DYNAMICS OF RIGID BODIES IN A TWO DIMENSIONAL INCOMPRESSIBLE PERFECT FLUID

Transcription

1 DYNAMICS OF RIGID BODIES IN A TWO DIMENSIONAL INCOMPRESSIBLE PERFECT FLUID OLIVIER GLASS, CHRISTOPHE LACAVE, ALEXANDRE MUNNIER, AND FRANCK SUEUR Abstract. We consider the motion of several rigid bodies immersed in a two-dimensional incompressible perfect fluid, the whole system being bounded by an external impermeable fixed boundary. The fluid motion is described by the incompressible Euler equations and the motion of the rigid bodies is given by Newton s laws with forces due to the fluid pressure. We prove that, for smooth solutions, Newton s equations can be recast as a second-order ODE for the degrees of freedom of the rigid bodies with coefficients depending on the fluid vorticity and on the circulations around the bodies, but not anymore on the fluid pressure. This reformulation highlights geodesic aspects linked to the added mass effect, gyroscopic features generalizing the Kutta-Joukowski-type lift force, including body-body interactions through the potential flows induced by the bodies motions, body-body interactions through the irrotational flows induced by the bodies circulations, and interactions between the bodies and the fluid vorticity. 1. Introduction We consider the motion of rigid bodies immersed in a two-dimensional incompressible perfect fluid. The whole system occupies a fixed impermeable bounded cavity Ω a bounded simply connected open subset of R 2. At the initial time, the domain occupied by the rigid bodies are assumed to be disjoint non-empty regular connected and simply connected compact sets S,0 Ω, with {1, 2,..., N}, and F 0 := Ω \ S,0, {1,2,...,N} The rigid motion of the solid is described at every moment by a rotation matrix [ ] cos θ t sin θ Rθ t := t, θ sin θ t cos θ t t R, and by the position h t R 2 of its center of mass starting with the initial position h,0. The domain of the solid at every time t > 0 is therefore S t := Rθ ts,0 h,0 + h t, while the domain of the fluid is Ft := Ω \ S t. {1,2,...,N} Date: February 17,

2 2 OLIVIER GLASS, CHRISTOPHE LACAVE, ALEXANDRE MUNNIER, AND FRANCK SUEUR The system is governed by the following set of coupled equations: Fluid equations: 1.1a u + u u + π = 0 t in Ft, for t > 0, 1.1b div u = 0 in Ft, for t > 0, 1.1c 1.1d 1.1e 1.1f 1.1g 1.1h Solids equations: for any {1, 2,..., N}, m h t = u t=0 = u 0 in F 0, J θ t = = h 0, θ 0, h 0, θ 0 Boundary conditions: and for any {1, 2,..., N}, S t S t πn ds, for t > 0, x h t πn ds, for t > 0, h,0, 0, l,0, r,0, u n = 0 on Ω, for t > 0, u n = θ h + h n on S t, for t > 0. These are respectively the incompressible Euler equations, the Newton s balance law for linear and angular momenta of each body and impermeable boundary conditions. Above u = u 1, u 2 t and π denote the velocity and pressure fields in the fluid, m > 0 and J > 0 denote respectively the mass and the moment of inertia of the body while the fluid is supposed to be homogeneous of density 1, to simplify the notations. The exponent t denotes the transpose of the vector. When x = x 1, x 2 t the notation x stands for x = x 2, x 1 t, n denotes the unit normal vector pointing outside the fluid, so that n = τ, where τ denotes the unit counterclockwise tangential vector on S t and the unit clockwise tangential vector on Ω. Let us also emphasize that we will use ds as length element without any distinction on Ω, St and on S,0. We will use the notations q and q for vectors in R 3 gathering both the linear and angular parts of the position and velocity: q := h t, θ t and q := h t, θ t. The vectors q and q are next concatenated into vectors of length 3N: q = q t 1,..., qt N t and q = q 1 t,..., q N tt, whose entries are relabeled respectively q k and q k with k ranging over {1,..., 3N}. Hence we have also: q = q 1, q 2,..., q 3N t and q = q 1, q 2,..., q 3N t. Consequently, k {1,..., 3N} denotes the datum of both a solid number and a coordinate in {1, 2, 3} so that q k and q k denote respectively the coordinate of the position and of the velocity of a given solid. More precisely, for all k {1,..., 3N}, we denote by k the quotient of the Euclidean division of k 1 by 3, [k] = k + 1 {1,..., N} denotes the number of the solid and k := k 3 k {1, 2, 3} the considered coordinate. Throughout this paper we will not consider any collision, then we introduce the set of body positions without collision: Q := {q R 3N : min ν ds q, Ω c S ν q > 0}, where d is the Euclidean distance. The fluid domain is then totally described by q Q: Ft = Fqt. The fluid vorticity ω is defined by ω := curl u = 1 u 2 2 u 1 and we set γ := γ =1,...,N, where γ := S u τ ds is the circulation around the rigid body S. Let us recall that, for each, the circulation γ remains constant over time according to Kelvin s theorem.

