈ [ν -ω -, ν + ω + ] ≤ (ερ) γκ(ν)-η(ε,ρ) .
Proof. Let us denote by A ν (ε, ρ) the event of interest in (9.47), by A ν (ε) the event {N 0 (ε) ≤ ν ln(1/ε)}, and by Āν (ε) the latter's complement. Define also the logarithmic ratio,

r = r(ε, ρ) := ln(1/ε) ln(1/ερ) ; r(ε, ρ) → 0 as ρ → 0.
For a lower bound, we write

P A ν (ε, ρ) ≥ P A ν (ε, ρ) ∩ A ν 0 (ε) = P(A ν 0 (ε)) P A ν (ε, ρ) A ν 0 (ε) .
Choosing ν 0 as in (9.45), the first factor is bounded from below by 1 2 , and using the lower bound (9.46) for the second factor, we get the desired lower bound in (9.47), up to replacing ω(ερ) of (9.46) by ω ± (ε, ρ) := ω(ερ) ∓ (ν 0 + c 0 ) r(ε, ρ).

For the upper bound, we write (9.48)

P A ν (ε, ρ) ≤ P( A ν (ε, ρ) ∩ A ν 1 (ε) + P( Āν 1 (ε) ,
where, by using the estimate (9.44) for ν 1 large enough, P( Āν 1 (ε) ≤ ε γκ(ν 1 )-η(ε) . We will choose ν 1 = ν 1 (ε, ρ), such that ν 1 (ε, ρ) → ∞ when ρ → 0, as allowed by uniformity of (9.44). As γ κ (ν) grows quadratically in ν (see Equation (9.42)) the latter estimate can be bounded, for large enough ν 1 , as (9.49)

ε γκ(ν 1 )-η(ε) ≤ ε C ν 2 1 = (ερ) C ν 2 1 r(ε,ρ)
, for some constant C > 0. On the other hand, the first term in (9.48) can be estimated via the upper bound in (9.46) to yield an upper bound as in (9.47), provided that (9.50)

ν 1 (ε, ρ) r(ε, ρ) → 0, ρ → 0,
as this is the error term to be subtracted, together with c 0 r(ε, ρ), from ω(ερ) as the result of the restriction to event A ν 1 (ε). If we would like (9.49) to be negligible in front of the first term in (9.48), we would have to choose ν 1 in such a way that (9.51)

ν 2 1 (ε, ρ) r(ε, ρ) → ∞, ρ → 0.
To satisfy both (9.50) and (9.51), choose for instance, ν 1 (ε, ρ) = r(ε, ρ) -3/4 . Then, the second term in (9.48) is bounded by (ερ) Cr -1 2 , which, since r → 0 as ρ → 0, is negligible as compared to the first term of order (ερ) γκ(ν) . This completes the proof of (9.47). □ As explained above, the exponentially fast convergence in ln(1/ε) when ε → 0 (see [START_REF] Miller | The conformal loop ensemble nesting field[END_REF]Theorem A.1]), of the approximation of CLE κ ( C) by the restriction of CLE κ (D) to the ball B(0, ε), allows us to translate result (9.47), valid for ρ = ε 1 ε 2 → 0, into Theorem 9.8. The nesting probability in CLE κ ( C) between two balls of radius ε 1 and ε 2 and centered at two distinct punctures, has the large deviations form,

P C N (ε 1 ε 2 ) ≈ ν ln(1/ε 1 ε 2 ) ≍ (ε 1 ε 2 ) γκ(ν) , ν ≥ 0, ε 1 , ε 2 → 0,
where γ κ (ν) is the same large deviations function (9.5) as in the case of the disk topology, and where notations are as in (9.18)- (9.19).

Even though the sphere and disk large deviations involve the same function γ κ , the scalings involved actually differ by powers of 2. Indeed, if we take the two balls on the Riemann sphere to have same radius ε, and measure nesting in ln 1 ε units, we have from Theorem 9.8, Corollary 9.9. The nesting probability in CLE κ ( C) between two balls of same radius ε and centered at two distinct punctures, has the large deviations form,

P C N (ε) ≈ ν ln(1/ε) ≍ ε γκ(ν) , ν ≥ 0, ε → 0,
where γ κ (ν) is related to the disk large deviations function (9.5) by

γ κ (2ν) = 2γ κ (ν).
Using hereafter the variables t i := ln 1 ε i , i = 1, 2, we have, (9.52)

P C N (ε 1 ε 2 ) ≈ ν(t 1 + t 2 ) ≍ e -γκ(ν)(t 1 +t 2 ) , t 1 , t 2 → +∞.
9.4.2. Nesting on the quantum sphere. In Liouville quantum gravity, following the same steps as in Section 9.3, let us condition on each ball having the same quantum area δ = e -γA . The desired distribution should be given by the convolution (9.53)

P C Q (N | A) := ∞ 0 ∞ 0 dt 1 dt 2 P C (N | t 1 , t 2 ) P(t 1 | A) P(t 2 | A),
where P(t i | A), i = 1, 2 are as in (9.16)-(9.17). Note that this definition readily asserts a factorisation, hence independence, of these two distributions, because their two ball centers (z i , i = 1, 2) have been taken as (0, ∞) on the Riemann sphere.

For large A, we let N scale as N ≈ γpA, with p ∈ R + , and also set N ≈ ν(t 1 + t 2 ), where ν is now defined such that, (9.54)

ν = ν(t 1 , t 2 ) := γpA/(t 1 + t 2 ),
where p and A are thought of as parameters. By the same argument as in Section 9.3.2, the asymptotic result (9.52) then yields when A → +∞

P C Q (N z ≈ γpA | A) ≍ ∞ 0 ∞ 0 A 2 dt 1 dt 2 2π t 3 1 t 3 2 exp [-E(t 1 ) -E(t 2 )] E(t 1 ) + E(t 2 ) = 1 2t 1 (A -a γ t 1 ) 2 + 1 2t 2 (A -a γ t 2 ) 2 + γ κ (ν)(t 1 + t 2 ). (9.55)
The above integral is evaluated by a saddle point method, by looking for the minimum of E(t 1 ) + E(t 2 ) at fixed ν(t 1 + t 2 ) = γpA. We then have for each i = 1, 2,

(t 1 + t 2 )∂ t i γ κ (ν) = -ν ∂γ κ ∂ν ,
and using (9.8),

∂ ∂t i (t 1 + t 2 )γ κ (ν) = γ κ (ν) -ν ∂γ κ ∂ν = λ.
This in turn gives for each i = 1, 2,

∂ ∂t i E(t 1 ) + E(t 2 ) = λ - 1 2 A t i 2 -a 2 γ ,
so that both saddle points t * 1 and t * 2 for t 1 and t 2 are located at the same point t * as in (9.27) in the case of the disk topology. We thus have at this double saddle point

2νt * = γpA E(t * 1 ) + E(t * 2 ) = 2E(t * ). Setting: Θ(p) := 2E(t * ) γA we deduce
Theorem 9.10. The large deviations function Θ(p) which governs the quantum nesting probability of CLE κ on C, p) , δ → 0, is related to the large deviations function Θ(p) for the disk topology (Theorem 9.2) by

P C Q (N ≈ p ln(1/δ) | δ) ≍ δ Θ(
Θ(2p) = 2Θ(p).
Using alternatively the explicit formulation, as in Theorem 9.6, we get Corollary 9.11. In the same setting as in Theorem 9.10,

P C Q N ≈ cp π ln(1/δ) δ ≍ δ c π J(p) , δ → 0,
where J(p) is as in (9.41).

This is in complete agreement with:

• The first result in Theorem 2.2, which describes the large deviations of the number of separating loops between a marked point and a microscopic boundary in a critical O(n) model on a random map with a disk topology; • The first result in Theorem 7.1, which describes the large deviations of the number of separating loops between two microscopic boundaries in a critical O(n) model on a random map with a cylinder topology. These are indeed the sort of topologies considered in Section 9.4.1 above. 9.5. Weighted loops. 9.5.1. Weighting CLE κ . Our argument can be refined to include a model where loops receive independent random weights, in parallel to the results in Ref. [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF]Section 5]. A motivation to introduce this model, beyond the fact it offers a natural generalisation of the counting of loops, is that loops weighted with a Bernoulli random variable for κ = 4 are related to the extremes of the GFF [START_REF] Hu | Thick points of the Gaussian free field[END_REF].

Conditionally on a configuration Γ of a CLE κ in a proper simply connected domain D, let (ξ l ) l∈Γ be a collection of independent, identically distributed real random variables indexed by Γ. We denote by µ the law of each ξ l . For z ∈ D and ε > 0, let Γ z (ε) be the set of loops which surround B(z, ε), and define

Ξ z (ε) = l∈Γz(ε) ξ l , Ξ z (ε) = Ξ z (ε) ln(1/ε) .
For a realisation of the CLE κ and of the (ξ l ) l , and any fixed

(ν, α) ∈ R + × R, let Φ µ ν,α = z ∈ D : lim ε→0 N z (ε) = ν and lim ε→0 Ξ z (ε) = α .
The cumulant generating function associated with the moments of µ is

(9.56) Λ µ (λ) := ln E e λξ ,
where ξ is a random variable whose distribution is µ. Its symmetric Legendre-Fenchel transform, Λ ⋆ µ : R → R + , is defined as (9.57)

Λ ⋆ µ (x) := sup λ∈R (λx -Λ µ (λ)) .
The Hausdorff dimension of the set Φ µ ν,α is then almost surely constant, with value found in [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF]Theorem 5.1] dim H Φ µ ν,α = max{0, 2γ κ (ν, α)}, as long as γ κ (α, ν) ≤ 2, with Φ µ α,ν = ∅ otherwise, and with the definition

(9.58) γ κ (ν, α) :=    νΛ ⋆ µ (α/ν) + νΛ ⋆ κ (1/ν) if ν > 0 lim ν ′ →0 + γ κ (ν ′ , α) if ν = 0 and α ̸ = 0 lim ν ′ →0 + γ κ (ν ′ ) = 1 -2 κ -3κ 32 if (ν, α) = (0, 0),
where the limits exist by convexity of Λ ⋆ κ and Λ ⋆ µ . When ν ̸ = 0, we thus have

γ κ (ν, α) = γ κ (ν) + γ µ (ν, α), γ µ (ν, α) := νΛ ⋆ µ (α/ν) = λ ′ α -νΛ µ (λ ′ )
, where λ ′ is a function of (ν, α) determined by:

α ν = ∂Λ µ (λ ′ ) ∂λ ′ .
By homogeneity, we find the useful identity

(9.59) ν ∂ ∂ν + α ∂ ∂α γ µ (ν, α) = γ µ (ν, α).
Uniformly for a point z ∈ D, we have the following joint probability scaling [START_REF] Miller | Extreme nesting in the conformal loop ensemble[END_REF] (9.60) P(N z ≈ νt and Ξ z ≈ αt | t) ≍ e -γκ(ν,α)t . 9.5.2. Weighted CLE κ in Liouville Quantum Gravity. One follows exactly the same procedure as in Section 9.3. We study the nesting around small balls B(z, ε) conditionally to a given quantum area δ (9.14), hence conditionally on A (9.15), while the counts N z and Ξ z are unchanged, (9.61)

P Q (N z , Ξ z | A) := ∞ 0 dt P(N z , Ξ z | t) P(t | A),
where P(t | A) is as in (9.16)-(9.17).

For large A, we let N z ≈ γpA and Ξ z ≈ γqA, with (p, q) ∈ R + × R, and also have N z ≈ νt, Ξ z ≈ αt, where ν and α are defined by: (9.62) γpA = νt, γqA = αt, and p, q, A are considered as parameters. As in Section 9.3.2, the asymptotic result (9.60) then yields, for A → +∞,

P Q (N z ≈ γpA and Ξ z ≈ γqA | A) ≍ ∞ 0 Ae -Ew(t) dt √ 2πt 3 , E w (t) := 1 2t (A -a γ t) 2 + γ κ (ν, α)t. (9.63)
The above integral is evaluated by the saddle point method, looking for the minimum of E w (t) along trajectories at constant values of νt and αt according to (9.62). We then have

t ∂ ∂t γ µ (ν, α) = -ν ∂ ∂ν + α ∂ ∂α γ µ (ν, α),
and using (9.59),

∂ ∂t t γ µ (ν, α) = 0, so that, ∂ ∂t t γ κ (ν, α) = ∂ ∂t t γ κ (ν) = λ,
as in (9.25). This shows that ∂Ew ∂t is the same as in (9.26),

∂E w ∂t = λ - 1 2 A t 2 -a 2
γ , with the same saddle point as in (9.27),

A t * = u = u(λ) := 2λ + a 2 γ . The saddle point value resides at the minimum E * w of E w (t), (9.64)
E * w := E w (t * ) = A (u -a γ ) 2 2u + γ κ (ν, α) u ,
where, because of condition (9.62), ν and α are now functions of (p, q) determined by

(9.65) ν = γp A t * = γp u(λ), α = γq A t * = γq u(λ). It yields γ µ (ν, α) u = αλ ′ -νΛ µ (λ ′ ) u = γqλ ′ -γpΛ µ (λ ′ ), with α ν = q p = ∂Λ µ (λ ′ ) ∂λ ′ .
Recalling (9.30) and (9.31), we get the simple form,

Θ(p, q) := E * w γA = u(λ) -a γ γ + qλ ′ -p Λ κ (λ) + Λ µ (λ ′ ) .
Comparing to (9.33)-(9.34), we get Theorem 9.12. The joint distribution of the number of loops N z surrounding a ball of given quantum area δ centered at z in a simply connected domain D ⊂ C, and of the sum of weights Ξ z on these loops in the ensemble of µ-weighted loops in a CLE κ , satisfies the large deviations estimate,

P Q (N z ≈ p ln(1/δ) and Ξ z ≈ q ln(1/δ) | δ) ≍ δ Θ(p,q) , δ → 0, with Θ(p, q) = Θ(p) + qλ ′ -pΛ µ (λ ′ )
, where Θ(p) is as in Theorem 9.2, and where the conjugate variable λ ′ is the function of (p, q) uniquely determined by (9.66)

q p = ∂Λ µ (λ ′ ) ∂λ ′ .
We can also switch to parameters (p ′ , q ′ ) such that (9.67)

p = c 2π p ′ , q = c 2π q ′ ,
where c is the exponent defined in (9.39). Then, after writing Θ(p, q) = c 2π J(p ′ , q ′ ), we get Corollary 9.13. In the same setting as in Theorem 9.12, we have

P Q N z ≈ c 2π p ln(1/δ) and Ξ z ≈ c 2π q ln(1/δ) δ ≍ δ c 2π J(p,q) , δ → 0,
with the bivariate large deviations function

J(p, q) = J(p) + qλ ′ -pΛ µ (λ ′ ),
where J(p) is given by (9.41) and where λ ′ is uniquely determined as a function of (p, q) by q p = ∂Λ µ (λ ′ ) ∂λ ′ .

