Olivier Devillers

Charles Duménil

A Poisson sample of a smooth surface is a good sample

Keywords: 3D reconstruction, probabilistic analysis, point sampling Reconstruction de surface, analyse probabiliste, échantillon de points

. Using this result, we prove that when points are Poisson distributed on a surface under the same hypothesis, with intensity λ, the expected size is O(λ log 2 λ).

Introduction

While the complexity of the Delaunay triangulation of n points is strictly controlled in two dimensions to be between n and 2n triangles (depending on the size of the convex hull) the gap between the lower and upper bound ranges from linear to quadratic in dimension 3. The worst case is obtained using points on the moment curve 1 and the best case by using the center of spheres defining a packing. 2 Two relations connect the number of faces of different dimensions: the Euler relation says that the sum of the number of vertices and triangles is equal to the sum of the number of edges and tetrahedra, and counting the number of triangle-tetrahedra incidences yields that the number of tetrahedra is twice the number of triangles. Altogether, for a fixed number of vertices counting the number of edges, triangles, or tetrahedra are equivalent.

To get a more precise result on the size of the 3D Delaunay triangulation, it is possible to make different kinds of hypotheses on the point set. A first possibility is to assume a random distribution in 3D and if the points are evenly distributed, Dwyer proved that the expected size is Θ(n) [START_REF] Dwyer | The expected number of k-faces of a Voronoi diagram[END_REF]. But this hypothesis of random distribution is not relevant for all applications, for example when dealing with 3D reconstruction the Delaunay triangulation is an essential tool and it is much more natural to assume that the points are not distributed in space but on a surface [START_REF] Cazals | Delaunay triangulation based surface reconstruction[END_REF]. If the points are evenly distributed on the boundary of a polyhedron, the expected size was proved to be Θ(n) in the convex case [START_REF] Golin | On the average complexity of 3d-Voronoi diagrams of random points on convex polytopes[END_REF] and between Ω(n) and O(n log n) in the non convex case by Golin and Na [START_REF] Golin | The probabilistic complexity of the Voronoi diagram of points on a polyhedron[END_REF].

Instead of using probabilistic hypotheses one can assume that the points are a good sampling of the surface, namely an ( , η)-sample where any ball of radius centered on the surface contains at least one and at most η points of the point-set. Under such hypothesis Attali and Boissonnat proved that the complexity of the Delaunay triangulation of a polyhedron is linear [START_REF] Attali | A linear bound on the complexity of the Delaunay triangulation of points on polyhedral surfaces[END_REF]. Attali, Boissonnat, and Lieutier extend this result to smooth surfaces verifying some genericity hypotheses with an upper bound of O(n log n) [START_REF] Attali | Complexity of the Delaunay triangulation of points on surfaces: The smooth case[END_REF]. The genericity hypothesis is crucial since Erickson proved that there exists good sample of a cylinder with a triangulation of size Ω(n √ n) [START_REF] Erickson | Dense point sets have sparse Delaunay triangulations or ". . . but not too nasty[END_REF]. This example by Erickson arrange the point set in a very special position on an helix, nevertheless, even with an unstructured point set it is possible to reach a supra-linear triangulation since Erickson, Devillers, and Goaoc proved that the triangulation of points evenly distributed on a cylinder has expected size Θ(n log n) [START_REF] Devillers | Empty-ellipse graphs[END_REF].

Contribution In this paper we prove that a Poisson sample of intensity λ on a smooth surface of finite area is an (ε, η)-sample for ε = 3 log λ λ and η = 1000 log λ with high probability. Using the result of Attali, Boissonnat, and Lieutier, it yields that the complexity of the Delaunay triangulation of a Poisson sample of a generic surface is O(λ log 2 λ) loosing an extra logarithmic factor with respect to the case of good sampling (see Section 3).

Notations, definitions, previous results

We consider a surface Σ embedded in R 3 , compact, smooth, oriented and without boundary. At a point p ∈ Σ, for a given orientation, we denote by κ 1 (p) and κ 2 (p) the principal curvatures at p with κ 1 (p) > κ 2 (p). We assume that the curvature is bounded and define κ sup = sup p∈Σ max(|κ 1 (p)|, |κ 2 (p)|). We denote by σ(c, R) the sphere of center p and radius R. We denote by B(σ) the closed ball whose boundary is the sphere σ, by E the interior of a set E and, for p ∈ Σ, by D(p, R) the intersection between Σ and the B(p, R). Abusively we call D(p, R) a disk. For a discrete set X, we denote (X) the cardinality of X. If X is a set of points, Del (X) denotes the Delaunay triangulation of X. In the 3D case, (Del (X)) is the sum of the number of tetrahedra, triangles, edges and vertices belonging to the Delaunay triangulation. Definition 1. We say that a set of points X is a spatial Poisson process, or Poisson sample, over E if, for all bounded regions A ⊂ E measurable, the random variable (X ∩ A) has a Poisson distribution.

Without loss of generality, we assume that Area (Σ) = 1 and consider X as a Poisson sample over Σ of intensity λ > 0.

We recall classical properties of a Poisson sample:

Proposition 2. For two regions R and R of Σ,

• P [ (X ∩ R) = k] = (λ Area(R)) k k! e -λ Area(R) , in particular: P [ (X ∩ R) = 0] = e -λ Area(R) , • E [ (X ∩ R)] = λ Area (R) • R ∩ R = ∅ ⇒ (X ∩ R) and (X ∩ R ) are independent random variables.
We consider the same definition of genericity as Attali, Boissonnat and Lieutier, roughtly: the set of points where one of the principal curvatures is locally maximal is a finite set of curves whose total length is bounded, and, the number of contacts of a medial ball with the surface is uniformly bounded by a constant.

Then we define what is a good-sampling of a surface and precise the result by Attali, Boissonnat and Lieutier.

Definition 3 (Good sample). A point-set included in a surface is a ( , η)-sample if any ball of radius centered on the surface contains at least one and at most η points of the sample.

Theorem 4 ([2]

). The 3D Delaunay triangulation of an ( , η) sample of a generic smooth surface has complexity O η 2 2 log 1 .

Proof. Looking more carefully at the result of Attali et al. [2, Eq.( 14)], we notice that the actual complexity is smaller than C( η ε ) 2 log(ε -1 ) for C being a constant of the surface.

3 Is a random sample a good sample?

In a Poisson sampling of intensity λ on the surface, voids and accumulations of points may appear, thus such a sample is likely not to be a good sample with ε 2 = 1 λ and η constant. Nevertheless, it is possible to not consider η as a constant, namely, we take η = Θ(log(λ))

In a first lemma, we bound the area of D(p, R), for any p ∈ Σ and R > 0 sufficiently small. Lemma 5. Let Σ be a smooth surface of curvature bounded by κ sup , and consider p ∈ Σ and R > 0 smaller than 1 κsup . The area of D(p, R) is greater than 3 4 πR 2 .

Inria

Proof. The bound is obtained by considering the fact that the surface must stay in between the two tangent spheres of curvature κ sup tangent to the surface at p. The tangent disk at p of radius

√ 3 2 R > √ 3 2 1
κsup is uncluded in the projection of D(p, r) on the tangent plane and thus has a smaller area than D(p, R). Lemma 6. Let Σ be a C 3 surface of curvature bounded by κ sup . For R small enough, Area(D(p, R)) < 5 4 πR 2 . Proof. Let z = f (x, y) := 1 2 κ 1 x 2 + 1 2 κ 2 y 2 + O(x 3 + y 3 ) be the Monge patch [START_REF] Peter W Hallinan | Two-and three-dimensional patterns of the face[END_REF] at a point p on Σ. We denote by dσ an element of surface and by A(p, R) the projection of D(p, R) on the xy-plane, since on D(p, R) the slope of the normal to Σ is bounded, we have:

Area(D(p, R)) = D(p,R) dσ = A(p,R) 1 + ( ∂f ∂x (x, y)) 2 + ( ∂f ∂y (x, y)) 2 dxdy
That is smaller than

x 2 +y 2 ≤R 2 1 + ( ∂f ∂x (x, y)) 2 + ( ∂f ∂y (x, y)) 2 dxdy, since D(p, R) ⊂ B(p, R). Since f is C 3 and ∂f ∂x (x, y) ∼ κ 1 x
, we can say that there exists a neighborhood of p on which

| ∂f ∂x | ≤ √ 2κ 1 |x| ≤ √ 2κ sup |x|, i.e., ∂f ∂x 2 ≤ 2(κ sup x) 2 .
Applying the same for y, and turning to polar coordinates, we get:

Area(D(p, R)) ≤ 2π θ=0 R r=0 r 1 + 2(rκ sup ) 2 drdθ = π 3 (2(Rκ sup ) 2 + 1) 3 2 -1 κ 2 sup
Noticing that (a + 1)

3 2 -1 = a a+ √ a+1+2 √ a+1+1 ≤ 15
8 a for a < 1, we can conclude that for any R small enough,

Area(D(p, R)) ≤ π 3 15 4 (Rκ sup ) 2 κ 2 sup = 5 4 πR 2 . Lemma 7. Let Σ be a C 3 surface with Area(Σ) = 1. Let M R be a maximal set of k R disjoint disks D(p i , R) on Σ. If R is small enough then k R ≤ 4 3πR 2 .
Proof. Thanks to lemma 5, for R small enough, we have D(p, R) ≥ 3 4 πR 2 . Thus:

k R • 3 4 πR 2 ≤ i=k R i=1 Area (D(p i , R)) ≤ Area (Σ) = 1,
and we can deduce the following bound: k R ≤ 4 3πR 2 . Lemma 8. Let X be a Poisson sample of intensity λ distributed on a C 3 smooth closed surface Σ of area 1. If λ is large enough, the probability that there exists p ∈ Σ such that D p, 3 log λ λ does not contain any point of X is O(λ -2 ).