3 RIGID BODIES IN 2D EULER 3 To state our result let us introduce a few more notations. We denote by S ++ 3N R the set of real symmetric positive-definite 3N 3N matrices and by BL s R 3N R 3N ; R 3N the space of bilinear symmetric mappings from R 3N R 3N to R 3N. Definition 1.1. Given a C mapping q Q Mq S 3 ++ R, we say that the C mapping q Q Γq BL s R 3N R 3N ; R 3N is the connection associated with this mapping if for any p R 3N, Γq, p, p := Γq k i,jp i p j 1 k 3N R3N, 1 i,j 3N with for every i, j, k {1,..., 3N}, Γq k i,j := 1 Mqi,k 2 q j + Mq j,k q i Mq i,j. q k Let us emphasize that the coefficients Γ k i,j are the Christoffel symbols of the first kind associated with the metric Mq. The main result of this paper is the following reformulation of the dynamics of the rigid bodies as a second-order differential equation for q with respect to the fluid vorticity and the circulations around the bodies, but without any reference to the fluid velocity nor the pressure. Theorem 1.2. There exist a C mapping q Q Mq S ++ 3N R, which depends only on the shape of Fq, on the masses m 1,...,N and on the moments of inertia J 1,...,N, and a C mapping on Q which associates with q in Q the mapping F q, from R 3N C Fq R N to R 3N such that F q,, 0, 0 = 0, which depends only on the shape of Fq, such that if u and q are smooth functions which satisfy System 1.1, then, up to the first collision, q satisfies the second order ODE: 1.2 Mqq + Γq, q, q = F q, q, ω, γ, where Γ is the connection associated with q Mq. In the case where the vorticity and the circulations vanish, then the right hand side of 1.2 also vanishes and the equation then reduces to the geodesic equation associated with the metric Mq. This case was already treated in [9]. The matrix Mq is associated with the added mass effect. A well-known formula with respect to the so-called Kirchhoff potentials is recalled in Section 3.1. On the other hand some computations of the Christoffel symbols are given in [9, Lemma 6.3]. Some alternative formulas are given in Section 5. When the vorticity and the circulations are nonzero the force F in the right hand side of 1.2 has to be taken into account. In Section 3 we give a more explicit expression of this force F, see 3.5, which displays gyroscopic features generalizing the Kutta-Joukowski-type lift force and reads as a non-linear coupling between body-body interactions through the potential flows that their velocity induces, body-body interactions through the irrotational flows that their circulation induces, and body-vorticity interactions. This reformulation extends the works [3] and [4] where the case of one rigid body in an unbounded rotational flow was addressed and the work [5] where the case of one rigid body in a bounded irrotational flow was tackled. Let us mention two motivations for the result above. The first one is the zero-radius limit as considered in [3], [4], [5] in more simple settings. Another one is related to the controllability of the motion of the rigid bodies from a part of the external boundary, see [2] for the case of a single rigid body. Regarding the issue of collisions we refer to [6], [7] and the recent paper [1].