Corollary 9.13 in LQG matches with the bivariate large deviations of nesting and sum of loop weights for critical O(n) models on random maps with the topology of a pointed disk (first result of Theorem 8.1). The case of the bivariate distribution on the Riemann sphere can be analysed in exactly the same way as in Section 9.4, and we skip the details here.

Theorem 9.14. On the Riemann sphere C, the joint distribution of the nesting between two balls of given quantum area δ and the weight carried by the separating loops, behaves as

P C Q (N ≈ p ln(1/δ) and Ξ ≈ q ln(1/δ) | δ) ≍ δ Θ(p,q) , δ → 0,
where the large deviations function Θ(p, q) is given in terms of the large deviations function Θ(p, q) for the quantum disk, as obtained in Theorem 9.12, by

Θ(p, q) = 2 Θ p 2 , q 2
. Switching to variables (9.67), we get Corollary 9.15. In the same setting as in Theorem 9.14, we have

P C Q N ≈ cp π ln(1/δ) and Ξ ≈ cq π ln(1/δ) δ ≍ δ c π J(p,q) , δ → 0,
where J(p, q) is the function as defined in Corollary 9.13.

This last result is the exact analog, in Liouville quantum gravity, of the first large deviations result of Theorem 8.1 in the critical O(n) model on random disks with µweighted loops, for the topology of a pointed disk with a microscopic boundary. real axis from ς(γ + ) to γ + , v moves from 0 to a purely imaginary value denoted τ = iT . Then, the function v → x(v) has the properties:

x(v + 2τ ) = x(v + 1) = x(-v) = x(v), ς(x(v)) = x(v -τ ),
and is depicted in Figure 8. x ′ (v) has zeroes when v ∈ 1 2 Z + τ Z, and double poles at v = v ∞ + Z + 2τ Z. From (B.3), paying attention to the determination of the square root at infinity obtained by analytic continuation, we can read in particular:

(B.4) x ′ (v) ∼ iC (v -v ∞ ) 2 , v → v ∞ .
There is an alternative expression for (B.3) in terms of Jacobi functions:

(B.5) v = 2iC arcsn ς(γ -)-γ + ς(γ + )-γ + x-ς(γ + ) x-ς(γ -) ; m (ς(γ + ) -γ -)(ς(γ -) -γ + ) ,
This formula can be easily checked by differentiating both sides with respect to x and using

∂ v sn[v; m] = (1 -sn 2 [v; m])(1 -m sn 2 [v; m]).
Note that m is for us the square of the elliptic modulus usually denoted k. For (γ -, γ + ) ∈ A R , we have m ∈ (0, 1).

Recall the expression of the complete elliptic integral

K(m) = 1 0 dt (1 -t 2 )(1 -mt 2 ) = arcsn[1; m]. Matching x = γ + with v = iT we obtain (B.6) T = 2CK(m) (ς(γ + ) -γ -)(ς(γ -) -γ + ) . Matching x = ς(γ -) with v = 1 2 we obtain (B.7) C = (ς(γ + ) -γ -)(ς(γ -) -γ + ) 4K(1 -m) .
Together this implies

(B.8) T = K(m) 2K(1 -m)
.

Later, we will need the following expansion.

Lemma B.1. When v → v ∞ , we have the expansion:

(B.9) x(v) = -iC v -v ∞ + E 1 4 + i C 3E 2 1 -8E 2 48 (v -v ∞ ) + O(v -v ∞ ) 2
where we introduced the symmetric polynomials in the endpoints:

E 1 = γ -+ γ + + ς(γ + ) + ς(γ -), E 2 = γ -γ + + ς(γ + ) + ς(γ -) + γ + ς(γ + ) + ς(γ -) + ς(γ + )ς(γ -), (B.10)
More generally, the coefficient of (vv ∞ ) k in this expansion is a homogeneous symmetric polynomial of degree (k + 1) in the endpoints, with rational coefficients up to an overall factor (iC) -k .

Proof. This can be easily derived from the integral representation (B.3). □ B.2. Changes of parameters. It is often convenient to trade (γ -, γ + ) for another set of parameters. The first change of variables we will consider is χ :

(γ -, γ + ) → (m, p) with (B.11) p = ς(γ -) -γ - ς(γ + ) -γ - ,
and we assume here α ̸ = 1. The case α = 1 will be treated in Section B.5. χ is then an analytic map in the domain A which has degree 2. It admits an inverse map χ -1 : (m, p) → (γ -, γ + ) given by the formula

(B.12) γ -= α (α 2 -1)h - √ 1 -m (α 2 -1)(p -1)h , γ + = α (α 2 -1)h - p √ 1 -m (α 2 -1)(p -m)h .
This map χ -1 is analytic in the domain

A 1 := (m, p) ∈ C 2 | |m| < 1 and p ̸ = m ,
and in (B.12) we use the square root with its standard determination and branchcut on the negative real axis. We have chosen the sign in front of the square root so that the m = 0 specialisation of χ -1 gives (γ * -, γ * + ) where (B.13)

γ * + = 1 h(α + 1)
is the fixed point of the involution ς. Note that γ * -is still a function of p -see later (B.17) and (B.18).

When (γ -, γ + ) ∈ A R , we know that m ∈ (0, 1) and p > 0. We can rewrite (B.5) using (B.7) as

(B.14) v = i arcsn p m
x-ς(γ + )

x-ς(γ -) ; m 2K(1m) .

Specialising to x = ∞, we obtain

(B.15) v ∞ = i arcsn p m ; m 2K(1 -m)
.

Decomposing v ∞ = 1 2 + iT w ∞ with (B.8), we can rewrite using the transformation law of the Jacobi elliptic functions (B. [START_REF] Borot | Formal multidimensional integrals, stuffed maps, and topological recursion[END_REF])

√ p = √ m sn -iK(1 -m) + K(m)w ∞ ; m = 1 sn K(m)w ∞ ; m]
.

With χ -1 , we can see w ∞ as a function of (m, p) and we denote w * ∞ the specialisation of this function to m = 0. As K(m = 0) = π 2 and the Jacobi sn function degenerates to the sine function, we deduce (B.17)

p = 1 sin 2 πw * ∞ 2 . the composed map (B.24) (γ -, γ + ) χ -→(m, p) -→ (q 1 2 , w * ∞ ) is analytic in the domain U = A ∩ χ -1 (T ). Then, the composed map (B.25) (q 1 2 , w * ∞ ) -→ (m, p) χ -1
-→(γ -, γ + ) using (B.12) is an analytic function in the domain

(B.26) V := B(0; 1) × w * ∞ ∈ C Re w * ∞ ∈ (0, 2) and sin πw * ∞ 2 < 1 ,
where we imposed the last inequality to guarantee that m ̸ = p in this domain. This function is by construction an inverse to (γ -, γ + ) → (q 1 2 , w * ∞ ). Formula (B.20) comes from the expansion of (B.12) when m → 0, using (B.17), (B.21) and trigonometric identities. □ Remark B.4. From (B.22) we see that that the preimage of q ∈ (-1, 0] ∩ Q via the map m → q is m ∈ (-1, 0]. B.3. Allowing complex parameters in x(v). For (γ -, γ + ) ∈ A R we recall that m ∈ (0, 1) and p > 0, and we can use the reciprocal of (B.14) to parametrise the complex x plane:

(B.27) x(v) = ς(γ + ) -ς(γ -) m p sn 2 [2iK(1 -m)v ; m] 1 -m p sn 2 [2iK(1 -m)v ; m]
.

As sn[•; m] is an analytic family of meromorphic functions indexed by m ∈ B(0; 1), we may continue (B.27) analytically to complex values of γ -, γ + . In view of Lemma B.3, we can considering x(v) as an analytic family of meromorphic function of v, parametrised by (q [START_REF] Aru | Two perspectives of the 2d unit area quantum sphere and their equivalence[END_REF]. Properties of x(v) when q → 0. Let us insert (B.12) of γ ± in terms of (m, p) in the formula (B.7) for C to get

1 2 , w * ∞ ) ∈ V. B.
C 2 = p 2 -2p + m 4h(1 -α 2 )K(1 -m) 2 1 p(p -1)(1 -m)(p -m)
.

In view of Lemma B.3, the right-hand side is an analytic function of (q

1 2 , w * ∞ ) ∈ V.
We notice indeed that by definition of the domains, (γ -, γ + ) only take finite values, so C 2 has no singularities in V. We now want to identify the sign of the square root to get C itself. Up to restricting V to a domain

V ′ (η) := (q 1 2 , w * ∞ ) ∈ V Re( 1 p ) ∈ (η, 1)
where η ∈ (0, 1) is fixed, and as we have |p| > 1 due to the last condition in (B.26), we get Re(pm) ≥ Re( 1 p )η ′ > 0. for some η ′ > 0 depending on η. When (γ -, γ + ) ∈ A R , we know that C > 0 and taking into account Remark B.2 it follows that p > 2 and therefore

(B.28) C = p(p -2) + m 4h(1 -α 2 )K(1 -m) 1 p(p -1)(1 -m)(p -m) is the analytic continuation of C to (q 1 2 , w * ∞ ) ∈ V ′ (η). Lemma B.5. Let η ∈ (0, 1). In view of Lemma B.3, w ∞ , πC
T and E 1 , E 2 can be considered as an analytic function of (q 1 2 , w * ∞ ) ∈ V ′ (η), and when q → 0

w ∞ = w * ∞ - 4 sin(πw * ∞ ) π q 1 2 + 6 sin(2πw * ∞ ) π q + O(q 3
2 ),

πC T = 2 cot(πw * ∞ ) h(1 -α 2 ) + 8 sin(πw * ∞ ) h(1 -α 2 ) q 1 2 + 8 cos(πw * ∞ ) 2 cos 2 (πw * ∞ ) + 1 h(1 -α 2 ) sin 2 (πw * ∞ ) q + O(q 3
2 ),

E 1 = 4 1 -α sin 2 (πw * ∞ ) h(1 -α 2 ) sin 2 (πw * ∞ ) + 32 cos(πw * ∞ ) h(1 -α 2 ) sin 2 (πw * ∞ ) q 1 2 + 64 -cos 4 (πw * ∞ ) + 2 cos 2 (πw * ∞ ) + 1 h(1 -α 2 ) sin 2 (πw * ∞ ) q + O(q 3
2 ),

E 2 = 2 3(1 -α) 2 + (1 -3α 2 ) cos 2 (πw * ∞ ) h 2 (1 -α 2 ) 2 sin 2 (πw * ∞ ) + 32(2 -3α) cos(πw * ∞ ) h 2 (1 -α 2 ) 2 sin 2 (πw * ∞ ) + 64 (3α + 2) cos 4 (πw * ∞ ) + (2 -3α)(2 cos 2 (πw * ∞ ) + 1) h 2 (1 -α 2 ) 2 sin 2 (πw * ∞ ) q + O(q 3 2 ), (B.29)
Proof. Combining (B. [START_REF] Borot | Formal multidimensional integrals, stuffed maps, and topological recursion[END_REF]) and (B.17) we have

(B.30) w * ∞ = 2 π arcsin sn K(m)w ∞ ; m .
Using the three first terms of the Fourier expansion

sn[K(m)w ; m] = 2π √ m K(m) ℓ≥0 q ℓ 2 + 1 4 1 -q ℓ+ 1 2 sin (ℓ + 1 2 )πw (B.31)
and solving for w ∞ in terms of (q 1 2 , w * ∞ ) in the limit q → 0, we find the desired expansion. By combining (B.28) and (B.8), we have

πC T = π 2K(m) p(p -2) + m h(1 -α 2 ) 1 p(p -1)(1 -m)(p -m) . Using (B.32) K(m) = π 2 1 + m 4 + 9m 2 64 + O(m 3 )
and (B.22), we obtain the desired expansion of πC T . The expansion at q → 0 of the E i comes from (B.20), the expression of ς and elementary identities between trigonometric functions. □

We shall need the asymptotic behavior of x(v) near the vertical lines Im v = 0 and 1 2 }, and η ∈ (0, 1). We have when q → 0 and w * ∞ such that B(0;

Im v = 1 2 . Lemma B.6. Let v = ε + τ w for ε ∈ {0,
1) × {w * ∞ } ⊂ V ′ (η) (B.33) x(v) -γ + = q 1 2 -ε x * ε (w) + O(q 1
2 ) .