Proof. We prove that a Poisson sample has no void of radius 3 log λ λ with probability O(λ -2 ). In a first part we use a packing argument. On the one hand, for any ε > 0 small enough and given a maximal set M ε/3 and any point p ∈ Σ, the disk D(p, ε) contains entirely one of the disks

D(p i , ε
3 ) belonging to M ε/3 . Indeed, by maximality of M ε/3 , the disk D(p, ε/3) intersects a disk of M ε/3 whose diameter is 2ε/3 so D(p, ε) contains it entirely. On the other hand, remember from lemma 6 that if ε is small enough then Area(D(p, R)) ≤ 4 3 πR 2 . Then we can bound the probability of existence of an empty disk for ε small enough:

P [∃p ∈ Σ, (X ∩ D(p, ε)) = 0] ≤ P ∃i < k ε/3 , (X ∩ D(p i , ε/3)) = 0 ≤ k ε/3 P [ (X ∩ D(c, ε/3)) = 0] for a point c on Σ ≤ 4 3π(ε/3) 2 e -λ 4 3 π( ε 3 ) 2 = 12
πε 2 e -λ 4πε 2 27 .

By taking ε = 3 log λ λ we get:

P ∃p ∈ Σ, X ∩ D(p, 3 log λ λ ) = 0 ≤ 12λ 9π log λ e -4 * 9π log λ 27 = O(λ -2 ).
We have proved that when a Poisson sample is distributed on a surface, the points cover sufficiently the surface, i.e., there is no large empty disk on the surface with high probability. Now we have to verify the other property of a good sample, namely, a Poisson sample does not create large concentration of points in a small area. Lemma 9. Let X be a Poisson sample of intensity λ distributed on a C 3 closed surface of area 1. If λ is large enough, the probability that there exists p ∈ Σ such that D(p, 3 log λ λ ) contains more that 1000 log(λ) points of X is O(λ -2 ).

Proof. Consider a M ε maximal set, we can notice that for any p ∈ Σ, the disk D(p, ε) with p ∈ Σ is entirely contained in one disk D(p i , 3ε) that is an augmented disk of M ε . Indeed, by maximality of M ε , the disk D(p, ε) intersects a disk from M ε say D(p j , ε) so D(p j , 3ε) contains entirely D(p, ε).

Then we can bound the probability of existence of a disk containing more than η points:

P [∃p ∈ Σ, (X ∩ D(p, ε)) > η] ≤ P [∃i < k ε , (X ∩ D(p i , 3ε)) > η] ≤ k ε P [ (X ∩ D(c, 3ε)) > η] for a point c on Σ ≤ 4 3πε 2 P [ (X ∩ D(c, 3ε)) > η]
We use a Chernoff inequality [START_REF] Mitzenmacher | Probability and computing: Randomized algorithms and probabilistic analysis[END_REF]

to bound P [ (X ∩ D(c, 3ε)) > η]: If V follows a Poisson law of mean v 0 , then ∀v > v 0 , P (V > v) ≤ e v-v0 ( v 0 v ) v .
From lemmas 5 and 6, we have that: Proof. Given a Poisson sample X we distinguish two cases:

• If X is a good sample, i.e., an (ε, η)-sample with ε = 3 log λ λ and η = 1000 log λ, we apply Attali et al. result and get a complexity bounded by ( η ε ) 2 log(ε -1 ) up to a constant that is O(λ log 2 λ).

• If X is not a good sample, which arises with small probability by Lemma 10, we bound the triangulation size by the quadratic bound:

k∈N k 2 P [ (X) = k] = k∈N k 2 λ k k! e -λ = λ ∞ k=1 k λ k-1 (k -1)! e -λ = λ ∞ k=1 (k -1) λ k-1 (k -1)! e -λ + ∞ k=1 λ k-1 (k -1)! e -λ = λ λ ∞ k=2 λ k-2 (k -2)! e -λ + 1 = λ(λ + 1) = O(λ 2 ) RR n°9239

27 4 πε 2 ≤

 2 Area(D(c, 3ε)) ≤ 45 4 πε 2 for ε small enough. Consequently we can say that the expected number of points v 0 in D(c, 3ε) verifies 27 4 λπε 2 ≤ v 0 ≤ 45 4 λπε 2 . Then we apply the above Chernoff bound with v = 45 4 eπλε 2 ( chosen for the convenience of the calculus) Inria Theorem 11. For λ great enough, the Delaunay triangulation of a point set Poisson distributed with intensity λ on a closed smooth generic surface of area 1 has O(λ log 2 λ) expected size.

The moment curve is parameterized by (t, t

, t

). When computing the Delaunay triangulation of points on this curve, any pair of points define a Delaunay edge.[START_REF] Attali | Complexity of the Delaunay triangulation of points on surfaces: The smooth case[END_REF] The kissing number in 3D is 12, thus in such a point set, the number of edges is almost 6n.RR n°9239

RR n°9239

Funded by grant ANR-17-CE40-0017 of the French National Research Agency (ANR project ASPAG). .

So for ε = 3 log λ λ and η = 45 4 eπλε 2 = 405 4 eπ log λ, we have:

Since 405 4 eπ < 1000, it is sufficient for our purpose to say:

Theorem 10. On a C 3 closed surface, a Poisson sample of intensity λ large enough is a

Proof. From lemmas 8 and 9, we have that a Poisson sample is not a (3 log λ λ , 1000 log λ)-sample with probability O(λ -2 ).


Jiao He

IFTIMIE And Dragos

ON THE SMALL RIGID BODY LIMIT IN 3D INCOMPRESSIBLE FLOWS

We consider the evolution of a small rigid body in an incompressible viscous fluid filling the whole space R 3 . The motion of the fluid is modelled by the Navier-Stokes equations, whereas the motion of the rigid body is described by the conservation law of linear and angular momentum. Under the assumption that the diameter of the rigid body tends to zero and that the density of the rigid body goes to infinity, we prove that the solution of the fluid-rigid body system converges to a solution of the Navier-Stokes equations in the full space without rigid body.

Introduction and Statement of results

The motion of one or several rigid bodies in a liquid is a classical topic in fluid mechanics. We consider here the motion of an incompressible viscous fluid and a small smooth moving rigid body in the three-dimensional space. In this fluid-rigid body system, we will not take into account the gravity, and we suppose that the rigid body moves under the influence of the fluid. We study the asymptotic behavior of the fluid-rigid body system as the diameter of the rigid body tends to zero.

Assume that the whole three-dimensional space is occupied by an incompressible viscous fluid of viscosity ν > 0 and by a rigid body of size ε. At the initial time, the domain of the rigid body S ε 0 is a small non-empty smooth compact simply-connected subset of R 3 included in the ball B(0, ε) and F ε 0 = R 3 \ S ε 0 is the domain of the fluid. We also denote by S ε (t) the region occupied by the rigid body and by F ε (t) = R 3 \ S ε (t) the region occupied by the viscous fluid at time t.

In order to describe the motion of the rigid body, we need to specify its center of mass, that we denote by h ε (t) and a rotation matrix R(t) ∈ SO(3) which describes how the body rotates compared to the initial position. In other words, we have that S ε (t) = {x ∈ R 3 | x = h ε (t) + R(t)x 0 , x 0 ∈ S ε 0 }. The velocity of the solid particle x(t) = h ε (t) + R(t)x 0 is given by

x (t) = h ε (t) + R (t)x 0 = h ε (t) + R (t)R(t) -1 (x -h ε (t)) = h ε (t) + R (t)R(t) T (x -h ε (t))
where the superscript T denotes the transpose. Since R(t) ∈ SO(3), the matrix R (t)R(t) T is skew-symmetric and can therefore be identified to a three-dimensional rotation vector ω ε (t): R (t)R(t) T z = ω ε (t) × z, z ∈ R 3 where × denotes the standard cross product of vectors in R 3 . Therefore the velocity of the solid particle x is given by h ε (t) + ω ε (t) × (x -h ε (t)), x ∈ S ε (t). [START_REF] Chipot | Limits of the Stokes and Navier-Stokes equations in a punctured periodic domain[END_REF] We assume that the rigid body is homogeneous of density ρ ε . We denote its total mass by m ε so that m ε = ρ ε |S ε 0 | where |S ε 0 | is the volume of the rigid body. We also introduce J ε the matrix of inertia of the rigid body defined by

(J ε a) • b = ρ ε S ε a × (x -h ε (t) • b × (x -h ε (t) dx, for any a, b ∈ R 3 ,
(see [START_REF] Gunzburger | Global Existence of Weak Solutions for Viscous Incompressible Flows around a Moving Rigid Body in Three Dimensions[END_REF]).

We assume that the fluid is governed by the classical Navier-Stokes equations with noslip boundary conditions on the boundary of the rigid body, and the dynamics of the rigid body is described by the equations of the balance of linear and angular momentum. We suppose that the fluid is homogeneous of constant density 1 to simplify the notations and we denote by u ε (t, x) the velocity of the fluid and by p ε (t, x) the pressure of the fluid. Moreover, we also denote by Σ(u ε , p ε ) the stress tensor of the fluid Σ(u ε , p ε ) = 2νD(u ε ) -p ε I 3 , where I 3 is identity matrix of order 3 and D(u ε ) is the deformation tensor [START_REF] Conca | Existence of solutions for the equations modelling the motion of a rigid body in a viscous fluid[END_REF] D(u ε ) := 1 2 ∂u ε,i ∂x j + ∂u ε,j ∂x i i,j i, j = 1, 2, 3.

With the notation introduced above, we have the following mathematical formulation for the fluid-rigid body system (see [START_REF] Desjardins | Existence of weak solutions for the motion of rigid bodies in a viscous fluid[END_REF], [START_REF] Gunzburger | Global Existence of Weak Solutions for Viscous Incompressible Flows around a Moving Rigid Body in Three Dimensions[END_REF] and [START_REF] Serre | Chute Libre d'un Solide dans un Fluide Visqueux lncompressible[END_REF]):

• Fluid equations:

∂u ε ∂t + (u ε • ∇)u ε -ν∆u ε + ∇p ε = 0 for t ∈ (0, +∞), x ∈ F ε (t).
div u ε = 0 for t ∈ (0, +∞), x ∈ F ε (t).