4 4 OLIVIER GLASS, CHRISTOPHE LACAVE, ALEXANDRE MUNNIER, AND FRANCK SUEUR The remainder of this article is divided into four Sections. We first determine the fluid velocity u in terms of q, q, ω, γ in Section 2. In Section 3, we give the explicit formulas of M, Γ, F which appear in 1.2. Section 4 is dedicated to the proof of Theorem 1.2 whereas Section 5 contains the proof of an explicit formula concerning Γ. Finally Section 6 is devoted to the proof of Proposition 3.1 which highlights a property of a part of the force F due to the circulations around the body. 2. Decomposition of the fluid velocity into elementary velocities In this section, we determine the fluid velocity u in terms of q, q, ω, γ. This material follows from well-known property of incompressible flows in multiply-connected domains. We refer in particular to Kato [8] for more details. Kirchhoff potentials. Consider for any {1, 2,..., N}, the functions ξ,j q, = ξ k q,, for j = 1, 2, 3 and k = j, defined by ξ,j q, x := 0 on Fq \ S and by ξ,j q, x := e j, for j = 1, 2, and ξ,3 q, x := x h on S. Above e 1 and e 2 are the unit vectors of the canonical basis. We denote by K,j q, = K k q, the normal trace of ξ,j on Fq, that is: K,j q, := n ξ,j q, on Fq, where n denotes the unit normal vector pointing outside Fq. We introduce the Kirchhoff potentials ϕ,j q, = ϕ k q,, for j = 1, 2, 3 and k = j, which are the unique up to an additive constant solutions in Fq of the following Neumann problem: 2.1a 2.1b We also denote ϕ,j = 0 ϕ,j q, = K,jq, in Fq, on Fq. 2.2 K q, := K,1 q,, K,2 q,, K,3 q, t and ϕ q, := ϕ,1 q,, ϕ,2 q,, ϕ,3 q, t. Following our rules of notation for q, we define as well the function ϕq, by concatenating into a vector of length 3N the functions ϕ q,, namely: ϕq, := ϕ 1 q, t,..., ϕ N q, t t. Stream functions for the circulation. To take into account the circulations of the velocity around the solids, we introduce for each {1,..., N} the stream function ψ = ψ q, defined on Fq of the harmonic vector field which has circulation δ,ν around S ν q. More precisely, for every q, there exists a unique family C,ν q ν {1,2,...,N} R N such that the unique solution ψ q, of the Dirichlet problem: 2.3a 2.3b 2.3c ψ q, = 0 ψ q, = C,ν q ψ q, = 0 in Fq on S ν q, for ν {1, 2,..., N}, on Ω, satisfies 2.3d S νq ψ q, ds = δ,ν, for ν {1, 2,..., N}, where δ ν, denotes the Kronecker symbol. As before, we define the concatenation into a vector of length N: ψq, := ψ 1 q,,..., ψ N q, t.

5 RIGID BODIES IN 2D EULER 5 Hydrodynamic stream function. For every smooth scalar function ω over Fq, there exists a unique family C ω,ν q ν {1,2,...,N} R N such that the unique solution ψ ω q, H 1 Fq of: 2.4a 2.4b 2.4c satisfies 2.4d ψ ω q, = ω ψ ω q, = C ω,ν q ψ ω q, = 0 S νq in Fq on S ν q, for ν {1, 2,..., N}, on Ω, ψ ω q, ds = 0, for ν {1, 2,..., N}. Then the decomposition of the fluid velocity u is given by the following result. Proposition 2.1. Let q Q. For any q in R 3N, for any ω smooth over Fq and for any γ in R N, there exists a unique smooth vector field u such that div u = 0 in Fq, curl u = ω in Fq, u n = 0 on Ω, u n = θ h + h n on S t and ut τ ds = γ, for all {1, 2,..., N}. Moreover, we have the decomposition S t 2.5 u = u 1 q, q, + u 2 q, ω, γ,, with u 1 q, q, := N ϕ q, q = =1 N 3 ϕ,j q, q,j = =1 j=1 3N k=1 q k ϕ k, u 2 q, ω, γ, := ψ ω,γ q,, where ψ ω,γ q, := ψ ω q, + ψq, γ. 3. Explicit formulas of the coefficients in the reformulation of the dynamics of the rigid bodies In this section we give some explicit expressions of the quantities Mq and F q which are involved in 1.2. These expressions give more insights on the various effects involved in the dynamics of the rigid bodies Inertia matrices. Let us gather the mass and moment of inertia of the solid into the following matrix: M g := m m J The total genuine inertia matrix of the system is the 3N 3N bloc diagonal matrix: 3.1 M g := diagm g 1,..., Mg N. which is diagonal and in the set S ++ 3N R of the real symmetric positive definite 3N 3N matrices. In addition to their genuine inertia the rigid bodies have also to accelerate the surrounding fluid as they move through it. This is the phenomenon of added inertia, which is encoded by the matrices: 3.2 M a,νq := ϕ ν q, ϕ q, dx = ϕ q, ϕ ν q, dx. S q S νq