The limit functions are:

x * 0 (w) = 16 cos(πw * ∞ ) h(1 -α 2 ) cos 2 πw 2 , x * 1 2 (w) = 2 cos(πw * ∞ ) h(1 -α 2 ) 1 cos(πw) -cos(πw * ∞ )
, where cos(πw * ∞ ) was given in (B.18) and γ * + in (B.13). For ε = 0, the error in (B. [START_REF] Cardy | [END_REF]) is uniform for w in any compact. For ε = 1 2 , the error is uniform for w in any compact of C \ (w * ∞ + Z). In both cases, the error is stable under differentiation with respect to v. Proof. Our starting point is the formula (B.27) for x(v). where the error term is uniform when w belongs to any fixed compact and we have used (B.32) to obtain the second line. Together with the expansion of (γ -, γ + ) from Lemma B.3 and the formula p = sin -2 ( πw * ∞ 2 ), we deduce from (B.27) after some elementary algebra

x(τ w) = 16 cos(πw * ∞ ) h(1 -α 2 ) cos 2 πw * ∞ 2 q 1 2 + O(q).
For x = 1 2 + τ w = 1 2 + iT w, we rather need

sn 2iK(1 -m) • ( 1 2 + iT w ; m = - 1 √ m sn[K(m)w ; m] ,
which comes from the identity already used in (B. [START_REF] Borot | Formal multidimensional integrals, stuffed maps, and topological recursion[END_REF]. Inserting this in (B.27) and using again (B.34), we obtain

x 1 2 + τ w = 2 cos(πw * ∞ ) h(1 -α 2 ) 1 cos(πw) -cos(πw * ∞ ) + O(q 1
2 ). Lemma B.7. The map (γ -, γ + ) → (q 1 2 , ρ) is analytic in the domain

U 1 = A ∩ χ -1 1 (B(0; 1) × C)
On its image V 1 ⊂ B(0; 1) × C, it admits an analytic inverse map (q 1 2 , ρ) → (γ -, γ + ). Besides, we have when q → 0 2h(γ * +γ + ) = 4ρq

1 2 + O(q 3
2 ).

where the error is uniform when ρ is bounded.

Proof. The map χ 1 admits an inverse χ -1 1 given by

(B.35) γ -= 1 -ρ 2h , γ + = ρ + 1 2h - ρ hm 1 - √ 1 -m .
The map χ 1 is analytic in the domain A, while the inverse χ -1 1 is extends to an analytic function on (m, ρ) ∈ B(0; 1) × C. We get the conclusion by further using the change of variable m → q 1 2 already discussed in the proof of Lemma B.3. □

We then observe that p defined by (B.11) is equal to

(B.36) p = m 1 - √ 1 -m .
The discussion of Appendix B.3 can be specialised using this expression: it shows that x(v) becomes an analytic family of meromorphic functions of v, parametrised by (q

1 2 , ρ) ∈ V 1 .
We have the following analog of Lemma B.5.

Lemma B.8. In view of Lemma B.7, πC

T and E 1 , E 2 can be seen as analytic functions of (q

1 2 , ρ) ∈ V 1 . The function E 1 is constant E 1 = 2 h ,
We also have the expansion when q → 0

πC T = ρ 2h - 2ρ h q + O(q 2 ), E 2 = 6 -ρ 2 4h 2 - 4ρ 2 h 2 q + O(q 2 ), (B.37) Proof. Inserting (B.35) in (B.6) we find πC T = πρ(1 - √ 1 -m) 2h mK(m)
.

Using (B.32) and (B.22) then implies the desired expansion when q → 0. Note that

E 1 = γ -+ γ + + 1 h -γ -+ 1 h -γ + = 2 h .
The q → 0 expansions of E The analog of Lemma B.6 for the expansion of x(v) itself is Lemma B.9. Let v = ε + τ w for ε ∈ {0,1 2 }. We have for (q 12 , ρ) ∈ V 1 , when q → 0 and uniformly for ρ bounded

(B.38) x(v) = q 1 2 -ε x * ε (w) + O(q 1 2 ) ,
where the limit functions are

x * 0 (w) = 4ρ h cos πw 2 , x * 1 2
(w) = ρ 2h cos(πw) .

(B.39)

If ε = 0, the error in (B. [START_REF] Cori | Planar maps are well-labeled trees[END_REF]) is uniform for w in any compact. If ε = 1 2 , the error is uniform for w in any compact of C \ ( 1 2 + Z). In both cases, the error is stable under differentiation with respect to v.

Proof. The starting point is the expression (B.27) for x(v) with p replaced by (B.36) and using the change of variables (B.35). The proof then becomes similar to that of Lemma B.6 and is omitted. □ Some of these results can be retrieved from those with α ̸ = 1 by taking the limit α → 1 and w * ∞ in such a way that

(B.40) 1 2 -w * ∞ ∼ 1 -α 2π ρ.
This asymptotic relation is compatible with identifying ρ with 1 -2hγ * -and using (B.18). However, as the change of variable (γ -, γ + ) → (q Corollary C.1. Assume α ̸ = 1. For i = 0, 1, 2, 3, (q 1 2 , w * ∞ ) → g i is an analytic function in the domain V ′ (η) for η small enough. We have the following expansions when q → 0:

g 2 = 2 4 -n 2 1 + 2g h(1 -α 2 ) α - 1 sin 2 (πw * ∞ ) - 32g h(1 -α 2 )(4 -n 2 ) cos(πw * ∞ ) sin 2 (πw * ∞ ) q 1 2 + O(q), g 1 = 2 h(4 -n 2 )(1 -α 2 ) g h(1 -α 2 ) (1 + 3α 2 ) - 2(2 + 3α) sin 2 (πw * ∞ ) + 6 sin 4 (πw * ∞ ) + α - 1 sin 2 (πw * ∞ ) + 16 cos(πw * ∞ ) h(4 -n 2 )(1 -α 2 ) sin 2 (πw * ∞ ) 2g 3h (2 + 3α) cos 2 (πw * ∞ ) + 4 -3α (1 -α 2 ) sin 2 (πw * ∞ ) -1 q 1 2 + O(q).

□

We denote g * i the value of this function g i at q = 0. There are some simplifications for α = 1. Owing to the exact relation E 1 = 2 h , only g 1 has a non trivial dependence in q.

Corollary C.2. Assume α = 1. For i = 0, 1, 2, 3, (q 1 2 , ρ) → g i is an analytic function in the domain V 1 (η) for η small enough, We have

g 2 = 2 4 -n 2 1 - g h ,
and when q → 0

g 1 = 1 h(4 -n 2 ) -1 + g 12h (ρ 2 + 6) + 4gρ 2 3h 2 (4 -n 2 ) q + O(q 2 ). □ Appendix D. The special function Υ b (v) Υ b (v)
is the unique meromorphic function with a simple pole at v = 0 with residue 1, and the pseudo-periodicity properties:

Υ b (v + 1) = Υ b (v), Υ b (v + τ ) = e iπb Υ b (v).
We have several expressions:

Υ b (v) = m∈Z e -iπbm π cot π(v + mτ ) = ϑ ′ 1 (0|τ ) ϑ 1 -b 2 τ ϑ 1 v -b 2 τ ϑ 1 (v|τ ) = e iπbv τ iT ϑ ′ 1 0 -1 τ ϑ 1 -b 2τ -1 τ ϑ 1 v-b/2 τ -1 τ ϑ 1 v τ | -1 τ . (D.1)
Curiously, this function also appears in the dynamical R-matrix of the elliptic Calogero system [START_REF] Babelon | Introduction to classical integrable systems[END_REF].

Remark D.1. Due to the presence of -1 τ in the argument of ϑ 1 , Υ b (v) is a family of meromorphic functions of v ∈ C, only in the domain q T (1-q b ) , the prefactor of u in the left-hand side becomes in the q → 0 limit

-2 2 + n Υ b 1 2 + τ (w ∞ + 1) + Υ b 1 2 + τ (w ∞ -1) -Υ b 1 2 + τ (w ∞ -1) -Υ b 1 2 -τ (1 + w ∞ ) = - 8i sin(πb) 2 + n cos(πbw * ∞ ) + o(1)
.

(E.2)
As we assumed b ∈ (0, 1 2 ) and in the definition of the domain, restricting to the range of w * ∞ to Re w * ∞ ∈ (η, 1), i.e. restricting (q 1 2 , w * ∞ ) further to the domain V ′′ (η) shows that the leading term in Equation (E.2) does not vanish in a neighborhood of q = 0 in this domain. Therefore, Equation (E.1) allows expressing u as an analytic function of (q 1 2 , w * ∞ ) ∈ V ′′ (η). For α = 1, the argument is similar but it is not necessary to restrict further the range of the extra variable ρ because (E.2) becomes -8i sin(πb) cos(πb/2) 2+n ̸ = 0 under the assumption b ∈ (0, 1 2 ), so we can use the domain V ′′ 1 . □

In the non generic critical regime, we have γ + → γ * + = 1 h(α+1) , thus q → 0 in terms of the parametrisation of Lemma B.3 or Lemma B.7. Inserting the asymptotic expansions from Corollary D.2 yields:

3 k=0 g k k! πC T k Y (k) b,0 (πw ∞ ) -q 1-b Y (k) b-2,0 (πw ∞ ) + q Y (k) b-2,0 (πw ∞ ) + Y (k) b+2,0 (πw ∞ ) + O(q 1+b ) = 0, 3 k=0 g k k! πC T k Y (k) b, 1 2 (πw ∞ ) -q b Y (k) b+2, 1 2 (πw ∞ ) + O(q 2-b ) = 0. (E.3)
with coefficients:

Y b,0 (w) = cos(bw), Y b, 1 2 (w) = sin[(1 -b)w] sin w .
E.1. The non generic critical line. At a non generic critical point, we must have u = 1 and q = 0, thus:

- 2 2 + n + 3 k=1 g * k k! 2 cot(πw * ∞ ) (1 -α 2 )h k Y (k) b,ε (πw * ∞ ) Y b,ε (πw * ∞ ) = 0 ε ∈ {0, 1 2 }.
where we have used the expression for πC T at q = 0 given in Lemma C.1 and we should insert the expression for g * k given in Lemma C.2. We note that the critical values g * k obtained in Section C are such that (E.3) give a linear system of equations for ( g h , h 2 ), parametrised by w * ∞ for α ̸ = 1, and by ρ if α = 1. These equations, as well as their explicit solution for α = 1, already appeared in [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF]Sections 4.1 and 4.2].

For α = 1, the solution is

g h = 4(ρb √ 2 + n - √ 2 -n) -ρ 2 (1 -b 2 ) √ 2 -n + 4ρb √ 2 + n -2 √ 2 -n , h 2 = ρ 2 b 24 √ 4 -n 2 ρ 2 b(1 -b 2 ) √ 2 + n -4(1 -b 2 )ρ √ 2 -n + 6b √ 2 + n -ρ 2 (1 -b 2 ) √ 2 -n + 4ρb √ 2 + n -2 √ 2 -n , (E.4)
as claimed in Theorem 6.1 and in agreement with [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF]Equation 4.15]. Since g h and h 2 must be non negative, we must have ρ ∈ [ρ ′ min , ρ max ], with:

ρ ′ min = 2 √ 1 -b 2 √ 2 -n - √ 2 (10 + n)b 2 -4 + 2n b √ 1 -b 2 √ 2 -n , ρ max = 1 b 2 -n 2 + n . (E.5)
However, we will see later that the non generic critical line only exists until some value ρ min > ρ ′ min , so (E.5) will become irrelevant. In the general case α ̸ = 1, the expression is more complicated.

g h = 6(1 -α 2 ) sin 2 (πw * ∞ ) 1 k=0 b k Pk (πw * ∞ ) 2 k=0 b k P k (πw * ∞ ) , h 2 = 2b cos 2 (πw * ∞ ) (1 -α 2 ) 2 (2 -n) sin 4 (πw * ∞ ) 3 k=0 b k Qk (πw * ∞ ) 2 k=0 b k P k (πw * ∞ )
, (E.6) with:

P1 (w) = sin(2w) 3 -2 sin 2 (bw) -α sin 2 (w) , P0 (
Q0 (w) = 2 sin(2w) (1 -4α -3α 2 ) cos 4 (w) + 2(3α 2 -2α -1) cos 2 (w) -3α 2 + 8α -5 , Q 3 (w) = -sin 2 (2w), Q 2 (w) = 3 sin 2 (2w) sin(2bw), Q 1 (w) = 2 sin(2w) (3α 2 + 1) cos 4 (w) + 2 6(α + 1) cos 2 (bw) -3α 2 + 3α + 1 cos 2 (w), + 12(1 -α) cos 2 (bw) + 3(1 -α) 2 , Q 0 (w) = -3 sin(2bw) (α + 1)(α + 3) cos 4 (w) + 2(-α 2 -α + 3) cos 2 (w) + (1 -α) 2 .
We have checked that, in the limit α → 1 such that ( 1 2w * ∞ ) ∼ 1-α 2 ρ, these expressions retrieve (E.4). This completes the proof of Theorem 6.1. E.2. Near criticality. Let us fix (g, h) on the non generic critical line for u = 1. We now study the behavior when u ̸ = 1 but u → 1 of the endpoints γ ± . In view of the change of variables in Lemma B.3 for α ̸ = 1 (Lemma B.7 for α = 1), it amounts to determining the dependence of u in the variable q while the second parameter w * ∞ (resp. ρ) is specified by the position of (g, h) on the non generic critical line via Equation E.6 (resp. Equation E.4).

For this purpose, we look at (E.3), and note that u only appears in g 0 . There could be a term of order q 12 stemming from near-criticality corrections to w ∞ , g k and πC

T , but the computation reveals that it is absent. Therefore, we obtain:

(E.7) 1 -u = n + 2 2 3 k=0 g * k k! 2 cot(πw * ∞ ) (1 -α 2 )h k Y (k) b-2,0 (πw * ∞ ) Y b,0 (πw * ∞ ) q 1-b + O(q),
where g * 0 = -2 2+n and ( g * k ) k≥1 should be replaced by their values in terms of (g, h, w * ∞ ) from Corollary C.1 or Corollary C.2. E.2.1. Case α = 1. Here, we rather use the parametrisation (E.4), and the resulting formula is relatively simple:

(E.8) 1 -u = ∆ q 1-b + O(q),
When we restrict to real values of γ -, γ + -hence real values of ρ -we have ∆ ≥ 0 iff ρ ∈ [ρ min , ρ max ] with (E.9)

ρ min = √ 6 + n - √ 2 -n (1 -b) √ 2 + n .
and we note by comparing with (E.5) that ρ min > ρ ′ min for n ∈ [0, 2]. At ρ = ρ min , we have ∆ = 0, and we need to go further in the q → 0 expansion. The next term is of order q. To compute it, we need to take into account in Equation E.1 the term of order q arising from πC T and g k (Lemma B.8) and from the expansion of Υ b (Lemma D.2). The result for a general value of ρ is

1 -u = ∆q 1-b + ∆ 1 q + O(q 1+b ), with ∆ 1 = 24 b -ρ 2 (3b 2 + 1) √ 2 + n + 4ρb √ 2 -n + 2 √ 2 + n -ρ 2 b(1 -b 2 ) √ 2 + n + 4ρ(1 -b 2 ) √ 2 -n -6b √ 2 + n .
and for ρ = ρ min it specialises to

∆ 1 = 24(1 + b) b(1 -b)(2 -b) .
If we are at a dense critical point, we must have ∆ > 0, hence ρ ∈ (ρ min , ρ max ]. If we are at a dilute critical point, we must have ∆ = 0 and ∆ 1 > 0, hence ρ = ρ min . These necessary conditions were already obtained in [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF] -where the lower bound arose from the constraint of positivity of the spectral density associated with the generating series of disks F(x). Modulo Remark 5.4 about the justification that this condition is also sufficient, this establishes the phase diagram of the model for α = 1.