(3)

• Rigid body equations:

m ε h ε (t) = - ∂S ε (t)
Σ(u ε , p ε )n ε ds for t ∈ (0, +∞). ( 4)

(J ε ω ε ) (t) = - ∂S ε (t)
(x -h ε ) × (Σ(u ε , p ε )n ε )ds for t ∈ (0, +∞). [START_REF] Desjardins | On weak solutions for fluid-rigid structure interaction: compressible and incompressible models[END_REF] • Boundary conditions:

u ε (t, x) = h ε (t) + ω ε (t) × x -h ε (t) , for t ∈ (0, +∞), x ∈ ∂S ε (t). lim |x|→∞ u ε (t, x) = 0 for t ∈ [0, +∞). ( 6
)
In the above system, we have denoted by n ε (t, x) the unit normal vector to ∂S ε pointing outside the fluid domain F ε . The first line in [START_REF] Galdi | Strong Solutions to the Problem of Motion of a Rigid Body in a Navier-Stokes Liquid under the Action of Prescribed Forces and Torques[END_REF] is the Dirichlet boundary condition: the fluid velocity and the solid velocity must agree on the boundary of the body.

The system (3)-( 6) should be completed by some initial conditions. As mentioned at the beginning, we assume that the initial position of the center of mass of the rigid body is in the origin. We denote by u 0 ε the initial fluid velocity:

u ε (0, x) = u 0 ε , h ε (0) = 0, h ε (0) = l 0 ε , ω ε (0) = ω 0 ε . (7)
The coupled system satisfies some L 2 energy estimates at least at the formal level. Taking the inner product of (3) with u ε , integrating the result by parts and using the equations ( 4) and ( 5), we get the following energy estimate (see [START_REF] Gunzburger | Global Existence of Weak Solutions for Viscous Incompressible Flows around a Moving Rigid Body in Three Dimensions[END_REF]):

(8) u ε (t) 2 L 2 (F ε (t)) + m ε |h ε (t)| 2 + (J ε ω ε (t)) • ω ε (t) + 4ν t 0 D(u ε ) 2 L 2 (F ε (t)) ≤ u 0 ε 2 L 2 (F ε 0 ) + m ε |l 0 ε | 2 + J ε ω 0 ε • ω 0 ε .
The sum of the first three terms on the left-hand side of ( 8) is called the kinetic energy of the system at time t, while the forth term is called viscous dissipation. Obviously the initial kinetic energy is the right-hand side of [START_REF] He | A small solid body with large density in a planar fluid is negligible[END_REF].

Over the last few years, there were a lot of works dealing with the well-posedness of the fluid-rigid body system by using energy estimates. Both weak finite energy solutions (Leray solutions) and strong H 1 solutions were constructed. When the fluid is enclosed in a bounded region, the existence of solutions is proved under some constraints on the collisions between the rigid body and the boundary of the domain. When the domain of motion is the whole of R 3 there is of course no such constraint. We give some references below but we would like to say that this list is not exhaustive. The existence of weak Leray solutions have been proved in [START_REF] Conca | Existence of solutions for the equations modelling the motion of a rigid body in a viscous fluid[END_REF], [START_REF] Desjardins | On weak solutions for fluid-rigid structure interaction: compressible and incompressible models[END_REF], [START_REF] Gunzburger | Global Existence of Weak Solutions for Viscous Incompressible Flows around a Moving Rigid Body in Three Dimensions[END_REF] and [START_REF] Serre | Chute Libre d'un Solide dans un Fluide Visqueux lncompressible[END_REF] (see also the references therein). We refer to [START_REF] Cumsille | Wellposedness for the system modelling the motion of a rigid body of arbitrary form in an incompressible viscous fluid[END_REF], [START_REF] Desjardins | Existence of weak solutions for the motion of rigid bodies in a viscous fluid[END_REF] and [START_REF] Galdi | Strong Solutions to the Problem of Motion of a Rigid Body in a Navier-Stokes Liquid under the Action of Prescribed Forces and Torques[END_REF] for results about strong H 1 solutions. The vanishing viscosity limit was considered in [START_REF] Sueur | A Kato Type Theorem for the Inviscid Limit of the Navier-Stokes Equations with a Moving Rigid Body[END_REF]. Let us also mention that the case of the dimension two was also considered in the literature, see for example [START_REF] Desjardins | Existence of weak solutions for the motion of rigid bodies in a viscous fluid[END_REF], [START_REF] Hoffmann | On a motion of a solid body in a viscous fluid. Two-dimensional case[END_REF], [START_REF] San Martín | Global Weak Solutions for the Two-Dimensional Motion of Several Rigid Bodies in an Incompressible Viscous Fluid[END_REF] and [START_REF] Takahashi | Global strong solutions for the two-dimensional motion of an infinite cylinder in a viscous fluid[END_REF].

The initial conditions should satisfy the following compatibility conditions (see [START_REF] Desjardins | Existence of weak solutions for the motion of rigid bodies in a viscous fluid[END_REF]):

(9) u 0 ε ∈ L 2 (F ε 0 ), div u 0 ε = 0 in F ε 0 , u 0 ε • n ε = (l 0 ε + ω 0 ε × x) • n ε on ∂S ε 0 .
The second condition above is a weak version of the Dirichlet boundary condition in which only the normal components of the fluid velocity and of the solid velocity must agree on the boundary of the obstacle. This is in agreement with the usual theory of Leray solutions of the Navier-Stokes equations where the initial velocity is assumed to be only tangent to the boundary.

Before stating a result of existence of weak solutions for the motion of a rigid body in a fluid, let us introduce the global density and the global velocity, defined on the whole of R 3 . The fluid is homogeneous of constant density 1 while the rigid body is of density ρ ε , so we can define the global density ρ ε (t, x) as follows:

ρ ε (t, x) = χ F ε (t) (x) + ρ ε χ S ε (t) (x), for x ∈ R 3
where we denote χ A denotes the characteristic function of the set A. Moreover, recalling the formula for the velocity of the rigid body, see [START_REF] Chipot | Limits of the Stokes and Navier-Stokes equations in a punctured periodic domain[END_REF], one may define a global velocity u ε by

u ε (t, x) = u ε (t, x) if x ∈ F ε (t) h ε (t) + ω ε (t) × (x -h ε (t)) if x ∈ S ε (t).
Clearly, by conditions (9), we know that

u 0 ε ∈ L 2 (R 3 ), div u 0 ε = 0 in R 3 .
Motivated by the energy estimates [START_REF] He | A small solid body with large density in a planar fluid is negligible[END_REF] and by the construction of ρ ε and u ε we introduce the following notion of weak solution (see [START_REF] Conca | Existence of solutions for the equations modelling the motion of a rigid body in a viscous fluid[END_REF], [START_REF] Desjardins | On weak solutions for fluid-rigid structure interaction: compressible and incompressible models[END_REF], [START_REF] Gunzburger | Global Existence of Weak Solutions for Viscous Incompressible Flows around a Moving Rigid Body in Three Dimensions[END_REF] and [START_REF] Serre | Chute Libre d'un Solide dans un Fluide Visqueux lncompressible[END_REF]).

Definition 1. A triplet ( u ε , h ε , ω ε ) is a weak Leray solution of (3)-(7), if • u ε , h ε , ω ε satisfying h ε ∈ W 1,∞ (R + ; R 3 ), ω ε ∈ L ∞ (R + ; R 3 ), u ε ∈ L ∞ R + ; L 2 (F ε ) ∩ L 2 loc R + ; H 1 (F ε ) , u ε ∈ C 0 w R + ; L 2 (R 3 ) ; • u ε is divergence free in the whole of R 3 with D u ε (t, x) = 0 in S ε (t);
• u ε verifies the equation in the following sense:

- ∞ 0 R 3 ρ ε u ε • ∂ t ϕ ε + ( u ε • ∇)ϕ ε + 2ν ∞ 0 R 3 D( u ε ) : D(ϕ ε ) = R 3 ρ ε (0) u 0 ε • ϕ ε (0).
for any test function

ϕ ε ∈ W 1,∞ R + ; H 1 σ (R 3 ) , compactly supported in R + × R 3 such that Dϕ ε (t, x) = 0 in S ε (t).
One has the following result of existence of weak solutions of the initial-boundary value problem (3)- [START_REF] Gunzburger | Global Existence of Weak Solutions for Viscous Incompressible Flows around a Moving Rigid Body in Three Dimensions[END_REF] in the sense defined above (see [START_REF] Conca | Existence of solutions for the equations modelling the motion of a rigid body in a viscous fluid[END_REF], [START_REF] Desjardins | On weak solutions for fluid-rigid structure interaction: compressible and incompressible models[END_REF], [START_REF] Gunzburger | Global Existence of Weak Solutions for Viscous Incompressible Flows around a Moving Rigid Body in Three Dimensions[END_REF] and [START_REF] Serre | Chute Libre d'un Solide dans un Fluide Visqueux lncompressible[END_REF]).

Theorem 1. Let u 0 ε ∈ L 2 (R 3
) be divergence free and such that D u 0 ε = 0 in S ε 0 . Then, there exists at least one global weak solution ( u ε , h ε , ω ε ) of the initial-boundary value problem (3)- [START_REF] Gunzburger | Global Existence of Weak Solutions for Viscous Incompressible Flows around a Moving Rigid Body in Three Dimensions[END_REF] in the sense of Definition 1. Moreover, u ε satisfies the following energy estimate:

R 3 ρ ε | u ε (t)| 2 + 4ν t 0 R 3 |D( u ε )| 2 ≤ R 3 ρ ε (0)| u 0 ε | 2 ∀t > 0. ( 10
)
We now let ε → 0 and wish to find the limit of the solution given in Theorem 1. Let us first review the literature available on related results.