In particular, we see that at a dense critical point

q . ∼ (1 -u) 1 1-b ,
while at a dilute critical point we rather have q .

∼ (1u).

E.2.2. General α. The method is similar but the explicit results are cumbersome and we will not reproduce them here. We start from (E.3) but now have to take into account that w ∞ now depends on (q 1 2 , w * ∞ ), that it contains a q 1 2 term in its q → 0, and that so do πC T , g 1 and g 2 . We have nevertheless checked that the q 1 2 term is absent in the q → 0 expansion of (E.3), which gives an expansion of the form

1 -u = ∆ q 1-b + ∆ 1 q + O(q 1+b )
for some ∆ and ∆ 1 which are complicated functions of w * ∞ . If ∆ > 0 we have a dense critical point, if ∆ = 0 and ∆ 1 > 0 we have a dilute critical point. This reasoning is still valid although describing explicitly the dense and dilute critical locus requires the explicit expressions of ∆ and ∆ 1 . E.3. Delta-analyticity. Let us recall an important notion of singularity analysis [START_REF] Flajolet | Analytic combinatorics[END_REF].

Definition E.2. A delta-domain at z 0 ∈ C \ {0} is an open subset of the complex plane of the form z ∈ C \ {z 0 } | | z z 0 -1| < R, |arg( z z 0 -1)| > ϕ with R > 1 and ϕ ∈ (0, π 2 ).
A function is said delta-analytic if it is analytic in some delta-domain.

Let us introduce a weaker notion: we say that a function is delta-analytic locally at z 0 if it is analytic in the intersection of a delta-domain at z 0 and of a neighborhood of z 0 . It is not difficult to check that a function is analytic in a delta-domain at z 0 if and only if:

• it is analytic in the open disk of radius |z 0 | centered at 0,

• it is analytic at every point of modulus |z 0 | other than z 0 ,

• it is delta-analytic locally at z 0 .

Lemma E.3. If (g, n, α, h) is a non generic critical point (dense or dilute) and n ∈ (0, 2), the maps described in Lemma E.1 have an inverse: specialising the inverse to the value of w * ∞ if α ̸ = 1 (resp. ρ if α = 1), we obtain a map u → q which is delta-analytic locally at 1, and behaves like

q ∼ 1 -u ∆ c , c = 1 1-b dense phase 1 dilute phase
for some constant ∆ > 0.

Proof. Let us assume first α = 1. We have justified in the previous paragraphs that the maps (q

1 2 , ρ) → u from Lemma E.1 satisfy 1 -u = ∆ q 1-b + O(q),
where ∆ is a function of ρ. At a dense critical point, the value of ρ is such that ∆ > 0.

As 1b ∈ ( 1 2 , 1). the image of C \ R ≤0 by the map q → q 1-b is a delta-domain. Therefore, for η > 0 small enough the image of B(0; η) via the map q → u of Lemma E.1 contains a local delta-domain centered at 1 and on the latter we can find an inverse map u → q which is analytic, hence delta-analytic locally at u = 1, by definition. This map behaves like

q ∼ 1 -u ∆ 1 1-b .
At a dilute critical point, we have ∆ = 0 and pushing further the expansion we have

1 -u = ∆ 1 q + O(q 1+b ).
The image of C \ R ≤0 by the identity map being a delta-domain, we can repeat the same argument and conclude that we have a map u → q which is delta-analytic locally at u = 1.

For positive α ̸ = 1, we should distinguish (see Remark 5.1) between the case w ∞ ∈ τ, τ + 1 2 which can occur when α is small enough, and w ∞ ∈ 1 2 , 1 2 + τ on which we have focused since Appendix B. We only discuss the second case, as the first case can be obtained similarly, after an adaptation without further difficulty of the previous appendices. The condition ∆ > 0 (resp. ∆ = 0 and ∆ 1 > 0) is necessary to be at a dense (resp. dilute) critical point, so the discussion for α = 1 extends here using as second parameter w * ∞ instead of ρ: the explicit expressions for ∆, ∆ 1 are not needed in this argument. □ Appendix F. Scaling limits for pointed disks

We are going to prove Theorem 6.5 and Corollaries 6.6-6.7, i.e. analyse the generating series of pointed disks (F.1)

F • (x) = v ′ (x) G • (v(x)) -∂ x nu ln[ς ′ (x)] 2(2 + n) .
Here x is in the physical sheet, that is

v(x) ∈ R = v ∈ C, Re v ∈ -1 2 , 1 2 , Im v ∈ [0, T ]
. and we also assume that (g, h) are chosen at a non generic critical point when u = 1. According to the previous sections, it amounts to fixing a value of w * ∞ (if α ̸ = 1) or ρ (if α = 1) and take (g, h) given by (E.6) or (E.4).

Let us first fix the value of b. As the second term in (F.1) is linear in u, it will not contribute to the singularity analysis when u → 1. We therefore focus on the first term, as given by Proposition 5.5

G • (v) = u 2 + n -Υ b (v + v ∞ ) -Υ b (v -v ∞ ) + Υ b (-v + v ∞ ) + Υ b (-v -v ∞ ) .
In view of Remark D. We first analyse the regime x = x(v) with v = 1 2 + τ w and w in a compact region of the complex plane containing a u-independent neighborhood of w * ∞ . This means that x remains in a u-independent region away from

[γ -, γ + ]. We first need v ′ (x(v)) = 1 x ′ (v) . By Lemma B.6 we have x 1 2 + τ w = x * 0 (w) + O(q 1
2 ) with (F.2) x * 0 (w) := 2 cos(πw * ∞ ) h(1 -α 2 ) 1 cos(πw) -cos(πw * ∞ )
.

Differentiating with respect to v we get

x ′ 1 2 + τ w = π iT 2 cos(πw * ∞ ) h(1 -α 2 ) sin(πw) (cos(πw) -cos(πw * ∞ )) 2 + O(q 1
2 ).

Owing to Lemma D.2, we have

G • 1 2 + τ w = 2π T u 2 + n -Υ * b,0 (τ (w + w ∞ )) -Υ * b,0 (τ (w -w ∞ )) + Υ * b,0 (τ (-w + w ∞ )) + Υ * b,0 (τ (-w -w ∞ )) + q b 1 -q b (Υ * b+2,0 -Υ * b,0 )(w + w ∞ ) + (Υ * b+2,0 -Υ * b,0 )(w -w ∞ ) -(Υ * b+2,0 -Υ * b,0 )(-w + w ∞ ) -(Υ * b+2,0 -Υ * b,0 )(-w -w ∞ ) + O(q) . (F.3)
where we have used 1 1-q b = 1 + q b 1-q b to write separately the leading term. The quantity in brackets can be computed from (D.2). The prefactor u can be replaced by

1 up to O(q c ) = O(q 1 2 ) since c > 1 2 when b ∈ 0, 1 2 . All calculations done we obtain (F.4) v ′ (x(v))G • (v) = Ψ b (x) - q b 1 -q b Ψb (x) + O(q 1 2 ), with Ψ b (x * 0 (w)) = -1 2 + n h(1 -α 2 ) cos(πw) -cos(πw * ∞ ) 2 cos(πw * ∞ ) sin(πw) × cos[π(1 -b)(w + w * ∞ )] sin[π(w + w * ∞ )] + cos[π(1 -b)(w -w * ∞ )] sin[π(w -w * ∞ )] Ψb (x * 0 (w)) = Ψ b+2 (x * 0 (w)) -Ψ b (x * 0 (w)) = - 4 2 + n h(1 -α 2 ) cos(πbw * ∞ ) cos(πw) -cos(πw * ∞ ) 2 cos(πw * ∞ )
sin(πbw) sin(πw) .

(F.5)

For α = 1, this simplifies to

x * 0 (w) = ρ 2h cos(πw) , Ψ b (x * 0 (w)) = 2h cot 2 (πw) ρ √ 2 + n sin π(1 -b)w), Ψb (x * 0 (w)) = - 8h ρ √ 2 + n cos 2 (πw) sin(πbw) sin(πw) . (F.6)
In the regime v = τ w with w in a compact, we have according to Lemma B.6

q -1 2 (x(v) -γ + ) = x * 1 2 (w) + O(q 1
2 ), meaning that q -1 2 (xγ + ) remains in a u-independent compact. A similar analysis can be carried out and we only give the result

v ′ (x(v))G • (v) = q b-1 2 1 -q b Φ b x -γ + q 1 2 + O(q b 2 ), with x * 1 2 (w) = 16 cos(πw * ∞ ) (1 -α 2 )h cos 2 πw 2 , Φ b x * 1 2 (w) = h(1 -α 2 ) 2 + n cos(πbw * ∞ ) cos(πw * ∞ )
sin(πbw) sin(πw) .

(F.7)

For α = 1, it simplifies to

x * 1 2 (w) = 4ρ h cos 2 πw 2 , Φ b x * 1 2 (w) = 4h ρ √ 2 + n sin(πbw) sin(πw) . (F.8)
One can check that this analysis remains valid if b = b(s) and s is complex-valued but such that Re b(s) ∈ 0, 1 2 -noting this inequality also implies Re 1 1-b(s) > 1 2 . This completes the proof of Theorem 6.5.

We move to the proof of Corollary 6.6. Planar pointed rooted maps are pointed disks whose boundary face is a triangle. Therefore, their generating series with vertex weight u is:

[x -4 ]F • = -Res x=∞ dx x 3 F • (x) = -Res v=v∞ dv (x(v)) 3 G • (v) = -iT Res w=w∞ dw x 1 2 + τ w 3 G • 1 2 + τ w .
(F.9)

After taking the residue and taking into account Remark D.1 and the analyticity properties established in Appendix B, we find that [x -4 ]F • is an analytic function of q ∈ B(0; η) \ R ≤0 . We will see in Theorem J.1 that q is a delta-analytic function of u, so this implies that [x -4 ]F • is a delta-analytic function of u.

To compute (F.9), we use (F.2) and (F.4). We first treat α ̸ = 1. The leading term u • q 0 does not contribute to the singularity as it is an entire function of u, so the relevant part for the singularity analysis therefore comes from Ψb . We then use the Laurent expansion of

x(v) when v → v ∞ from Lemma B.1 to get [x -4 ]F • | sing = 16uπ sin(πbw * ∞ ) 2 + n • 3bπC 2 E 1 4T 2 q b + o(q b ).
Taking the leading term when q → 0 of E 1 and πC T from Lemma B.5, and replacing u by 1 up to negligible terms, we obtain (F.10)

[x -4 ]F • | sing = A q b + o(q b ), with (F.11) A = 96b sin(πbw * ∞ ) cos(πw * ∞ ) 1 -α sin 2 (πw * ∞ ) (2 + n)h 2 (1 -α 2 ) 2 sin 3 (πw * ∞ )
, where it remains to substitute the value of h 2 in terms of w * ∞ from (E.6). We can also do the computation for α = 1 in terms of the parameter: the result is correctly reproduced The first term R b(s) does not feature a singularity when u → 1, and thus will not contribute to large volume asymptotics. We compute using the expression of Υ * b,0 in (D.2):

(G.1) R b(s) (w 1 , w 2 ) -R b(s)+2 (w 1 , w 2 ) = -8πb (
s) sin(πb(s)w 1 ) sin(πb(s)w 2 ).

Therefore:

F (2) s (x 1 , x 2 )| sing = - b(s) q b(s) 1 -q b(s) Ξ b(s),3 (x * 1 2 (w 1 ), x * 1 2
(w 2 )) + O(q), with:

Ξ b(s),3 = 2h 2 (1 -α 2 ) 2 4 -n 2 s 2 2 i=1 (cos(πw i ) -cos(πw * ∞ )) 2 sin(πb(s)w i ) cos(πw * ∞ ) sin(πw i )
.

For α = 1, it specialises to:

Ξ b(s),3 = -32h 2 ρ 2 (4 -n 2 s 2 ) 2 i=1 cos 2 (πw i ) sin(πb(s)w i ) sin(πw i ) .
G.2. Refined cylinders: finite/large. This is governed by x 1 = x 1 2 + τ w 1 and x 2 = x(τ w 2 ), and leads to:

F (2) s (x 1 , x 2 )| sing = q (b(s)-1)/2 1 -q b(s) (1 -α 2 ) 2 h 2 (cos(πw 1 ) -cos(πw * ∞ )) 2 16π(4 -n 2 s 2 ) cos 2 (πw * ∞ ) sin(πw 1 ) sin(πw 2 ) × Rb(s) (w 1 , w 2 ) + O(q (1-b(s))/2 ) , with: Rb(s) (w 1 , w 2 ) = -2i (Υ * b(s), 1 2 ) ′ (w 1 + w 2 ) -(Υ * b(s), 1 2 ) ′ (w 1 -w 2 ) -(Υ * b(s), 1 2 ) ′ (w 2 -w 1 ) + (Υ * b(s), 1 2 ) ′ (-w 1 -w 2 )
= 8π b(s) sin(πb(s)w 1 ) sin(πb(s)w 2 ). Therefore:

F (2) s (x 1 , x 2 )| sing = b(s) q (b(s)-1)/2 1 -q b(s) Ξ b(s),4 (x * 1 2 (w 1 ), x * 0 (w 2 )) + O(q (1-b(s))/2 ), with: Ξ b(s),4 = (1 -α 2 ) 2 h 2 [cos(πw 1 ) -cos(πw * ∞ )] 2 2(4 -n 2 s 2 ) cos 2 (πw * ∞ ) 2 i=1
sin(πb(s)w i ) sin(πw i ) .