In dimension two the literature is richer. Iftimie, Lopes Filho and Nussenzveig Lopes [START_REF] Iftimie | Two-dimensional incompressible viscous flow around a small obstacle[END_REF] proved convergence towards the Navier-Stokes equations in R 2 in the case when the rigid body does not move. Lacave [START_REF] Lacave | Two dimensional incompressible ideal flow around a thin obstacle tending to a curve[END_REF] considered the case of a thin obstacle tending to a curve. Recently, Lacave and Takahashi [START_REF] Lacave | Small Moving Rigid Body into a Viscous Incompressible Fluid[END_REF] considered a small disk moving under the influence of a two-dimensional viscous incompressible fluid. Under the condition that the density of the solid is independent of ε and assuming that the initial data is sufficiently small, they used the L p -L q decay estimates of the semigroup associated to the fluidrigid body system to deduce the convergence towards the solution of the Navier-Stokes equations in R 2 . In [START_REF] He | A small solid body with large density in a planar fluid is negligible[END_REF], the authors extended the result of [START_REF] Lacave | Small Moving Rigid Body into a Viscous Incompressible Fluid[END_REF] to the case of arbitrary shape of the body and with no restriction on the size of the initial data but assuming that the density of the obstacle is large.

In dimension three, Iftimie and Kelliher [START_REF] Iftimie | Remarks on the vanishing obstacle limit for a 3D viscous incompressible fluid[END_REF] considered the case of a fixed obstacle and proved convergence towards the Navier-Stokes equations in R 3 . Lacave [START_REF] Lacave | 3D viscous incompressible fluid around one thin obstacle[END_REF] considered more general shrinking obstacles (for instance shrinking to a curve) but still fixed. When the obstacle is moving with the fluid, the limit ε → 0 was considered in [START_REF] Silvestre | The Motion of a Fluid-Rigid Ball System at the Zero Limit of the Rigid Ball Radius[END_REF] in the case when the rigid body is a ball. Unfortunately, the elliptic estimates in that paper, see [START_REF] Silvestre | The Motion of a Fluid-Rigid Ball System at the Zero Limit of the Rigid Ball Radius[END_REF]Theorem 3.1], are not correct as was observed in [START_REF] Chipot | Limits of the Stokes and Navier-Stokes equations in a punctured periodic domain[END_REF]Subsection 2.1].

As far as we know, Theorem 2 below is the first result on the limit ε → 0 in dimension three for a moving obstacle. We will essentially show that if the density of the rigid body goes to infinity, then the energy estimates are sufficient to pass to the limit in the weak formulation by using a truncation procedure. We obtain then the convergence of the solutions constructed in Theorem 1 to a solution of the Navier-Stokes equations in R 3 under the assumption that the initial data u 0 ε is bounded in L 2 . We do not need to impose any small data condition or any restriction on the shape of the body.

Let us now state the main result of this paper.

Theorem 2. Let u 0 ε ∈ L 2 (R 3 ) be divergence free and such that D u 0 ε = 0 in S ε 0 . We assume that

• S ε 0 ⊂ B(0, ε); • the mass m ε of the rigid body satisfies that

(11) m ε ε 3 → ∞ as ε → 0; • u 0 ε converges weakly in L 2 (R 3 ) towards some u 0 . • √ m ε h ε (0) and J ε ω 0 ε • ω 0 ε are bounded uniformly in ε. Let ( u ε , h ε , ω ε )
be the global solution of the system (3)- [START_REF] Gunzburger | Global Existence of Weak Solutions for Viscous Incompressible Flows around a Moving Rigid Body in Three Dimensions[END_REF] given by Theorem 1. Then there exists a subsequence u ε k of u ε which converges

u ε k u weak * in L ∞ R + ; L 2 (R 3 ) and weakly in L 2 loc R + ; H 1 (R 3
) towards a solution u of the Navier-Stokes equations in R 3 in the sense of distributions with initial data u 0 (x).

Moreover, suppose in addition that u 0 ε converges strongly in L 2 (R 3 ) to u 0 (x) and that both √ m ε h ε (0) and J ε ω 0 ε • ω 0 ε converge to 0 as ε → 0. Then the limit solution u satisfies the energy estimate

∀t ≥ 0 u(t) 2 L 2 (R 3 ) + 4ν t 0 D(u) 2 L 2 (R 3 ) ≤ u 0 2 L 2 (R 3 ) .
Let us give a few remarks on the hypotheses of the Theorem above. First, if the rigid body shrinks isotropically to a point, then hypothesis [START_REF] Iftimie | Two-dimensional incompressible viscous flow around a small obstacle[END_REF] means that the density ρ ε of the rigid body tends to infinity as ε → 0. If the rigid body does not shrink isotropically to a point, then condition [START_REF] Iftimie | Two-dimensional incompressible viscous flow around a small obstacle[END_REF] is stronger than simply saying that the density of the rigid body goes to infinity. Indeed, since S ε 0 ⊂ B(0, ε) we have that

|S ε 0 | ≤ 4π 3 ε 3 so ρ ε = m ε |S ε 0 | ≥ 3m ε 4πε 3 → ∞ as ε → 0. Next, the weak convergence of u 0 ε in L 2 (R 3 ) implies its boundedness in L 2 (R 3
). Together with the hypothesis that √ m ε h ε (0) and J ε ω 0 ε •ω 0 ε are bounded uniformly in ε this implies that the right-hand side of ( 8) is bounded. Then [START_REF] Iftimie | Remarks on the vanishing obstacle limit for a 3D viscous incompressible fluid[END_REF]

implies that ρ ε u ε is bounded in L ∞ (R + ; L 2 (R 3 )) and D( u ε ) is bounded in L 2 (R + ; L 2 (R 3 )).
We observed above that ρ ε → ∞ so we can assume that ρ ε ≥ 1. Then we have that ρ ε ≥ 1 (recall that ρ ε = 1 in the fluid region and

ρ ε = ρ ε in the solid region) so u ε is bounded in L ∞ (R + ; L 2 (R 3 )). We infer that (12) u ε (t, x) is bounded in L ∞ R + ; L 2 (R 3 ) ∩ L 2 loc R + ; H 1 (R 3
) and we will see that this is all we need to pass to the limit in our PDE. We require neither the Dirichlet boundary conditions nor the special form of u ε inside the rigid body. All we need is the above boundedness and the fact that the Navier-Stokes equations are satisfied in the exterior of the ball B(0, ε). More precisely, we can prove the following more general statement.

Theorem 3. Let v ε (t, x) be a divergence free vector field bounded independently of ε in

L ∞ loc (R + ; L 2 (R 3 )) ∩ L 2 loc (R + ; H 1 (R 3 )) ∩ C 0 w (R + ; L 2 (R 3
)). We make the following assumptions:

• The vector field v ε verifies the Navier-Stokes equations

(13) ∂ t v ε -ν∆v ε + v ε • ∇v ε = -∇π ε
in the exterior of the ball B(h ε (t), ε) with initial data v ε (0, x) in the following sense:

- ∞ 0 R 3 v ε • ∂ t ϕ + ν ∞ 0 R 3 ∇v ε : ∇ϕ + T 0 R 3 v ε • ∇v ε • ϕ = R 3 v ε (0) • ϕ(0)
for every test function ϕ ∈ W 1,∞ R + × R 3 which is divergence free, compactly supported in R + × R 3 and such that for all t the function x → ϕ(t, x) is smooth and compactly supported in the set {|x -h ε (t)| > ε}. • The initial data v ε (0, x) is divergence free, square integrable and converges weakly to some

v 0 (x) in L 2 (R 3 ). • The center of the ball verifies h ε ∈ W 1,∞ (R + ; R 3 ) and ε 3 2 h ε (t) → 0 strongly in L ∞ loc (R + ) when ε → 0. Then there exists a subsequence of v ε which converges weak * in L ∞ loc (R + ; L 2 (R 3 )) and weakly in L 2 loc (R + ; H 1 (R 3
)) to a solution v of the Navier-Stokes equations in R 3 in the sense of distributions with initial data v 0 (x).

Moreover, if we assume in addition that v ε (0, x) converges strongly in L 2 to v 0 (x) and that the following energy estimate holds true for v ε

(14) ∀t ≥ 0 v ε (t) 2 L 2 (R 3 \B(hε(t),ε)) +4ν t 0 D(v ε ) 2 L 2 (R 3 \B(hε(t),ε)) ≤ v ε (0) 2 L 2 (R 3 ) +o(1)
as ε → 0, then the limit solution v satisfies the following energy estimate

∀t ≥ 0 v(t) 2 L 2 (R 3 ) + 4ν t 0 D(v) 2 L 2 (R 3 ) ≤ v 0 2 L 2 (R 3 ) . (15)
Let us observe that Theorem 2 follows from Theorem 3 applied for v ε (t, x) = u ε (t, x). Indeed, from [START_REF] Lacave | Two dimensional incompressible ideal flow around a thin obstacle tending to a curve[END_REF] we have that

v ε is bounded in L ∞ loc (R + ; L 2 (R 3 )) ∩ L 2 loc (R + ; H 1 (R 3
)). Next we obviously have that u ε verifies the Navier-Stokes equations in the exterior of the ball B(h ε (t), ε) and so does v ε . We observed that the right-hand side of ( 8) is bounded so √ m ε h ε is bounded. From [START_REF] Iftimie | Two-dimensional incompressible viscous flow around a small obstacle[END_REF] we infer that ε Let us now assume in addition the L 2 strong convergence of u 0 ε towards u 0 and let us prove [START_REF] Lacave | Small Moving Rigid Body into a Viscous Incompressible Fluid[END_REF]. We have the L 2 strong convergence of v ε (0, x) to v 0 . Recalling that the matrix of inertia is non-negative we can ignore the second and the third terms in [START_REF] He | A small solid body with large density in a planar fluid is negligible[END_REF] to estimate [START_REF] Lacave | Small Moving Rigid Body into a Viscous Incompressible Fluid[END_REF] follows. The passing to the limit stated in Theorem 3 uses the boundedness of v ε in the energy space

v ε (t) 2 L 2 (R 3 \B(hε(t),ε)) +4ν t 0 D(v ε ) 2 L 2 (R 3 \B(hε(t),ε)) = u ε (t) 2 L 2 (R 3 \B(hε(t),ε)) + 4ν t 0 D(u ε ) 2 L 2 (R 3 \B(hε(t),ε)) ≤ u ε (t) 2 L 2 (F ε (t)) + 4ν t 0 D(u ε ) 2 L 2 (F ε (t)) ≤ u 0 ε 2 L 2 (F ε (t)) + m ε |l 0 ε | 2 + J ε ω 0 ε • ω 0 ε ≤ v ε (0) 2 L 2 (R 3 ) + m ε |l 0 ε | 2 + J ε ω 0 ε • ω 0 ε . By hypothesis m ε |l 0 ε | 2 + J ε ω 0 ε • ω 0 ε → 0 so
L ∞ R + ; L 2 (R 3 ) ∩ L 2 loc R + ; H 1 (R 3
) and the construction of a cut-off ϕ ε supported in the exterior of the ball B(h ε (t), ε). We multiply [START_REF] Lacave | 3D viscous incompressible fluid around one thin obstacle[END_REF] with the cut-off ϕ ε , and then pass to the limit by means of classical compactness methods. The main obstruction is that, when the rigid body moves under the influence of the fluid, not only the velocity depends on time, but also the cut-off function. Time derivative estimates for v ε are not easy to obtain and, once obtained, it is not easy to pass to the limit in the term with the time derivative.