In particular for α = 1, we find:

Ξ b(s),4 = 8h 2 ρ 2 (4 -n 2 s 2 ) cos 2 (πw 1 ) 2 i=1 sin(πb(s)w i ) sin(πw i ) . algorithm if h ↓ (0) = 1 and (H.6) h ↓ (p) = ∞ k=0 ν(k -p)h ↓ (k) + ∞ k=1 ∞ k ′ =0 A k,k ′ γ k+k ′ + 2 ν(-k -p)h ↓ (k ′ ), p ≥ 1.
We claim that such a function h ↓ exists and can be interpreted as the probability that a certain generalisation of the ricocheted random walk of [START_REF] Budd | The peeling process on random planar maps coupled to an O(n) loop model (with an appendix by L. Chen[END_REF]Section 4] gets trapped at 0. This generalisation is in fact rather straightforward: we consider a random walk with step distribution ν which gets trapped when touching 0 and, when it would jump to some position -k < 0, gets ricocheted to position k ′ ≥ 0 with probability

k ′ ≥0 A k,k ′ (γ * + ) k+k ′ = n, k ≥ 1.
Note that, when γ + = γ * + , the probability to remain trapped when jumping to position -k < 0 is equal to 1 -n 2 > 0 independently of k. It is higher and dependent on k for γ + < γ * + . It follows that the ricocheted walk gets trapped almost surely, since the walk cannot drift to +∞ by [29, Proposition 4], and therefore there indeed exists a nonnegative function h ↓ satisfying (H.6). Note that the case n = 2 and γ + = γ * + is slightly subtler since the walk always ricochets when jumping to a negative position. We do not consider this case here, even though we expect the same conclusion to hold.

Straightforward adaptations of the other arguments given in [32, Section 5] lead to Proposition H.2, and furthermore imply that the expected number of vertices of a loopdecorated map with perimeter p is equal to f ↓ (p), hence is finite. This concludes the proof of Theorem H.1.

Remark H.4. Here we are considering a martingale, whereas Budd considers a supermartingale, since he only defines the ricocheted random walk corresponding to the non generic critical case.

Remark H.5. Using targeted peeling and the uniqueness of the solution of (H.6) for given boundary conditions, we may identify (H.9)

f ↓ (p) = F • p F p , h ↓ (p) = F • p γ p + ,
and we may interpret h ↓ as the harmonic function used to condition the ricocheted walk to get trapped at 0 via a Doob h-transform. Changing the boundary condition of h ↓ to condition the walk to get trapped at -k < 0 should give a relation with the generating series of cylinders. α = 0. In this identification, the weight per visited quadrangle, denoted g in Budd's paper and h 1 in [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF], is equal to h 2 in our present notations.

I.1. An explicit expression for F • s (x) at a non generic critical point. In this section we set the vertex weight u to 1. Consider the generating series F(x) as defined in (4.1). Noting that the sum is restricted to even ℓ's, we see that the cut of F is necessarily symmetric and we denote it by [-γ, γ], dropping the ± subscripts. The condition for non generic criticality reads

(I.1) γ = γ * := h -1
which is nothing but the case α = 0 of (6.1). It was shown in [START_REF] Borot | A recursive approach to the O(n) model on random maps via nested loops[END_REF] that, at a non generic point of the model on quadrangulations with a weight g 4 per unvisited quadrangle and for n ∈ (0, 2), we have the explicit expression

(I.2) F(x) = F part (x) + F hom (x)
where

F part (x) := 2(x -g 4 x 3 ) -n γ 4 x 3 -g 4 γ 8 x 5 4 -n 2 + n (2 + n)x F hom (x) := f(x) -γ 2 x 2 f γ 2 x x -γ x + γ b -f(-x) -γ 2 x 2 f -γ 2 x x + γ x -γ b f(x) := g 4 4 -n 2 x 3 + 2bγx 2 + 2b 2 γ 2 x + 2(b + 2b 3 )γ 3 3 - x + 2bγ 4 -n 2 (I.3)
and we recall b = 1 π arccos n 2 . A nice feature of this explicit expression is that it bypasses the use of the elliptic parametrisation, which makes the singularity analysis somewhat simpler. In particular, we immediately see why b appears in the singular expansions for x → ±γ. The method that was used to obtain the expressions (I.3) may be generalised to the case where the unvisited faces have arbitrary even degrees.

It is natural to ask whether similar explicit expression exist for the other generating series that we consider in this paper. We will not consider the case of cylinders here but, in the case of pointed disks, the question admits an affirmative answer.

Proposition I.1 (see also [START_REF] Bouttier | Planar maps and random partitions[END_REF]Section 3.4]). At a non generic critical point of the rigid model with n ∈ (0, 2), possibly with unvisited faces of arbitrary even degrees, the refined generating function F • s (x) of pointed disks, defined as in (4.3), admits the universal expression

(I.4) F • s (x) = 1 (2 + ns)x ns + x + γ x -γ b(s)-1 + x -γ x + γ b(s)-1
where b(s) = 1 π arccos ns 2 > 0 is defined as in (5.26). Notice (again, considering γ fixed) that this expression depends on n and s only via the combination ns.

Proof. We specialise the functional equation (5.20) with ς(x) = γ 2

x (since α = 0, h = γ -1 , γ denoting now the positive endpoint of the cut) and u = 1. This yields

(I.5) ∀x ∈ (-γ, γ), F • (x + i0) + F • (x -i0) + nγ 2 x 2 F • γ 2 x = n x .
We may solve this equation using the method described in [17, Section 6.2], the function f(x) being here proportional to (xγ) -1 . This yields (I.4) for s = 1. Then, we recall from § 4.4 that adding the refinement parameter s amounts to changing n into ns. □ Interestingly, the universal form (I.4) also appears implicitly in [START_REF] Budd | The peeling process on random planar maps coupled to an O(n) loop model (with an appendix by L. Chen[END_REF]. To make the connection precise, we combine Equations ( 23), ( 25) and [START_REF] Nijs | Extended scaling relations for the magnetic critical exponents of the Potts model[END_REF] of that paper, which yield the relation

(I.6) ∞ ℓ=0 h ↓ n/2 (ℓ)x 2ℓ = γ x F • γ x for s = 1.
Here, h ↓ p (ℓ) denotes the probability that Budd's p-ricocheted random walk gets trapped at 0.

It is very easy to analyse the singular behaviour of (I.4). We find

(I.7) F • s (x) ∼ x→±γ ± 2 1-b(s) (2 + ns)γ • (1 ∓ γ/x) b(s)-1 ,
which implies for the refined generating series of pointed disks of perimeter 2ℓ

(I.8) F • 2ℓ [s] ∼ ℓ→∞ 2Γ(b(s)) 4 -b(s) π 2 -ns 2 + ns • γ 2ℓ ℓ b(s) ,
consistently with [START_REF] Budd | The peeling process on random planar maps coupled to an O(n) loop model (with an appendix by L. Chen[END_REF]Equation (24)]. This yields the asymptotic behaviour (I.9)

E s P L = 2ℓ = F • 2ℓ [s] F • 2ℓ [1] ∼ ℓ→∞ C(s)ℓ b-b(s) .
for the probability generating function of the number P of separating loops in a pointed disk of prescribed perimeter 2ℓ and fluctuating volume. The varying exponent in (I.9) is a smoking gun evidence that P grows logarithmically with ℓ. In fact, a straightforward adaptation of the method of the proof -which crucially on Hwang's quasi-powers theorems [69, Theorems IX.8 and IX.15] -of Proposition 6.9 and Theorem 6.10 in the main text, we obtain the following variant of Theorem 2.2 and Proposition 2.3.

Theorem I.2 (see also [START_REF] Budd | The peeling process on random planar maps coupled to an O(n) loop model (with an appendix by L. Chen[END_REF]Theorem 5] and [START_REF] Bouttier | Planar maps and random partitions[END_REF]Theorem 3.3]). At a non generic critical point of the rigid model with n ∈ (0, 2), possibly with unvisited faces of arbitrary even degrees, the distribution of the number P of separating loops in the ensemble of random pointed disks with prescribed perimeter L = 2ℓ and fluctuating volume behaves when ℓ → ∞ as (I.10)

P P = ln ℓ π p L = 2ℓ . ≍ (ln ℓ) -1 2 ℓ -1 π J(p)
where J is the same rate function as in Theorem 2.2, and p bounded, bounded away from 0 and chosen so that P is an integer. We have the convergence in law (I. .

Two remarks are now in order. First, we note that Budd's theorem [32, Theorem 5] also treats the case n = 2. Nothing would prevent from rederiving his result by taking n → 2 in Proposition I.1.

Second, we observe that Theorem I.2 makes no distinction between dilute or dense critical points. In contrast, Theorem 2.2 and Proposition 2.3 involved the critical exponent c, which depends on the nature of the non generic critical point (c = 1 in the dilute phase and c = 1 1-b in the dense phase). In fact, the large perimeter versions of Theorem 2.2 and Proposition 2.3 are totally consistent with Theorem I.2, when we replace ln V with c 2 ln ℓ. This means that, if we fix a large perimeter L, then further conditioning on a large volume V ∼L 2 c does not affect the asymptotics of P under consideration. I.2. Delta-analyticity with respect to the vertex weight u. Recall Definition E.2 of delta-domain and delta-analyticity. In this section, we consider the rigid loop model on bipartite maps, with the parameters n (weight per loop), h 2 (weight per visited square) and g 2k (weight per unvisited face of degree 2k ≥ 2) fixed to nonnegative real values. We assume that n, h > 0 (to have a nontrivial loop model), that g 2 < 1 (to avoid the proliferation of digons) and that g 2k = 0 for k large enough (i.e., the face degrees are bounded). We will vary the vertex weight u, hence we will keep the dependence on u explicit.

The partition function F 2ℓ (u) is a series in u with nonnegative coefficients and, for ℓ positive, has a finite radius of convergence u c which does not depend on ℓ. Recall from Proposition 4.1 the definition of r(u) = 1 2 γ 2 + (u) (in the bipartite case, we have s(u) = 0 since the cut is symmetric). By Remark 4.2, it is essentially the same as the series F • 2 (u) = 2ur(u) of rooted maps with a marked point in the gasket, thus has positive coefficients and radius of convergence u c . The purpose of this section is to establish the following:

Theorem I.3. If there exists an integer k such that g 4k > 0, then r(u) and F 2ℓ (u) are analytic functions of u in a delta-domain at u c , for all ℓ > 0. When g 4k vanishes for all integer k, they are analytic in the intersection of a delta-domain at u c and a delta-domain at -u c , since we have the parity relations r(u) = -r(-u) and F 2ℓ (u) = (-1) ℓ+1 F 2ℓ (-u). q, seen as a function of u, has the same properties.

The delta-analyticity of q is a direct corollary of the delta-analyticity of r(u) and the fact that q is an analytic function of r(u), which we observe in two steps: m is an analytic function of r(u) as we see later in (I.15) and q is an analytic function of m by the definition (B. [START_REF] Borot | Loop models on random maps via nested loops: case of domain symmetry breaking and application to the Potts model[END_REF]).

The reason why the case g 4k = 0 is special is the following. In a bipartite map, an elementary counting argument based on Euler's formula shows that the number of vertices and the number of faces with degree divisible by 4 have the same parity. When the map carries a rigid loop configuration, the number of visited squares is necessarily even, since the loops form annuli whose contours must have even length. Therefore, if we consider a map contributing to F 2ℓ (u) with no unvisited inner face of degree divisible by 4, then the parity of the number of vertices is opposite to that of ℓ. For a map contributing to r(u) with the same constraint, the number of vertices is even, but we assign no weight to the marked vertex.

We will make use of the equation (4.6) determining r(u) which, in the rigid bipartite case, may be rewritten in the form (I.12) r(u) = u + k≥1 2k -1 k g 2k + nh 4k F 2k (u) r(u) k making sense whenever the series r(u) is absolutely convergent. We have the following elementary lemma, relying on the nonnegativity of the coefficients of r(u).

Lemma I.4. We have r(u c ) ≤ 1 4h 2 so that r(u) converges normally on its closed disk of convergence. For every u in this disk, different from u c , and different from -u c if g 4k vanishes for all integer k, we have (I. [START_REF] Benjamini | KPZ in one dimensional random geometry of multiplicative cascades[END_REF] |r(u)| < r(u c ).

Proof. By monotone convergence, we have r(u c ) = lim u→u - c r(u), so we need to prove that r(u) ≤ 1 4h 2 for every u ∈ (0, u c ). For such u, we know by Proposition 4.1 that

lim k→∞ F 2k (u) 1 k → 4r(u).
Since the sum appearing in (I.12) must converge, we conclude that 16h 4 r(u) 2 ≤ 1 as wanted. To obtain (I.13), we apply the Daffodil Lemma [69, Lemma VI], which requires checking that r(u) is aperiodic if one g 4k is nonzero, and has period 2 otherwise. For this, we observe that (I.12) implies that [u 2k+1 ]r(u) > 0 for all k. Indeed, [u k+1 ]F 2k (u) > 0 as trees with k + 1 vertices contribute, and when g 4k > 0 we also have [u 2k ]r(u) > 0. □

We will also make use of the exact solution of the model, discussed in Section 5 and in the appendices, via the following: Proposition I.5. There exists functions φ and ψ ℓ (ℓ ≥ 0) which are meromorphic in the domain C \ ((-∞, -1 4h 2 ] ∪ [ 1 4h 2 , ∞)) and such that (I. [START_REF] Bonnet | The Potts-q random matrix model: loop equations, critical exponents, and rational case[END_REF] u = φ(r(u)), F 2ℓ (u) = ψ ℓ (r(u)).

The set of poles of ψ ℓ is included in that of φ.

Proof. For u ∈ (0, u c ) and given the values of γ ± (u) = ±2 r(u), Theorem 5.3 (specialised to the rigid bipartite case) gives an explicit expression of G(v), which is related to F(x) via (5.15). Notice that the expression of G(v) depends linearly on u via the gk defined in (5.16). Thus, the conditions (5.17) determining γ ± (u), which turn out to be equivalent to each other in the rigid case, yield a linear condition on u, which is nontrivial by the discussion of Appendix E. Solving this linear condition, we express u as a rational function of derivatives of the function Υ b (v) at v = τ ± 1 4 (we have v ∞ = 1 4 in the rigid case). By (D.1), Υ b is itself a rational function of the Jacobi theta functions, which are analytic in the elliptic parameter m except at the singularities 0, 1, ∞. Specialising (B.1) to the rigid bipartite case, the elliptic parameter is given by (I.15) m = 1 -4h 2 r(u) 1 + 4h 2 r(u)

2

.

Grouping all the steps together, we get a meromorphic function φ in C * \ ((-∞, -1 4h 2 ] ∪ [ 1 4h 2 , ∞)) such that u = φ(r(u)). Since r(u) is analytic at u = 0 with r(u) = u 1-g 2 + o(u), φ has no singularity at 0. Now, the F 2ℓ are given by the expansion of F(x) around x = ∞, or equivalently of G(v) around v = 1 4 . This expansion involves those of Υ b (v) around v = 0, 1 2 and of x(v) around v = 1 4 . The functions Υ b (v) and x(v) are precisely constructed to have simple poles at respectively v = 0 and v = 1 4 for all m, and the coefficients in their expansions are analytic in m. Finally, we substitute u = φ(r(u)), to find that F 2ℓ (u) = ψ ℓ (r(u)) for some meromorphic function ψ ℓ whose set of poles in included in that of φ. □

By the discussion at the beginning of Appendix E.3, the proof of Theorem I.3 requires to check two things: local delta-analyticity at u c , and analyticity at every other point of modulus u c (except -u c when g 4k = 0, which we can be treated by symmetry).

In the case of a non generic critical point (r(u c ) = 1 4h 2 ), local delta-analyticity at u c is found in Lemma E.3, whose proof was detailed for the loop model triangulations with bending energy α not too small, but can be adapted to all nonnegative α including the rigid loop model at α = 0. Thus, what we still have to prove is local delta-analyticity at u c for generic critical points (r(u c ) < 1 4h 2 ), and analyticity at other points of modulus u c . In view of Lemma I.4 and Proposition I.5, it is sufficient to establish these for r(u). We start with the analyticity statement. Proof. Let r * = r(u * ), which lies in the domain of analyticity of φ. We want to show that φ ′ (r * ) ̸ = 0, since we may then apply the analytic inverse function theorem to show that φ admits an inverse in a neighborhood of u * , providing the analytic continuation we are looking for. Instead of trying to compute φ ′ (r * ) directly, we will rather use (I.12), which amounts to the relation We will show that, for r → r * , the quantity 1 -A(r) tends to a nonzero limit and B(r) to a finite limit, which implies that φ ′ (r * ) ̸ = 0 since φ ′ is continuous at r * .

weight g k per unvisited face of degree k ≥ 1, and the weight u per vertex. We fix n, h, α and (g k ) k≥2 to nonnegative real values, with α, h > 0, n ∈ (0, 2), g 2 < 1 and g k = 0 for k large enough. We will however let u and g 1 vary in the complex plane, thus we will keep the dependence on them explicit (we may think of u as being g 0 ). We aim at establishing the following result.

Theorem J.1. Assume u c (0) is a non generic critical point, i.e. s(u c (0), 0)+2r(u c (0), 0) = γ * + . Then r(u, g 1 = 0), s(u, g 1 = 0), q(u, g 1 = 0), F ℓ (u, g 1 = 0) (ℓ > 0) are delta-analytic functions of u.

In this theorem, the delta-analyticity of q is directly implied by the delta-analyticity of r and s, as it is an analytic function of γ ± = s ± 2 √ r (consider together (B.1), (B.8), and (B. [START_REF] Borot | Loop models on random maps via nested loops: case of domain symmetry breaking and application to the Potts model[END_REF]). As the delta-analyticity statement locally around u = u c (0) is a consequence of Lemma E.3 and the preceding discussion on analyticity in q 1 2 of all the quantities of concern near q 1 2 → 0, we focus on the justification of the existence of an analytic continuation at the other points on the closure of the disk of convergence in the u-plane. Our proof will in fact give a similar property when g 1 is set to small enough (perhaps non-zero) value. Treating g 1 as a parameter is the trick making possible to adapt the strategy of Appendix I.2 to this bivariate situation.

Consider the partition functions F ℓ (u, g 1 ) (ℓ > 0) and the series r(u, g 1 ) and s(u, g 1 ) of Proposition 4.1 and Remark 4.2. All these are series in u and g 1 with nonnegative coefficients, which are absolutely converging in an (ℓ-independent) open subset B ⊂ C 2 which is a neighborhood of (0, 0). This domain of convergence is such that for any g 1 there exists some u c (g 1 ) ≥ 0 such that B ∩ (C × {g 1 }) = B(0; u c (g 1 )) × {g 1 }, and u c (g 1 ) > 0 for g 1 small enough.

Following the notations from [18, Section 6], let us define (J.1) P k (r, s) :=

⌊ k 2 ⌋ i=0 k! (i!) 2 (k -2i)! r i s k-2i ,
and define similarly

(J.2) Q k (r, s) := ⌊ k-1 2 ⌋ i=0 k! i!(i + 1)!(k -2i -1)! r i+1 s k-2i-1 .
These are polynomials with nonnegative coefficients, counting certain lattice paths. For r, s > 0, we have lim k→∞ P k (r, s)

1 k = lim k→∞ Q k (r, s) 1 k = s + 2 √ r.
Then, the relations (4.6) determining (r, s) may be rewritten r(u, g 1 ) = u + k≥2 G k (u, g 1 ) Q k-1 (r(u, g 1 ), s(u, g 1 )), s(u, g 1 ) = k≥1 G k (u, g 1 ) P k-1 (r(u, g 1 ), s(u, g 1 )), (J.3) and p ∈ (-∞, 0), hence the only possible singularities occur on the locus m ∈ {1, ∞} or p ∈ {0, ∞}. When (r, s) ∈ Y, the points γ ± = s ± 2 √ r are contained B(0; 1 h(α+1) ) 2 . Recall that γ * + is a fixed point of ς, and the other fixed point is 1 h(α-1) which is outside B(0; 1 h(α-1) ). We then observe that the image of B(0; 1 h(α+1) ) via the involution ς is disjoint from B(0; Therefore, m = 1 corresponds to r = 0 and the complement of this locus in Y is not simply-connected (its fundamental group is Z). We are going to show, using modular transformations for the theta functions and Jacobi elliptic functions, that there are in fact no singularities at m = 1. Since Y is simply-connected, this will justify that the coefficients of the system (J.5) can be continued (uniquely) to analytic functions on the whole Y. The important variable after modular transformation is

q = e 2iπτ = e -πK(m) K(1-m) ∼ m→1 1 -m 16 .
This is an analytic function of m in a neighborhood of 1. The expression (A.1) of ϑ 1 (v|τ ) is a series of terms involving q 1 8 + m(m+1) 2

. Up to the q 1 8 prefactor this contains only integer powers of q. So, the ratio Υ b (v) in (D.1) involves only integer powers of q, hence is an analytic family (over q in a neighborhood of 0) of meromorphic functions of v. With Jacobi imaginary transformations we also convert (B.15) into

v ∞ = arcsc i p m ; 1 -m 2K(1 -m) ∼ m→1 arctan i √ p) π ,
where arcsc is (an analytic continuation of) the reciprocal function of sc = sn cn . The singularity at m = 1 is now absent as these quantities are analytic near the locus m = 1, and Υ (l) b (v ∞ + ε) for ε ∈ {0, 1 2 } and l ∈ N are analytic functions near the locus m = 1, as desired. The case α = 1 is in fact simpler since w ∞ = 1 2 is independent of γ ± and the previous discussion of analytic continuation for q 1 2 was sufficient to conclude. It remains to justify that det(D) is not identically zero. For this, we evaluate it when γ + approaches γ * + . Using the variables (m, p) of Section B, this corresponds to m → 0, i.e. q → 0. According to (B.30), we have v = 1 2 + τ w ∞ with

w ∞ ∼ w * ∞ = 2 π arcsin 1 √ p .
Using Lemma D.2, we obtain Proof of Proposition J.2. We will again invoke the analytic implicit function theorem, now in its bivariate form. Note that, by Lemma H.3, for any u > 0 and g 1 ≥ 0 such that (u, g 1 ) ∈ B, we have γ + (u, g 1 ) ≤ γ * + , and by monotone convergence the same property holds for (u, g 1 ) ∈ ∂B. Thus, for any (u * , g * 1 ) satisfying the hypotheses of Proposition J.2, (r * , s * ) := (r(u * , g * 1 ), s(u * , g * 1 )) belongs to the domain of analyticity of φ. What remains to check is that the differential of φ is nondegenerate at (r * , s * ).

f (v ∞ ) ∼ - 4π T cos(πbw * ∞ ), f ′ (v ∞ ) ∼ 4π T πb iT sin(πbw * ∞ ), f v ∞ + 1 2 ∼ 2π T sin π(b -1)w * ∞ ) sin(πbw * ∞ ) , f ′ v ∞ + 1 2 ∼ 2π T π iT (b -
We now substitute (u, g 1 ) = φ(r, s) in (J.3), and differentiate, which is possible whenever (r, s) is inside D = φ -1 (B). The result may be written compactly in matrix form (J.7)

Id -M = (Id + N)J φ , where J φ is the Jacobian matrix of φ:

(J.8) J φ = ∂ r u ∂ s u ∂ r g 1 ∂ s g 1 ,
and

M = k≥1 (k -1)G k P k-2 Q k-2 1 r Q k-2 P k-2 , N = k≥1 ℓ≥0 A k,ℓ Q k-1 ∂ u F ℓ Q k-1 ∂ g 1 F ℓ P k-1 ∂ u F ℓ P k-1 ∂ g 1 F ℓ .
(J.9)

Here, we are using the relation ∂ r Q k-1 = (k -1)P k-1 and its variants. Note that 1 r Q k-2 is still a polynomial in r, s.

Notice that, when expressing M and N as power series in u and g 1 , all their coefficients are nonnegative, and M has no constant coefficient. The eigenvalues of M are of the form X ±Y √ r, with X, Y also power series with nonnegative coefficients and no constant term. When restricting to u and g 1 real nonnegative in B, the nonvanishing of det J φ (since φ is a local diffeomorphism at (r, s) ∈ φ -1 (B)) implies that X + Y √ r must remain strictly smaller than 1. Thus, going back to complex values, the eigenvalues of M have modulus strictly smaller than 1 in all B, and the same holds for their limits at (r * , s * ), since it is assumed that |r * | < r(|u * |, |g * 1 |). We conclude that det(Id -M) tends to a nonzero limit at (r * , s * ). + , we find that N has a finite limit at (r * , s * ), and we conclude by continuity that det J φ (r * , s * ) ̸ = 0, as wanted. □

We expect that Proposition I.7 can be extended to treat generic critical points of the bending energy model, but we shall not attempt to do so here.

Figure 2 .

 2 Figure 2. Top row: local weights for the O(n) loop model on random triangulations. Bottom row: in the bending energy model, an extra weight α is attached to each segment of a loop between two successive turns in the same direction.

Figure 3 .

 3 Figure 3. Qualitative phase diagram of O(n) loop model on random maps: there is a line of critical points separating the subcritical and supercritical phase. Critical points may be in three different universality classes: generic, dilute and dense.

π arccos n 2 .

 2 Summary of the critical exponents for the O(n) model on random maps as functions of b = 1 Pure gravity corresponds to the n = 0 model in the dilute phase, critical percolation to the n = 1 model in the dense phase, the critical Ising model and its interfaces to both the n = 1 model in the dilute phase (for spin clusters) and the n = √ 2 model in the dense phase (for FK clusters). The Kosterlitz-Thouless transition is that of the n = 2 model where the dilute and dense exponents are identical. More generally, the critical Q-Potts model and its FK cluster boundaries correspond to the O(n = √ Q) model in the dense phase. the O(n) model on regular lattices, the relation being g = 1 + b (dilute) or g = 1b (dense).

3 2 and 5 2 ,

 2 which can take more precisely four values for a given value of n: 3 2 (subcritical point),5 2 (generic critical point), 2 + b (dilute critical point) and 2b (dense critical point).

Figure 4 .

 4 Figure 4. The gasket of the map depicted in Figure 1.

Figure 5 .

 5 Figure 5. The function J(p) for n = 1, n = √ 2 (Ising) and n = √ 3 (3-Potts). The larger is the value of n, the smaller is the slope when p → ∞.

Figure 6 .

 6 Figure 6. Left: schematic representation of a loop configuration on a planar map with one boundary. Right: the associated nesting tree (the red vertex corresponds to the gasket).

Figure 7 .

 7 Figure 7. Illustration of (3.6).

4. 4 .Proposition 4 . 8 .

 448 Separating loops. The functional relations for the refined generating series (cylinders or pointed disks) including a weight s per separating loop, are very similar to those of the unrefined case. At least for |s| < 1 and for s = 1, the formal series F[START_REF] Ambjørn | The toroidal Hausdorff dimension of 2d Euclidean quantum gravity[END_REF]

  as a function of s. Let F(2),|| (x, y) be the generating series of cylinders for face weights (|g k |) k and annuli weight (|A k,l |) k,l . As the latter are strictly admissible by assumption, F (2),|| satisfies the growth condition in Proposition 4.6. Since we have for (s, x, y) in the aforementioned domain of analyticity the bound |F

(

Figure 8 .

 8 Figure 8. The rectangle R in the v-plane. We indicate the image of special values of x in purple, and the image of the cut γ in red. The left (resp. right) panel is the image of Im x > 0 (resp. Im x < 0).

  s∈[0,2/n] p ln(s) + arccos(ns/2)arccos(n/2) = p ln 2 n p 1 + p 2 + arccot(p)arccos(n/2).(6.8)

where ( 6 6 p 2 p 2 +

 6622 .13) S (s) = -s ln Pcb(s) ln V + cb This function has critical points at s = ± s πP c ln V , where for p > 0 we have defined (and for the record we introduce (6.15) b(p) := b(s(p)) = arccot(arccot(p)arccos(n/2)

(6. 23 ) 2 ⌋

 232 Taking the ratio of (6.23) and(6.22) and replacing p and l with p and ℓ such that P = cp ln V 2π and L = ⌊ℓV c gives the desired distribution (6.7).