The paper is organized as follows. In Section 2, we introduce some notation and present some preliminary results. The construction of the cut-off near the rigid body is given in Section 3. We show the strong convergence by means of temporal estimates in Section 4 and pass to the limit to conclude our proof in Section 5.

Notation and Preliminary results

In this section, we will introduce some notations and preliminary results. For a sufficiently regular vector field u : R 3 → R 3 , we denote by ∇u the second order tensor field whose components (∇u) ij are given by ∂u j /∂x i , and by D(u) the symmetric part of ∇u (see ( 2)). The double dot product M : N of two matrices M = (m ij ) and N = (n ij ) denotes the quantity i,j m ij n ij .

For function spaces, we shall use standard notations L p and H m to denote the usual Lebesgue and Sobolev spaces. C m b denotes the set of bounded functions whose first m derivatives are bounded functions. We add subscripts 0 and σ to these spaces to specify that their elements are compactly supported and divergence free, respectively. For instance, the notation C ∞ 0,σ defines the space of smooth, compactly supported and divergence free vector fields on R 3 .

In addition, unless we specify the domain, all function spaces and norms are considered to be taken on R 3 in the x variable. For the t variable, we use the notation R + = [0, ∞) and emphasize that the endpoint 0 belongs to R + . Throughout this article, we denote by C a generic constant whose value can change from one line to another.

Let ϕ ∈ C 1 b (R + ; C ∞ 0,σ ). The stream function ψ of ϕ is defined by the following formula:

ψ(x) = - R 3
x -y 4π|x -y| 3 × ϕ(y)dy where × denotes the standard cross product of vectors in R 3 .

Because ϕ is divergence free, we have that curl ψ = ϕ and ψ = curl ∆ -1 ϕ. Furthermore,

ψ is smooth, ψ ∈ C 1 b (R + ; C ∞ )
, and vanishes at infinity. Moreover, we have the following well-known estimate:

∇ψ(t, •) H 2 ≤ C ϕ(t, •) H 2 . ( 16
)
In our case, in order to deal with the singularity in h ε , we need to have a stream function vanishing in h ε . The stream function ψ defined above has no reason to vanish in h ε , so we are led to introduce a modified stream function ψ ε . We define [START_REF] Silvestre | The Motion of a Fluid-Rigid Ball System at the Zero Limit of the Rigid Ball Radius[END_REF]

ψ ε (t, x) = ψ(t, x) -ψ(t, h ε (t)).
Clearly ψ ε (t, h ε (t)) = 0. We collect in the following lemma some useful properties of the modified stream function.

Lemma 1. Let ϕ ∈ C 1 b (R + ; C ∞ 0,σ
) and define the modified stream function ψ ε as in [START_REF] Silvestre | The Motion of a Fluid-Rigid Ball System at the Zero Limit of the Rigid Ball Radius[END_REF]. We have that:

(i)

ψ ε ∈ W 1,∞ (R + ; C ∞ ) and curl ψ ε = ϕ.
(ii) There exists a universal constant C > 0 such that for all R > 0 we have that

ψ ε (t, •) L ∞ (B(hε(t),R)) ≤ CR ϕ(t, •) H 2 (18)
for all t ≥ 0 and

∂ t ψ ε (t, •) L ∞ (B(hε(t),R)) ≤ C R ∂ t ϕ(t, •) H 2 + |h ε (t)| ϕ(t, •) H 2
for almost all t ≥ 0.

Proof. We observe first that curl

ψ ε = curl ψ = ϕ. Moreover, ψ ∈ C 1 b (R + ; C ∞ ) and h ε ∈ W 1,∞ (R + ) imply that ψ ε ∈ W 1,∞ (R + ; C ∞ ). This proves part (i).
Next, to prove (ii) we use the mean value theorem to estimate

ψ ε (t, x) L ∞ (B(hε(t),R)) = ψ(t, x) -ψ(t, h ε (t)) L ∞ (B(hε(t),R)) ≤ |x -h ε (t)| ∇ψ(t, x) L ∞ (B(hε(t),R)) ≤ R ∇ψ H 2 ≤ CR ϕ H 2
where we used relation [START_REF] Serre | Chute Libre d'un Solide dans un Fluide Visqueux lncompressible[END_REF]. This proves [START_REF] Sueur | A Kato Type Theorem for the Inviscid Limit of the Navier-Stokes Equations with a Moving Rigid Body[END_REF].

We recall now that h ε is Lipschitz in time so it is almost everywhere differentiable in time. Let t be a time where h ε is differentiable. We write

∂ t ψ ε (t, x) = ∂ t (ψ(t, x) -ψ(t, h ε (t))) = ∂ t ψ(t, x) -∂ t ψ(t, h ε (t)) -h ε (t) • ∇ψ(t, h ε (t)).
We can bound

∂ t ψ ε (t, •) L ∞ (B(hε(t),R)) ≤ ∂ t ψ(t, x) -∂ t ψ(t, h ε (t)) L ∞ (B(hε(t),R)) + |h ε (t)| ∇ψ(t, •) L ∞ ≤ |x -h ε (t)| ∂ t ∇ψ(t, •) L ∞ + |h ε (t)| ∇ψ(t, •) L ∞ ≤ C R ∂ t ∇ψ(t, •) H 2 + |h ε (t)| ∇ψ(t, •) H 2 ≤ C R ∂ t ϕ(t, •) H 2 + |h ε (t)| ϕ(t, •) H 2 .
This completes the proof of the lemma.

Cut-off near the rigid body

In this section, we will construct a cut-off ϕ ε near the rigid body, which will be used as a test function in the procedure of passing to the limit in Section 5.

Firstly, we construct a cut-off function η ε (t, x) near the ball B(h

ε (t), ε). Let η(x) ∈ C ∞ (R 3 ; [0, 1]) be a function such that η(x) : R 3 → [0, 1], η(x) = 0 if |x| ≤ 3 2 1 if |x| ≥ 2
The function η(x) is a cut-off function in the neighborhood of the unit ball B(0, 1). A cut-off η ε (t, x) in the neighborhood of the domain B(h ε (t), ε) is the following function

(19) η ε (t, x) = η x -h ε (t) ε = 0 if |x -h ε (t)| ≤ 3 2 ε 1 if |x -h ε (t)| ≥ 2ε.
.

Notice that η ε (t, x) is a space-time function while the function η(x) only has a space variable. We state some properties of this new cut-off in the following lemma.

Lemma 2. The cut-off function η ε satisfies (i)

η ε ∈ W 1,∞ (R + ; C ∞ );
(ii) η ε vanishes in the neighborhood of the ball B(h ε (t), ε);

(iii) For any real number q ≥ 1 there exists a constant C = C(q) such that

η ε (t, •) L ∞ = 1, η ε (t, •) -1 L q ≤ Cε 3 q , ∇η ε (t, •) L q ≤ Cε 3-q q , ∇ 2 η ε (t, •) L q ≤ Cε 3-2q q .
Proof. Since h ε is Lipschitz part (i) follows immediately. Part (ii) is also obvious. We prove now part (iii).

Clearly

η ε (t, •) L ∞ = 1. Next η ε (t, x) -1 L q = η x -h ε (t) ε -1 L q = ε 3 q η(x) -1 L q ≤ Cε 3 q .
Notice that ∇η(x) and ∇ 2 η(x) are bounded functions supported in the annulus

{ 3 2 < |x| < 2}. So ∇η ε (t, x) L q = 1 ε ∇η x -h ε (t) ε L q = ε 3-q q ∇η(x) L q ≤ Cε 3-q q , ∇ 2 η ε (t, x) L q = 1 ε 2 ∇ 2 η x -h ε (t) ε L q = ε 3-2q q ∇ 2 η(x) L q ≤ Cε 3-2q q .
This completes the proof of the lemma.

Given a test function ϕ ∈ C 1 b (R + ; C ∞ 0,σ ), we use the cutoff η ε and the modified stream function ψ ε defined in Section 2 (see relation [START_REF] Silvestre | The Motion of a Fluid-Rigid Ball System at the Zero Limit of the Rigid Ball Radius[END_REF]) to construct a new test function ϕ ε which vanishes in the neighborhood of the ball B(h ε (t), ε). We define (20)

ϕ ε = curl(η ε ψ ε ).
We notice that this new test function ϕ ε depends on time even if ϕ is assumed to be constant in time. We state some properties of ϕ ε in the following lemma: Lemma 3. The test function ϕ ε has the following properties:

(i) ϕ ε ∈ W 1,∞ (R + ; C ∞ 0,σ ) and ϕ ε vanishes in the neighborhood of B(h ε (t), ε); (ii) for all T > 0 we have that ϕ ε → ϕ strongly in L ∞ (0, T ; H 1 ) as ε → 0; (iii) there exists a universal constant C such that for all T > 0

ϕ ε L ∞ (0,T ;H 1 ) ≤ C ϕ L ∞ (0,T ;H 2 ) .
Proof. The various norms used below are in the x variable unless otherwise stated.

Clearly, η ε and ψ ε are W 1,∞ in time and smooth in space, so ϕ ε has the same properties. The function ϕ ε is a curl so it is divergence free. Because η ε vanishes in the neighborhood of B(h ε (t), ε), so is ϕ ε . The compact support in space follows immediately once we recall that curl ψ ε = ϕ and observe that

ϕ ε = curl(η ε ψ ε ) = η ε ϕ + ∇η ε × ψ ε Claim (i) is proved.
To prove (ii), we observe that supp ∇η ε ⊂ {|x -h ε (t)| ≤ 2ε} and we estimate

ϕ ε -ϕ L 2 ≤ (η ε -1)ϕ L 2 + ∇η ε × ψ ε L 2 ≤ η ε -1 L 2 ϕ L ∞ + ∇η ε L 2 ψ ε L ∞ (B(hε(t),2ε)) ≤ C ε 3 2 ϕ L ∞ + ε 3 2 ϕ H 2 ≤ Cε 3 2 ϕ H 2
where we used Lemmas 1 and 2.

Taking the supremum on [0, T ] we infer that

(21) ϕ ε -ϕ L ∞ (0,T ;L 2 ) ≤ Cε 3 2 ϕ L ∞ (0,T ;H 2 ) .
Next, by the Sobolev embedding H 2 (R 3 ) → W 1,6 (R 3 ) and by Lemma 2 we estimate

∇(ϕ ε -ϕ) L 2 = ∇ (η ε -1)ϕ + ∇η ε × ψ ε L 2 ≤ η ε -1 L 3 ∇ϕ L 6 + ∇η ε L 2 ϕ L ∞ + ∇η ε L 2 ∇ψ ε L ∞ + ∇ 2 η ε L 2 ψ ε L ∞ (B(hε(t),2ε)) ≤ C ε ϕ W 1,6 + ε 1 2 ϕ L ∞ + ε 1 2 ∇ψ ε L ∞ + Cε -1 2 ψ ε L ∞ (B(hε(t),2ε)) .
From relations ( 17) and ( 16) we get that

∇ψ ε L ∞ = ∇ψ L ∞ ≤ C ∇ψ H 2 ≤ C ϕ H 2 .
From Lemma 1 we have that

ψ ε L ∞ (B(hε(t),2ε)) ≤ Cε ϕ H 2 .
We conclude from the above relations that

∇(ϕ ε -ϕ) L 2 ≤ Cε 1 2 ϕ H 2 .
Taking the supremum on [0, T ] we deduce that

(22) ∇(ϕ ε -ϕ) L ∞ (0,T ;L 2 ) ≤ Cε 1 2 ϕ L ∞ (0,T ;H 2 ) .
We conclude form (21) and ( 22) that

ϕ ε -ϕ L ∞ (0,T ;H 1 ) ≤ Cε 1 2 ϕ L ∞ (0,T ;H 2 ) → 0 as ε → 0.
This proves (ii). To prove (iii) we simply bound

ϕ ε L ∞ (0,T ;H 1 ) ≤ ϕ L ∞ (0,T ;H 1 ) + ϕ ε -ϕ L ∞ (0,T ;H 1 ) ≤ C ϕ L ∞ (0,T ;H 2 ) .
This completes the proof of the lemma.

Temporal estimate and strong convergence

The aim of this section is to derive a temporal estimate and to prove the strong convergence of some sub-sequence of v ε in L 2 loc (R + × R 3 ). We will prove the following result. Proposition 1. There exists a sub-sequence

v ε k of v ε which converges strongly in L 2 loc (R + × R 3 ).
It suffices to prove that for any T > 0 there exists a sub-sequence v ε k of v ε which converges strongly in L 2 (0, T ; L 2 loc (R 3 )). A diagonal extraction then allows to choose the same subsequence for all times T . We choose some finite time T and for the rest of this section we assume that t ∈ [0, T ].

The main idea is to use the Arzelà-Ascoli theorem. Let ϕ ∈ C ∞ 0,σ (R 3 ) be a test function which does not depend on the time. By the definition of the modified stream function, we observe that even if ϕ is constant in time, ψ ε (t, x) still depends on the time through h ε (t). We construct a family of ϕ ε as in Section 3, so that ϕ ε is time-dependent and satisfies Lemma 3.

We first bound

R 3 v ε (t, x) • ϕ ε (t, x) dx = R 3 v ε • curl(η ε ψ ε ) dx = R 3 v ε • (η ε ϕ + ∇η ε × ψ ε ) dx ≤ v ε L 2 η ε L ∞ ϕ L 2 + v ε L 2 ∇η ε L 2 ψ ε L ∞ (B(hε(t),2ε)) ≤ C v ε L 2 ϕ L 2 + ε 3 2 v ε L 2 ϕ H 2 ≤ C v ε L 2 ϕ H 2 .
where we used Lemma 1 and Lemma 2. The boundedness of v ε in L 2 (R 3 ) implies that there exists a constant C 1 independent of ε and t such that

R 3 v ε (t, x) • ϕ ε (t, x) dx ≤ C 1 ϕ H 2 .
We infer that, for t fixed and ϕ ∈ C ∞ 0,σ , the map

ϕ → R 3 v ε (t, x) • ϕ ε (t, x) dx ∈ R
is linear and continuous for the H 2 norm. Then, there exists some

Ξ ε (t) ∈ H -2 σ such that Ξ ε (t), ϕ = R 3 v ε (t, x) • ϕ ε (t, x) dx ∀ϕ ∈ H 2 σ . Moreover (23) Ξ ε (t) H -2 ≤ C 1 ∀t ≥ 0.
From Lemma 3 , we know that ϕ ε vanishes in the neighborhood of B(h ε (t), ε), so it is compactly supported in the exterior of this ball. Therefore it can be used as test function in [START_REF] Lacave | 3D viscous incompressible fluid around one thin obstacle[END_REF]. Multiplying (13) by ϕ ε and integrating in space and in time from s to t yields

t s R 3 ∂ τ v ε • ϕ ε + ν t s R 3 ∇v ε : ∇ϕ ε + t s R 3 v ε • ∇v ε • ϕ ε = 0.
After integrating by parts in time the first term above and using the definition of Ξ ε (t), ϕ , we obtain that

(24) Ξ ε (t) -Ξ ε (s), ϕ = t s R 3 v ε • ∂ τ ϕ ε -ν t s R 3 ∇v ε : ∇ϕ ε - t s R 3 v ε • ∇v ε • ϕ ε .
To bound the second term in the right-hand side above, we recall that v ε is bounded independently of ε in L ∞ (0, T ; L 2 ) ∩ L 2 (0, T ; H 1 ). Thus, by the Hölder inequality and by Lemma 3, we deduce that

ν t s R 3 ∇v ε : ∇ϕ ε ≤ ν t s ∇v ε L 2 ∇ϕ ε L 2 ≤ Cν(t -s) 1 2 ϕ H 2 v ε L 2 (0,T ;H 1 )
≤ Cν(t -s)

1 2 ϕ H 2 .
Next, we estimate the non-linear term in (24) by the Hölder inequality and by the

Gagliardo-Nirenberg inequality v ε L 3 ≤ C v ε 1 2 L 2 ∇v ε 1 2 L 2 , | t s R 3 v ε • ∇v ε • ϕ ε | ≤ t s v ε L 3 ∇v ε L 2 ϕ ε L 6 ≤ C t s v ε 1 2 L 2 ∇v ε 3 2 L 2 ϕ ε H 1 ≤ C(t -s) 1 4 v ε 1 2 L ∞ (0,T ;L 2 ) v ε 3 2 L 2 (0,T ;H 1 ) ϕ H 2 ≤ C(t -s) 1 4 ϕ H 2
It remains to estimate the term with the time-derivative. Notice that since ϕ does not depend on time, we have that ∂ t ϕ = ∂ t curl ψ ε = 0. Several integrations by parts give us

t s R 3 v ε • ∂ τ ϕ ε = t s R 3 v ε • curl ∂ τ (η ε ψ ε ) = t s R 3 curl v ε • ∂ τ (η ε ψ ε ) = t s R 3 curl v ε • (∂ τ η ε ψ ε ) + t s R 3 curl v ε • (η ε ∂ τ ψ ε ) = t s R 3 curl v ε • (∂ τ η ε ψ ε ) + t s R 3 v ε • curl (η ε ∂ τ ψ ε ) = t s R 3 curl v ε • (∂ τ η ε ψ ε ) + t s R 3 v ε • (∇η ε × ∂ τ ψ ε )
We estimate the two terms in the right-hand side of the equality above by using Lemmas 1 and 2 and recalling that ε

3 2 |h ε | is bounded in L ∞ (0, T ) independently of ε: | t s R 3 curl v ε • (∂ τ η ε ψ ε ) | ≤ t s |h ε | ε curl v ε L 2 ∇η x -h ε ε L 2 ψ ε L ∞ (B(hε,2ε)) ≤ C t s ε 3 2 |h ε | curl v ε L 2 ϕ H 2 ≤ C(t -s) 1 2 v ε L 2 (0,T ;H 1 ) ϕ H 2 ≤ C(t -s) 1 2 ϕ H 2 and | t s R 3 v ε • (∇η ε × ∂ τ ψ ε ) | ≤ t s v ε L 6 ∇η ε L 6 5 ∂ τ ψ ε L ∞ (B(hε,2ε)) ≤ C t s ε 3 2 |h ε | v ε L 6 ϕ H 2 ≤ C(t -s) 1 2 v ε L 2 (0,T ;H 1 ) ϕ H 2 ≤ C(t -s) 1 2 ϕ H 2
where we used the Sobolev embedding H 1 (R 3 ) → L 6 (R 3 ).