Figure 9 .Figure 10 .

 910 Figure 9. The contour of integration for u.

9. 2 . 4 .

 24 Quantum and Lebesgue measures. Define the (random) Liouville quantum measure of the Euclidean ball B(z, ε), (9.14) δ := B(z,ε) µ γ (d 2 z), and the logarithmic coordinates, (9.15) t := ln(1/ε), A := γ -1 ln(1/δ).

1 4 C

 4 (z, D) ≤ dist(z, D) ≤ C(z, D) by Koebe 1 4

9. 3 . 3 .

 33 Role of the KPZ relation. Let us define: Θ(p) := E * γA .

( 9 .

 9 39) c = min 1, κ 4 , a ′ = πb = π 1 -4 κ = arccos n 2, where b and c are the exponents defined in (2.4) and Section 2.3. The explicit form (9.37) immediately yields the parametric solution to Legendre-Fenchel equations (9.38),(9.40)

1 4 sin πw 2 1 -4q 1 2

 121 For x = τ w = iT w, we need to study sn[2iK(1m) • iT w ; m] = -sn[K(m)w ; m]. For this we can use the Fourier expansion (B.31) sn[K(m)w ; m] = 4q + O(q) , (B.34)

□B. 5 . 1 .

 51 The case α = 1. There are some simplifications in absence of bending energy, i.e., α = We then have ς(x) = h -1x and the parameters (p, m) defined in (B.1)-(B.11) are not anymore independent as p(2p) = m. This phenomenon also shows up as a singularity in the inverse change of variables (B.12), or equivalently, in the fact that since ς(∞) = ∞ we must have w ∞ = 1 2 independently of (γ -, γ + ), hence w * ∞ = 1 2 . We are therefore going to define a different change of variables χ 1 : (γ -, γ + ) → (m, ρ) with m still defined by (B.1) and ρ = 1 -2hγ -.

  2 and E 3 are obtained by inserting again (B.35)-(B.22) into the definitions (B.10).□

1 2 =

 2 e -iπ 2τ ∈ B(0; 1) \ (-1, 0]. The values above and below the real negative axis in q are different. The poles of Υ b are located at Z ⊕ τ Z. Equation (C.1)). So, using Lemma D.2 and after dividing the equation by 2πq b 2

  w) = sin(2bw) -3 + (2 + α) sin 2 (w) , P 3 (w) =sin(2bw), P 2 (w) = -3 sin(2w) 2 sin(2bw), P 1 (w) = 2 sin(2w) (3α 2 + 1) cos 4 (w) + 12(α + 1) cos 2 (bw) -6α 2 + 6α + 2 cos 2 (w)+ 12(1α) cos 2 (bw) + 3(1α)2 , P 0 (w) = 6 sin(2bw) -(α + 1)(α + 3) sin 4 (w) + 6(α + 2) sin 2 (w) -10 , and Q4 (w) = sin 2 (w) sin 3 (2w), Q3 (w) =sin 2 (w) sin(2w) sin(2bw), Q2 (w) = 2 sin 2 (w) sin(2w) (3α 2 -1) cos 4 (w) -2 (α + 2) cos 2 (bw) + 3α 2 -5α + 3 cos 2 (w), + 4(1α) cos 2 (bw) -3α 2 + 10α -7 , Q1 (w) = 2 sin 2 (w) sin(2bw) (3α 2 + 12α + 7) cos 4 (w) + 2(-3α 2 -3α + 7) cos 2 (w) + 3(1α) 2 ,

  [START_REF] Aizenman | Path-crossing exponents and the external perimeter in 2d percolation[END_REF] and Lemma E.3, G • (v) can be considered as an analytic family of meromorphic functions of v, parametrised by u in a delta-domain centered at 1. On the other hand x → v(x) given by (B.14) is an analytic family of analytic functions of x in the physical sheet, parametrised by m in a small neighborhood of 0. Changing the variable to q (see Lemma B.3 or Lemma B.7) and then to u (Lemma E.3), we deduce that x → v ′ (x)G • (v(x)) is an analytic family of meromorphic functions of x in the physical sheet, parametrised by u in a delta-domain centered at 1. The map s → b(s) = 1 π arccos ns 2 is an analytic function of s in the strip |Re s| < 2 n . So, if we set b = b(s), one can extend the previous arguments to prove the analyticity of the family of functions F • s (x) with respect to s in this strip.

Proposition I. 6 .

 6 Let u * be such that |u * | = u c and |r(u * )| < r(u c ). Then, r(u) admits an analytic continuation in a neighborhood of u * .

(I. 16

 16 ) φ(r) = r -k≥1 2k -1 k g 2k + nh 4k ψ k (r) r kvalid for r in the closure of the domain (I.17)D = {r(u) | |u| < u c }.The convergence of the sum in the right-hand side of (I.[START_REF] Borot | Formal multidimensional integrals, stuffed maps, and topological recursion[END_REF]) is normal, and therefore (by Cauchy's integral formula) we may differentiate the relation at every point inside D. We may rearrange the result in the form(I.18) 1 -A(r) = B(r)φ ′ (r), A(r) := k≥1 k 2k-1 k g 2k + nh 4k ψ k (r) r k-1 , B(r) := 1 + n k≥1 2k-1 k h 4k ψ ′ k (r)φ ′ (r) r k .

1 2 1 - 16h 2 r 1 -

 111 1 h(α+1) ). By comparing with the definition of m, p in (B.1)-(B.11), it means that m and p as functions on Y avoid the values 0 and ∞. As a result, the only problem that could be met in continuing analytically (q , w ∞ ) occurs on the intersection of the locus m = 1 with Y. In fact, substituting γ ± = s + 2 √ r into the definition (B.1) of m, we have m = 2hαs + h 2 (4rs 2 )(1α 2 ) 2 .

,

  which does not vanish identically. □

  On the other hand, in N we may bound the derivatives ∂ u F ℓ and ∂ g 1 F ℓ by their values at (|u * |, |g * 1 |) which, by Propositions 4.6 and 4.7, are finite and grow as O (γ * + ) ℓ for ℓ → ∞. By (H.8), we deduce that ℓ≥0A k,ℓ ∂ u F ℓ and ℓ≥0 A k,ℓ ∂ g 1 F ℓ are O (γ * + ) -k . As Q k-1 and P k-1 are O(γ k ), with γ = |s * | + 2 |r * | < γ *

  Euclidean geometry to Liouville quantum gravity, holds for any large deviations problem, where the large deviations function is the Legendre-Fenchel transform of a certain generating function Λ.

	9.3.4. Comparison to Theorem 2.2. Let us finally compute explicitly the Liouville large
	deviations function Θ, in order to compare with the main results above regarding extreme
	nesting in the O(n) model on a random planar map. The easiest way is to rewrite (9.3)
	as
	(9.37)

  1 2 A k,k ′ γ k+k ′ ≥0 A k,k ′ γ k+k ′ +. The fact that these are indeed probabilities is ensured by the following lemma, whose proof is postponed to the end of the section.

		+	, and
	otherwise remains trapped at -k with probability 1 -1 2 k ′ Lemma H.3. For any admissible weight sequence satisfying (H.1), we have
	(H.7)	γ + ≤ γ *

+

where γ * = 1 h(α+1) is as in (6.1), and we have (H.8)

Our definition for A differs by a factor of n/x from the corresponding A in[START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF].

To be precise, we compute here the behavior of the singular part of F • s (x), i.e., we did not include the shift in (5.27), as it will always give zero when performing a contour integral against x L around the cut.

I.e., it still yields a negligible term as compared to the previous ones.

The fact that critical exponents for cylinders taking into account the number of separating loops are obtained by replacing b with b(s) can be observed indirectly in [101, Section 4.2], with the momentum p playing the role of b(s).

Note that q here is a parameter with the same status as p, and does not refer to the elliptic nome controlling e.g. in Theorem

[START_REF] Astala | Random conformal weldings[END_REF].3 the distance to criticality. As the context of their apparition is quite different, it should not lead to confusion.

Again, q here is not the variable of Theorem 6.3 controlling the distance to criticality.

, w * ∞ ) was singular at α → 1, this rule of thumb should not be used blindly. It gives correctly the constants in the above Lemmata that have a finite limit under this limiting procedure. But, for instance, it is meaningless for the second line of (B.20), due to the particular way we defined γ * -for α ̸ = 1.

+ n + 2ρ(1b) √ 2n -2 √ 2 + n -ρ 2 b(1b 2 ) √ 2 + n + 4ρ(1b 2 ) √ 2n -6b √ 2 + n .

Note that k∈Z ν(k) = 1 γ+ (2F(γ + ) + k≥1 G k γ k-1+ ) is indeed equal to 1, by taking x → γ + in (4.8).

program "Random Geometry" supported by EPSRC Grant Number EP/K032208/ (G.B. and B.D.), and from the Max-Planck-Institut für Mathematik in Bonn Bonn (J.B. and B.D.). We acknowledge financial support from the following institutions: the Simons Foundation (G.B. and B.D.); the Max-Planck Gesellschaft (G.B.); the Agence Nationale de la Recherche via the grants ANR-12-JS02-001-01 "Cartaplus" (J.B.) and ANR-14-CE25-0014 "GRAAL" (J.B. and B.D.); the City of Paris through the project "Combinatoire à Paris" (J.B.); the CNRS Projet international de coopération scientifique (PICS) "Conformal Liouville Quantum Gravity" n o PICS06769 (B.D.). This work was started while G.B. was affiliated with MIT Mathematics Department, and mainly conducted during his affiliation with the Max-Planck-Institut für Mathematik in Bonn.

Appendix A. Theta function

For properties of elliptic functions, we refer to [START_REF] Guo | Special functions[END_REF]. Let τ be a complex number in the upper-half plane. The Jacobi theta function is the entire function of v ∈ C defined by: (A.1)

2 ) 2 +iπ(v+ 1 2 )(2m+1) .

Its main properties are:

and the effect of the modular transformation:

We will also meet two other Jacobi theta functions In this section, we consider α, h fixed and γ -, γ + as varying complex parameters. The purpose of this section is to introduce a real-analytic change of variable (Lemma B.3) which will turn handy in the study the critical limit; and, to show that it can be promoted to an analytic change of variables for complex parameters. As we are primarily interested in the neighboorhood of γ + = γ * + , we do not attempt to describe the largest possible domain of analyticity. The information gained will also serve in Appendix J.

We define

and introduce the domains

We clearly have A R ⊂ A. We shall denote B(z; r) ⊂ C the open ball of radius r centered at z.

B.1.

Formulas in A R . We first assume that (γ -, γ + ) ∈ A R , and set

dy (yς(γ -))(yς(γ + ))(yγ + )(yγ -) .

The normalising constant is chosen such that, for x moving from the origin ς(γ + ) to ς(γ -) with a small negative imaginary part, v is moving from 0 to 1 2 . When x moves on the Using (B.11) and trigonometric identities, we find equivalently

where we recall that γ * -is the function of p coming from the specialisation of χ -1 at m = 0. Equation (B.18) uniquely determines w * ∞ ∈ (0, 1). We can also see w * ∞ as a function of (γ -, γ + ) ∈ A R by first applying the map χ : (γ -, γ + ) → (m, p).

An important role in our analysis will be played by the elliptic nome (B. [START_REF] Borot | Loop models on random maps via nested loops: case of domain symmetry breaking and application to the Potts model[END_REF])

is analytic in U, has image V and admits an analytic inverse on the domain V. Besides, we have when

2 ),

Proof. The elliptic nome q

is an analytic function of m ∈ B(0; 1) \ (-1, 0]. For later use, we record that (B. [START_REF] Borot | Abstract loop equations, topological recursion, and applications[END_REF])

Since the analytic continuation of the elliptic integral has the property that for m ∈ (-1, 0), Im(K(1m ± i0)) = ∓K(m), there is in fact no discontinuity across (-1, 0). Together with (B.21), this implies that q 1 2 is an analytic function of m ∈ B(0; 1), and its image Q is a neighborhood of 0. In fact, it is not hard to show that Q ⊆ B(0; 1). A converse identity is known

4

, involving the Jacobi theta functions defined in (A.3), showing that m → q 1 2 admits an analytic inverse map q 1 2 → m defined at least on the domain q The coefficients gk have been defined in (5.16) and a priori depend on the parameters of the model: g (resp. h) the weight per face not visited (resp. visited) by a loop, α the bending energy, n the weight per loop, and the weight u per vertex (when not set equal to 1). We again recall that the latter determine γ -, γ + in a way analysed later in Appendix E. For the moment, considering γ -, γ + -or equivalently (q

as variables, we can compute the gk using Lemma B.1. Namely, if we introduce gk = (iC) k g k , we find

We remark that g 3 and g 0 are constants (depending on the parameters of the model) with respect to the variables (γ -, γ + ). We can deduce the analyticity properties and q → 0 expansion of g 1 , g 2 thanks to Lemma B.5 or B.8.

The last expression in (D.1) is convenient to study the regime q

We have, for b ∈ (0, 1):

The errors are uniform for w in any compact independent of τ → 0, and the expressions for the limit functions are:

Proof. This is obtained by isolating carefully the terms dominating the q-series defining the theta functions that appear in the last line of (D.1). □

Appendix E. The phase diagram and volume exponent

The parameters of the model α, g, h, n, u determine γ -, γ + through the equations

2 + τ w ∞ and gk = (iC) k g k and according to Theorem 5.3, these equations take the form:

2 ). In light of Lemma B.3 for α ̸ = 1, for η small enough the equation (E.1) for ε = 0 determines a function (q

If α = 1 and in view of Lemma B.7, it determines likewise an analytic function (q

Proof. We first discuss α ̸ = 1. From Lemmata B.3 and B.5, w ∞ , ( g k ) 3 k=1 and πC T are analytic functions of (q

for η small enough. Taking into account Remark D.1 and the fact that the argument of Υ b always avoids the poles of v → Υ b (v), we deduce that the left-hand side of (E.1) with ε = 1 2ε = 1 2 is an analytic function of (q

by taking the limit (B.40) and yields (F.12)

,

where one substitute the value of h 2 on the critical line given in (E.4). Then using q ∼ 1-u ∆ c and transfer theorems, we deduce from (F.10) the large volume asymptotics stated in Corollary 6.6.

The parameter b appears in two ways in the previous computation: firstly via the value of c (coming from the critical behavior of γ according to Theorem 6.3), and secondly via the value n = 2 cos(πb) in the functional relation. If we substitute in this second dependence b → 1 2 but keep the first dependence unchanged, we obtain the generating series of disks with a marked point in the gasket:

, where one should still use (E.6) for h 2 . For α = 1 this is (F.15)

where one should still use (E.4) for h 2 . By transfer theorems, (F.13) implies the large volume asymptotics stated in Corollary 6.7.

Appendix G. Scaling limits for cylinder generating series

We distinguish whether the variable x i coupled to the perimeter of the i-th boundary is away from γ * + -in which case the perimeter remains typically finite -or close to γ * + at scale O(q

2 ) -in which case the perimeter typically diverges.

G.1. Refined cylinders: finite/finite. This is governed by the regime x i = x 1 2 + τ w i ), and leads to:

where:

Appendix H. Admissibility vs. finiteness in the bending energy model

In this appendix, we consider the bending energy model, as defined in Section 2.1.2. It depends on the parameters n, g, h and α, see again Figure 2 (the vertex weight u is set to 1). The corresponding generating series of annuli A k,ℓ (n, h, α) are given by (4.5), (5.1) and (5.2). Recall also the definition of admissibility for a sequence of face weights (g k ) k≥1 given in Section 4.2. Then, we have the following analogue of [32, Theorem 1]: Theorem H.1. For n ∈ (0, 2) and g, h, α ≥ 0, the bending energy model with parameters (n, g, h, α) is well defined (i.e., the partition function F ℓ (n, g, h, α) is finite for all ℓ) if and only if there exists an admissible weight sequence (G k ) k≥1 such that

In that case, we have F ℓ (n, g, h, α) = F ℓ (G 1 , G 2 , . . .), and the expected number of vertices in a disk of perimeter ℓ is finite.

The case α = 1 is established in [START_REF] Korzhenkova | The exploration process of critical Boltzmann planar maps decorated by a triangular O(n) loop model[END_REF]. We now explain how to prove the result for general α by adapting the strategy given in [START_REF] Budd | The peeling process on random planar maps coupled to an O(n) loop model (with an appendix by L. Chen[END_REF]. We will heavily use the notions of this paper, as well as those of [START_REF] Budd | The peeling process of infinite Boltzmann planar maps[END_REF]. The reader is invited to consult these references for more details. The proof does not depend on the specific form of g k , the only important assumption being that it is nonnegative for all k. Therefore, Theorem H.1 remains valid for a more general model in which we allow for unvisited faces of arbitrary degrees. Our proof however depends on the specific form of A k,k ′ in the bending energy model, precisely within the proof of Lemma H.3 below. We also assume that n < 2, but we believe the case n = 2 could be included as well by a slight adaptation.

The core idea is to use the peeling exploration of loop-decorated maps, as defined in [32, Sections 2 and 3]. There are actually two types of peeling explorations: untargeted peeling, which applies to disks, and targeted peeling, which applies to pointed disks. Their definitions are adapted straightforwardly to the bending energy model, with the following modifications:

• since the maps are no longer assumed bipartite, we should keep track of perimeters rather than half-perimeters, • since the model is not rigid, annuli (rings) may have different outer and inner perimeters. For these reasons, we now encounter the following possible events in untargeted peeling:

• C k : discovering a new (unvisited) face of degree k ≥ 1 (when considering triangulations, only C 3 may occur, but the arguments allow for unvisited faces of arbitrary degrees), • G k 1 ,k 2 : splitting a hole of degree k 1 + k 2 + 2 into two holes of degrees k 1 and k 2 , by identifying two active edges incident to it, • L k,k ′ : discovering an annulus with outer perimeter k ≥ 1 and inner perimeter k ′ ≥ 0.

The analogous events in targeted peeling are easy to deduce, but we do not enter into details here since we only allude to targeted peeling in Remark H.5.

Assuming that the model is well-defined, the probabilities of these events when peeling an active edge incident to a hole of degree ℓ ≥ 1 are given by

If we instead assume that (H.1) is satisfied for an admissible weight sequence (G k ) k≥1 , then we follow the strategy of [32, Section 5] and define the probabilities of these events by the putative expressions

where ν is the probability measure 7 on Z corresponding to the admissible weight sequence

and γ + = lim k→∞ (F k ) 1 k (the limit exists for any admissible weight sequence). Following the same reasoning as in [32, p. 29], we see that the quantities appearing in (H.3) are nonnegative and add up to one, which allows to interpret them as probabilities. Then, we have the analogue of [32, Proposition 8 and Lemma 5]: Proposition H.2. Consider an admissible weight sequence satisfying (H.1). If we construct a random loop-decorated map via the untargeted peeling algorithm with the event probabilities (H.3), then the algorithm terminates almost surely, and produces a sample of the bending energy model with parameters (n, g, h, α).

The proof of this proposition again follows Budd's steps. The most delicate point is the termination of the algorithm, which comes from a martingale argument. To a map M with holes of degrees k 1 , k 2 , . . . and with N vertices not incident to a hole, we assign the quantity (H.5)

where we sum over all holes, and where the function h ↓ is yet unspecified. Mimicking the proof of [START_REF] Budd | The peeling process on random planar maps coupled to an O(n) loop model (with an appendix by L. Chen[END_REF]Lemma 4], we see that V defines a martingale for the untargeted peeling

Proof of Lemma H.3. Let us prove that γ + ≤ γ * + . We first establish a lower bound for G k , namely that G k ≥ ς(β) -k for any β ∈ (0, γ + ) and k large enough. Here, ς is the rational involution defined by (5.2).

Fix some β ∈ (0, γ + ) and consider m such that

We may estimate both sums in the right-hand side using the explicit form (5.1) of the generating A(x, z), or alternatively the combinatorial arguments of [START_REF] Borot | More on the O(n) model on random maps via nested loops: loops with bending energy[END_REF]Section 3.2]. We find

where the second estimate follows from the expression (H.12)

hα . This establishes the wanted lower bound. On the other hand, the fact that (H.4) defines a probability distribution entails that lim k→∞ G k γ k + = 0. We conclude that ς(γ + ) ≥ γ + , hence γ + is smaller than or equal to the positive fixed point γ * + = 1 h(α+1) of the decreasing involution ς. Finally, the identity (H.8) is another consequence of (H.11), which was in fact valid for all β ≥ 0 hence for β = γ * + . □ Appendix I. On the rigid O(n) loop model on bipartite maps

In this appendix, we consider the rigid O(n) loop model, introduced originally in [17] in the case where the underlying map is a quadrangulation, and generalised in [START_REF] Budd | The peeling process on random planar maps coupled to an O(n) loop model (with an appendix by L. Chen[END_REF] by allowing the unvisited faces to have arbitrary even degrees. In all cases, the faces visited by loops are always quadrangles, and the rigidity constraint entails that, in each visited quadrangle, the loop enters and exits through opposite edges. This greatly simplifies the nested loop approach for the two following reasons.

• The annuli always have equal inner and outer perimeters hence the generating series A k,k ′ vanishes unless k = k ′ . Therefore, the fixed point equation (3.2) is simpler, as well as many related arguments. • It is well-known that working with bipartite maps makes life easier.

The rigid loop model may actually be viewed as a limit of the bending energy model: contemplating again Figure 2, we see that for α = 0 the visited triangles always come top to tail by pairs, and may therefore be merged in quadrangles satisfying the rigidity constraint. Note however that, in our computations, we assume that the unvisited faces are triangles, hence the underlying map is not necessarily bipartite. As pointed out in Appendix H, we could generalise the model by allowing the unvisited faces to have arbitrary degrees, which does not affect the validity of the nested loop approach, and then we could constrain the degrees to be even to recover precisely the model of [START_REF] Budd | The peeling process on random planar maps coupled to an O(n) loop model (with an appendix by L. Chen[END_REF] for For this, we observe that

are both series in u with nonnegative coefficients. Let r c = r(u c ). Since φ, A, B are all strictly increasing functions on the real interval (0, r c ), we see that 1 -A cannot vanish, and therefore A(r c ) ≤ 1. Thus, for r → r * , A(r) tends to a limit A(r * ) of modulus strictly smaller than 1, and 1 -A(r * ) is nonzero.

On the other hand, by Proposition 4.7 -or directly (I.8) in the non generic critical case -we know that F ′ 2k (u c ) is finite and grows as (4r c ) k for k → ∞. Thus, as r tends to r * in D, B(r) tends to a finite limit B(r * ) since 16h 4 (r c r * ) 2 < 1. Thus, φ ′ (r * ) ̸ = 0 as wanted.

□

We finish with the analysis of generic singularities.

Proposition I.7. If r(u c ) < 1 4h 2 , then r(u) is delta-analytic locally at u c . More precisely, there exists δ > 0 such that r(u) admits in the slit disk {|uu c | < δ, arg(uu c ) ̸ = 0} an analytic continuation of the form r(u c )r( √ u cu), with r analytic.

In other words, r(u) has a square root type singularity, and the volume exponent is that of pure gravity, as expected.

Proof. We will reuse ideas and notations from the proof of Proposition I.6. Since φ is analytic at r c , we must have φ ′ (r c ) = 0, as otherwise r(u) could be analytically continued at u c , contradicting Pringsheim's theorem [START_REF] Flajolet | Analytic combinatorics[END_REF]Theorem IV.6]. By differentiating (I.18), we get

By the same arguments as before, since 16h 4 r 4 c < 1, B(r) tends for r → r c to a finite limit, which is now manifestly positive. We also have A ′ (r c ) and B ′ (r c ) positive (the latter possibly infinite), thus φ ′′ (r c ) < 0 (this quantity being necessarily finite by analyticity of φ at r c ).

Let us define φ(x) = φ(rc)-φ(rc-x)

. It is analytic at x = 0 and φ(0) = -φ ′′ (rc) 2 is positive.

Thus, φ(x) is analytic and nonzero at x = 0 (we pick the principal branch of the square root). By the inverse function theorem, x → x φ(x) admits an inverse r locally around zero. The function u → r cr √ u cu is the analytic continuation we are looking for, since it coincides with r(u) on an interval (u cδ, u c ). □ Appendix J. Delta-analyticity in the bending energy model

The purpose of this appendix is to establish an analogue of Proposition I.6 in the more general case of the bending energy model. Our proof works in the even more general setting where we allow for unvisited faces of arbitrary degrees. The parameters are then the weight per loop n, the weight per visited triangle h, the bending energy factor α, the where G k (u, g 1 ) are the renormalised face weights given of (3.2). To connect with [18, Equation (6.7)], note that Q k-1 (r, s) = 1 2 (P k (r, s) -sP k-1 (r, s)). We give the following analog of Proposition I.6, which due to the previous remarks proves Theorem J.1.

Proposition J.2. Let (u * , g * 1 ) be a point on the boundary of B such that |r(u * , g * 1 )| < r(|u * |, |g * 1 |). Then, r, s and F ℓ (ℓ > 0) all admit an analytic continuation in a neighborhood of (u * , g * 1 ). The only way for the condition |r(u * , g * 1 )| < r(|u * |, |g * 1 |) not to be satisfied is to have u * and g * 1 both real and positive, or some periodicity phenomenon to occur: it may be seen that this only happens for the situation already discussed in Appendix I.2, namely u * negative, α = 0, g * 1 = 0 and g k = 0 for k ̸ = 2 mod 4. As here α > 0, there are no non-vanishing conditions on g k in Theorem J.1. Before proving Proposition J.2, we first state the analog of Proposition I.5 -recall that γ * + = 1 h(α+1) . Proposition J.3. There exists functions φ(r, s) and ψ ℓ (r, s) (ℓ > 0) which are meromorphic in a domain containing Y = (r, s) ∈ C 2 | |s| + 2 |r| < γ * + and such that, for (u, g 1 ) ∈ B,

The set of poles of ψ ℓ is included in that of φ.

Proof of Proposition J.3. We shall use the exact solution of the model, in particular Theorem 5.3. The vanishing conditions G(τ ) = G(τ + 1 2 ) = 0 form a 2 × 2 linear system for u and g 1 , namely

where we set f (v) := Υ b (v) + Υ b (-v), we have used Lemma B.1, and • • • are functions of the fixed parameters (g k ) k≥2 , n, h, α and γ -, γ + . More precisely, according to Lemma E.1 the coefficients in these equations are analytic functions of γ -, γ + (hence of r, s) such that (q 1 2 , w ∞ ) belongs to V ′′ (0). We explain in the next paragraph that they can in fact analytically continue to a larger domain containing Y. The matrix of this 2 × 2 system reads, up to multiplication of each column by a non-vanishing prefactor:

Due to the previous discussion, det(D) is an analytic function of (r, s) ∈ Y. We will justify at the end of the proof that it is not identically zero. Therefore, the system for u, g 1 has a solution which is a meromorphic function of γ -, γ + (zeroes of det(D) may create poles on a divisor). The rest of the proof is then similar to that of Proposition I.5 and thus omitted.

To show analytic continuation to Y, we first discuss the case α ̸ = 1. It is not hard to check that there exists analytic continuations for Υ (l) b (v ∞ + ε) for ε ∈ {0, 1 2 } and l ∈ N, as functions of (q 1 2 , w ∞ ) across the q 1 2 -negative real axis. Therefore, it is enough to discuss the analyticity and analytic continuation of (q 1 2 , w ∞ ) seen as a function of (γ -, γ + ). For the latter, can perform analytic continuation across the branch cuts on the loci m ∈ (1, +∞) Email address: jeremie.bouttier@ipht.fr Université Paris-Saclay, CNRS, CEA, Institut de physique théorique, 91191 Gif-sur-Yvette, France.

Email address: bertrand.duplantier@ipht.fr