Gathering the two estimates above, we infer that

| t s R 3 v ε • ∂ τ ϕ ε | ≤ C(t -s) 1 2 ϕ H 2 .
Putting together all the estimates above yields the following bound for Ξ ε :

| Ξ ε (t) -Ξ ε (s), ϕ | ≤ Cν(t -s) 1 2 ϕ H 2 + C(t -s) 1 4 ϕ H 2 + C(t -s) 1 2 ϕ H 2 ≤ C(t -s) 1
4 ϕ H 2 where the constant C above depends on T and ν.

By density of

C ∞ 0,σ in H 2 σ , we then obtain that Ξ ε (t) is equicontinuous in time with value in H -2 σ Ξ ε (t) -Ξ ε (s) H -2 ≤ C(t -s) 1 4 .
On the other hand, Ξ ε (t) is also bounded in H -2 σ , see relation (23). So the compact embedding H -2 → H -3 loc and the Arzelà-Ascoli theorem enable us to extract a subsequence Ξ ε k of Ξ ε converging to some Ξ strongly in

H -3 loc : (25) Ξ ε k → Ξ in C 0 T ; H -3 loc )
. We now use Lemmas 1 and 2 to estimate

| Ξ ε (t) -v ε (t), ϕ | = | R 3 v ε (t, x) • ϕ ε (t, x) - R 3 v ε (t, x) • ϕ(t, x)| = | R 3 v ε (t, x) • (η ε ϕ + ∇η ε × ψ ε ) - R 3 v ε (t, x) • ϕ(t, x)| = | R 3 (η ε -1)v ε (t, x) • ϕ + R 3 v ε • (∇η ε × ψ ε )| ≤ v ε L 2 η ε -1 L 2 ϕ L ∞ + v ε L 2 ∇η ε L 2 ψ ε L ∞ (B(hε,2ε)) ≤ C ε 3 2 v ε L 2 ϕ L ∞ + ε 3 2 v ε L 2 ϕ H 2 ≤ Cε 3 2 ϕ H 2 v ε L 2 .
Using again the density of C ∞ 0,σ in H 2 σ , the above estimate implies that

Ξ ε (t) -v ε (t) H -2 ≤ Cε 3 2 v ε L 2 . So Ξ ε -v ε → 0 in L ∞ (0, T ; H -2 ). In particular Ξ ε -v ε → 0 in L ∞ (0, T ; H -3 loc ). Recalling (25) and relabelling Ξ = v we infer that (26) v ε k → v in L ∞ (0, T ; H -3 loc ). Let f ∈ C ∞ 0 (R 3
). We have the interpolation inequality

f (v ε k -v) L 2 ≤ C f (v ε k -v) 1 4 H -3 f (v ε k -v) 3 4 H 1 so f (v ε k -v) L 8 3 (0,T ;L 2 ) ≤ C f (v ε k -v) 1 4 L ∞ (0,T ;H -3 ) f (v ε k -v) 3 4
L 2 (0,T ;H 1 ) . Given relation (26) and the boundedness of v ε in L 2 (0, T ; H 1 ) we observe that the righthand side above goes to 0 as ε k → 0. We deduce that

v ε k → v strongly in L 8 3 (0, T ; L 2 loc
). The embedding L

Passing to the limit

In this section we are going to complete the proof of Theorem 3 by passing to the limit with compactness methods.

Let T > 0 be finite and fixed. We will pass to the limit only on the time interval [0, T ]. A diagonal extraction allows us to find a subsequence which converges to the expected limit for all t ≥ 0.

Thanks to the assumptions on v ε , we know that

v ε is bounded in L ∞ 0, T ; L 2 ∩ L 2 0, T ; H 1 .
This implies that there exists some v ∈ L ∞ 0, T ; L 2 ∩ L 2 0, T ; H 1 and some sub-

sequence v ε k of v ε such that v ε k v weak * in L ∞ (0, T ; L 2 ), v ε k v weakly in L 2 (0, T ; H 1 ). ( 27
)
Moreover, using Proposition 1, we can further assume that v ε k → v strongly in L 2 (0, T ; L 2 loc ). The main goal of this Section is to prove that the limit v is the solution of the Navier-Stokes equations in R 3 with initial data v 0 (x).

Let ϕ ∈ C ∞ 0 ([0, T ) × R 3 ) be a divergence-free vector field. We construct the family of vector fields ϕ ε k as in Section 3 (see relation (20)). These vector fields are compactly supported in the exterior of the ball B(h ε k (t), ε k ), so they can be used as test functions in [START_REF] Lacave | 3D viscous incompressible fluid around one thin obstacle[END_REF]. Multiplying ( 13) by v ε k and integrating in space and time yields (28) -

T 0 R 3 v ε k • ∂ t ϕ ε k + ν T 0 R 3 ∇v ε k : ∇ϕ ε k + T 0 R 3 v ε k • ∇v ε k • ϕ ε k = R 3 v ε k (0) • ϕ ε k (0).
We will pass to the limit ε k → 0 in each of the term in the equation above. First, from Lemma 3, we have that

ϕ ε k (0) → ϕ(0) strongly in L 2 (R 3 ).
We also know by hypothesis that v ε (0, x) converges weakly to v 0 (x) in L 2 (R 3 ). We infer that

R 3 v ε k (0) • ϕ ε k (0) ε k →0 -→ R 3 v(0) • ϕ(0). (29)
Next, we also know from Lemma 3 that

∇ϕ ε k → ∇ϕ strongly in L ∞ (0, T ; L 2 ).
Recalling that ∇v ε k ∇v weakly in L 2 ([0, T ] × R 3 ), see relation (27), we deduce that

T 0 R 3 ∇v ε k : ∇ϕ ε k ε k →0 -→ T 0 R 3 ∇v : ∇ϕ. (30)
We decompose the non-linear term in the left-hand of (28) as follows:

T 0 R 3 v ε k • ∇v ε k • ϕ ε k = T 0 R 3 v ε k • ∇v ε k • ϕ + T 0 R 3 v ε k • ∇v ε k • (ϕ ε k -ϕ).
To treat the first term on the right-hand side, we know that ϕ is compactly supported, that ∇v ε k ∇v weakly in L 2 ([0, T ] × R 3 ) and that v ε k → v strongly in L 2 (0, T ; L 2 loc ). These observations enable us to pass to the limit:

T 0 R 3 v ε k • ∇v ε k • ϕ ε k →0 -→ T 0 R 3 v • ∇v • ϕ.
For the second term, we make an integration by parts to get that

T 0 R 3 v ε k • ∇v ε k • (ϕ ε k -ϕ) = - T 0 R 3 v ε k ⊗ v ε k : ∇(ϕ ε k -ϕ).
By the Hölder inequality, the Gagliardo-Nirenberg inequality

v ε k L 4 ≤ C v ε k 1 4 L 2 ∇v ε k 3 4 L 2
and the strong convergence of ϕ ε k in L ∞ (0, T ; H 1 ) stated in Lemma 3, we obtain that

| - T 0 R 3 v ε k ⊗ v ε k : ∇(ϕ ε k -ϕ)| ≤ T 0 v ε k 2 L 4 ∇(ϕ ε k -ϕ) L 2 ≤ C T 0 v ε k 1 2 L 2 ∇v ε k 3 2 L 2 ϕ ε k -ϕ H 1 ≤ CT 1 4 v ε k 1 2 L ∞ (0,T ;L 2 ) v ε k 3 2 L 2 (0,T ;H 1 ) ϕ ε k -ϕ L ∞ (0,T ;H 1 ) ε k →0 -→ 0
where we also used the boundedness of

v ε k in L ∞ 0, T ; L 2 ∩ L 2 0, T ; H 1 .
Combining the relations above, we deduce that (31)

T 0 R 3 v ε k • ∇v ε k • ϕ ε k ε k →0 -→ T 0 R 3 v • ∇v • ϕ.
Now, it remains to pass to the limit in the first term on the left-hand side of (28). Integrating by parts twice allows us to decompose this term into three parts as follows:

T 0 R 3 v ε k • ∂ t ϕ ε k = T 0 R 3 v ε k • curl ∂ t (η ε k ψ ε k ) = T 0 R 3 curl v ε k • ∂ t (η ε k ψ ε k ) = T 0 R 3 curl v ε k • (∂ t η ε k ψ ε k ) + T 0 R 3 curl v ε k • (η ε k ∂ t ψ ε k ) = T 0 R 3 curl v ε k • (∂ t η ε k ψ ε k ) + T 0 R 3 v ε k • curl (η ε k ∂ t ψ ε k ) = T 0 R 3 curl v ε k • (∂ t η ε k ψ ε k ) + T 0 R 3 v ε k • (∇η ε k × ∂ t ψ ε k ) + T 0 R 3 v ε k • (η ε k curl ∂ t ψ ε k ) = T 0 R 3 curl v ε k • (∂ t η ε k ψ ε k ) + T 0 R 3 v ε k • (∇η ε k × ∂ t ψ ε k ) + T 0 R 3 v ε k • (η ε k ∂ t ϕ)
where we used the fact that curl ψ ε k = ϕ (see Lemma 1).

We will treat the three terms in the right-hand side of the relation above. For the first term, we use the Hölder inequality twice, the definition of η ε (see relation [START_REF] Takahashi | Global strong solutions for the two-dimensional motion of an infinite cylinder in a viscous fluid[END_REF]) and Lemma 1 to bound

| T 0 R 3 curl v ε k • (∂ t η ε k ψ ε k ) | ≤ T 0 |h ε k (t)| ε k curl v ε k L 2 ∇η x -h ε k (t) ε k L 2 ψ ε k L ∞ (B(hε k (t),2ε k )) ≤ C T 0 ε 3/2 k |h ε k (t)| curl v ε k L 2 ϕ H 2 ≤ CT 1 2 ε 3/2 k h ε k (t) L ∞ (0,T ) v ε k L 2 (0,T ;H 1 ) ϕ L ∞ (0,T ;H 2 ) ε k →0 -→ 0.
where we used the hypothesis ε

3/2 k h ε k (t) → 0 in L ∞ loc (R + ) when ε k → 0.
To bound the second term, we use again the Hölder inequality, Lemmas 1 and 2 and the hypothesis on ε

3/2 k h ε k : | T 0 R 3 v ε k • (∇η ε k × ∂ t ψ ε k ) | ≤ T 0 v ε k L 6 ∇η ε k L 6 5 ∂ t ψ ε k L ∞ (B(hε k (t),2ε k )) ≤ C T 0 ε 3/2 k v ε k L 6 ε k ∂ t ϕ H 2 + |h ε k (t)| ϕ H 2 ≤ C T 0 v ε k H 1 ε 5/2 k ∂ t ϕ H 2 + ε 3/2 k |h ε k (t)| ϕ H 2 ≤ CT 1 2 v ε k L 2 (0,T ;H 1 ) ε 5/2 k ∂ t ϕ L ∞ (0,T ;H 2 ) + ε 3/2 k h ε k L ∞ (0,T ) ϕ L ∞ (0,T ;H 2 ) ε k →0 -→ 0.
where we also used the Sobolev embedding H 1 (R 3 ) → L 6 (R 3 ). For the third term, we shall write

v ε k η ε k = v ε k (η ε k -1) + (v ε k -v) + v to get that T 0 R 3 v ε k • (η ε k ∂ t ϕ) = T 0 R 3 (η ε k -1)v ε k • ∂ t ϕ + T 0 R 3 (v ε k -v) • ∂ t ϕ + T 0 R 3 v • ∂ t ϕ
Recalling that v ε k → v strongly in L 2 (0, T ; L 2 loc ), we observe that the second term in the right-hand side of the equality above converges to 0. We estimate the first term by the Hölder inequality and by Lemma 2

T 0 R 3 (η ε k -1)v ε k • ∂ t ϕ ≤ T 0 v ε k L 2 η ε k -1 L 2 ∂ t ϕ L ∞ ≤ Cε 3 2 k T 0 v ε k L 2 ∂ t ϕ L ∞ ≤ CT ε 3 2 k v ε k L ∞ (0,T ;L 2 ) ∂ t ϕ L ∞ (0,T ;L ∞ ) ε k →0 -→ 0.
We infer that

T 0 R 3 v ε k • (η ε k ∂ t ϕ) ε k →0 -→ T 0 R 3 v • ∂ t ϕ, which implies that (32) T 0 R 3 v ε k • ∂ t ϕ ε k ε k →0 -→ T 0 R 3 v • ∂ t ϕ.
Gathering (28), ( 29), ( 30), ( 31) and (32), we conclude that

- T 0 R 3 v • ∂ t ϕ + ν T 0 R 3 ∇v : ∇ϕ + T 0 R 3 v • ∇v • ϕ = R 3 v(0) • ϕ(0)
which is the weak formulation of the Navier-Stokes equations in R 3 . This completes the proof that v is a solution of the Navier-Stokes equations in R 3 in the sense of distributions.

In order to complete the proof of Theorem 3, it remains to prove the energy inequality (15) under the additional assumption that v ε (0) converges strongly to v 0 in L 2 .

Let us observe first that v ∈ C 0 w (R + ; L 2 (R 3 )). This follows from the fact that v ∈ L

∞ loc (R + ; L 2 (R 3
)) is a solution in the sense of distributions of the Navier-Stokes equations in R 3 . The argument is classical, but let us recall it for the benefit of the reader. We apply the Leray projector P in R 3 to the Navier-Stokes equations verified by v to obtain that

∂ t v -ν∆v + P div(v ⊗ v) = 0. Because v ∈ L ∞ loc (R + ; L 2 (R 3 )) we have that v⊗v ∈ L ∞ loc (R + ; L 1 (R 3 )) ⊂ L ∞ loc (R + ; H -2 (R 3 )). We also have that ∆v ∈ L ∞ loc (R + ; H -2 (R 3 )), so ∂ t v ∈ L ∞ loc (R + ; H -2 (R 3
)). We infer that v is Lipschitz in time with values in H -2 (R 3 ); in particular it is strongly continuous in time with values in H -2 (R 3 ). This strong continuity in time together with the boundedness of the L 2 norm implies the weak continuity of v in time with values in L 2 . In particular, we have that v(t) is well-defined and belongs to L 2 (R 3 ) for all times t ≥ 0 (and not only for almost all times).

Let us observe now that for all t ≥ 0 we have that v ε k (t) v(t) weakly in L 2 (R 3 ). Indeed, we know from relation (26) that v ε k (t) → v(t) strongly in H -3 loc (R 3 ), so v ε k (t), ϕ → v(t), ϕ for all test functions ϕ. The boundedness of v ε k (t) in L 2 and the density of the test functions in L 2 imply that v ε k (t), ϕ → v(t), ϕ for all ϕ ∈ L 2 , that is v ε k (t) v(t) weakly in L 2 (R 3 ).

Let us denote by χ A the characteristic function of the set A. We prove now that for all t ≥ 0 v ε k (t)χ B(hε k (t),ε k ) 0 weakly in L 2 . Indeed, let g ∈ L 2 . Then

| v ε k (t)χ B(hε k (t),ε k ) , g | = | B(hε k (t),ε k ) v ε k (t)g| ≤ v ε k (t) L 2 g L 2 (B(hε k (t),ε k )) ε k →0
-→ 0 because v ε k (t) L 2 is bounded and g L 2 (B(hε k (t),ε k )) goes to 0 as ε k → 0. We infer that v ε k (t)χ R 3 \B(hε k (t),ε k ) v(t) weakly in L 2 (R 3 ).

By the weak lower semi-continuity of the L 2 norm we infer that (33) v(t) L 2 (R 3 ) ≤ lim inf

ε k →0 v ε k (t) L 2 (R 3 \B(hε k (t),ε k )) .
Similarly, from the weak convergence

D(v ε k ) D(v) weakly in L 2 ((0, t) × R 3 )
we infer that χ R 3 \B(hε k (t),ε k ) D(v ε k ) D(v) weakly in L 2 ((0, t) × R 3 ) so by lower semi-continuity (34) D(v) 2 L 2 ((0,t)×R 3 ) ≤ lim inf

ε k →0 t 0 D(v ε k ) 2 L 2 (R 3 \B(hε k (t),ε k )) .
We also observe at this point that the strong L 2 convergence of v ε (0) towards v 0 gives that (35) v 0 L 2 = lim inf

ε k →0 v ε k (0) L 2 .
Finally, taking the lim inf

ε k →0
in [START_REF] Lacave | Small Moving Rigid Body into a Viscous Incompressible Fluid[END_REF] and using (33), ( 34) and (35) implies the required energy inequality [START_REF] San Martín | Global Weak Solutions for the Two-Dimensional Motion of Several Rigid Bodies in an Incompressible Viscous Fluid[END_REF]. This completes the proof of Theorem 3.

Remark 1. We end this paper with a final remark about the weak time continuity assumed in Theorem 3: v ε ∈ C 0 w (R + ; L 2 (R 3 )). We know that u ε ∈ C 0 w (R + ; L 2 (R 3 )) so we made this hypothesis for the sake of simplicity, but it is in fact not necessary to make such an assumption. Indeed, we used it to make sense of the various terms of the form R 3 v ε (t, x) • ϕ ε (t, x) dx, see for instance on page 11. But the Navier-Stokes equation itself implies a time-continuity property allowing to make sense of such terms. More precisely, let us make a change of variables to go to a fixed domain. The vector field v ε (t, x) = v ε (t, x -h ε (t)) verifies the following PDE:

(36) ∂ t v ε + h ε • ∇ v ε -ν∆ v ε + v ε • ∇ v ε = -∇ π ε for |x| > ε
where π ε (t, x) = π ε (t, x -h ε (t)). Since v ε ∈ L ∞ loc (R + ; L 2 (R 3 )) ∩ L 2 loc (R + ; H 1 (R 3 )) we also have that v ε ∈ L ∞ loc (R + ; L 2 (R 3 )) ∩ L 2 loc (R + ; H 1 (R 3 )). Recalling that h ε is Lipschitz, we infer by classical estimates that

h ε • ∇ v ε -ν∆ v ε + v ε • ∇ v ε ∈ L 4 3
loc (R + ; H -1 (R 3 )). So, if we choose some Φ ∈ C ∞ 0,σ (|x| > ε) and we multiply (36) by Φ, the pressure goes away and we obtain that

| ∂ t v ε , Φ | = | h ε • ∇ v ε -ν∆ v ε + v ε • ∇ v ε , Φ | ≤ h ε • ∇ v ε -ν∆ v ε + v ε • ∇ v ε H -1 Φ H 1 .
If we denote by X the dual of C ∞ 0,σ (|x| > ε) for the H 1 norm, the relation above implies that

∂ t v ε X ≤ h ε • ∇ v ε -ν∆ v ε + v ε • ∇ v ε H -1 so ∂ t v ε ∈ L 4 3
loc (R + ; X). In particular v ε ∈ C 0 (R + ; X). We infer that v ε (t, •) • Φ is welldefined for all t ≥ 0 and Φ ∈ C ∞ 0,σ (|x| > ε). Going back to the original variables, we infer that if ϕ ε ∈ C ∞ 0,σ (|x -h ε (t)| > ε) then v ε (t, •) • ϕ ε is well-defined.

3 2

 3 h ε (t) → 0 strongly in L ∞ (R + ) when ε → 0. Then all the hypothesis of the first part of Theorem 3 is verified and the first part of Theorem 2 follows.

(0, T ; L 2 loc ) ⊂ L 2 (0, T ; L 2 loc ) completes the proof of Proposition 1.

Acknowledgments J.H. and D.I. have been partially funded by the ANR project Dyficolti ANR-13-BS01-0003-01. D.I. has been partially funded by the LABEX MILYON (ANR-10-LABX-0070) of Université de Lyon, within the program "Investissements d'Avenir" (ANR-11-IDEX-0007) operated by the French National Research Agency (ANR).