6 6 OLIVIER GLASS, CHRISTOPHE LACAVE, ALEXANDRE MUNNIER, AND FRANCK SUEUR The total added inertia matrix of the system reads: 3.3 M a q := M a,νq 1,ν N = Fq ϕq, ϕ q, dx. Notice that this matrix is in the set S + 3N R of the real symmetric positive-semidefinite 3N 3N matrices. These matrices depend on the shape of the fluid domain, therefore on the shape of the external boundaries and of the shape and position of the rigid bodies. Finally, the overall inertia of the system is encoded in the inertia matrix: 3.4 Mq := M g + M a q S ++ 3N R Force term. From the stream function ψ ω,γ associated with ω, γ 2.7, and the Kirchhoff potentials , we define: ψ ω,γ ϕ A,ν q, ω, γ := q, S q ϕ ν q, ds ψ ω,γ ϕ q, S νq ϕ ν q, ds, Aq, ω, γ := A,ν q, ω, γ 1,ν N. We observe that the matrix A is skew-symmetric and linear with respect to ω and γ. With this matrix we associate the gyroscopic force Aq, ω, γq which generalizes the celebrated Kutta-Joukowski force, see for instance [10]. We also define: Finally we set E q, ω, γ := 1 2 S q ψ ω,γ 2 ϕ q, ds, Eq, ω, γ := E 1 q, ω, γ,..., E N q, ω, γ t, D k q, q, ω, γ := ωu q, q, ω, γ, x ϕ k q, dx, Fq Dq, q, ω, γ := D 1 q, q, ω, γ,..., D 3N q, q, ω, γ t. 3.5 F q, q, ω, γ := Eq, ω, γ + Aq, ω, γq + Dq, q, ω, γ. It follows from the definitions and properties of the elementary flows given in the previous section that the mapping which associates with q in Q the mapping F q, from R 3N C Fq R N to R 3N is C, such that F,, 0, 0 = 0, and depends only on the shape of Fq. Moreover, without vorticity, we can compute E in terms of the shape derivatives of the constants C,ν q appearing in the definition of the stream functions for the circulation terms 2.3. Proposition 3.1. For any q in Q and for any γ in R N, Eq, 0, γ = 1 2 q N N m=1 ν=1 γ γ ν C,ν q.

7 RIGID BODIES IN 2D EULER 7 4. Proof of the main result This section is devoted to the proof of Theorem 1.2. For each integer between 1 and N, q Q, l R 2 and r k R, we consider the following potential vector field Fq: u := ϕ q, p where p := l t, r t. By 2.1a, 4.1 u n = δ,ν l + r h n on S ν q and u n = 0 on Ω, Combining with 1.1d and 1.1e, we arrive at 4.2 m h l + J θ r = Fq πu n ds. Since, by 2.1b, u is divergence-free in Fq, with an integration by parts we arrive at m h l + J θ r = π u dx. Since, by 1.1a, Fq u π = t u2 + ωu we deduce from 4.2 that m h l + J θ r = Fq in Fq, u t u 2 + ωu u dx. Summing over all the and using the decomposition 2.5 therefore yields M g q p u1 + Fq t u 1 2 u 1 dx = Fq 2 u 2 2 u dx u 2 Fq t + u 1 u 2 u dx ωu u dx, for all p R 3N, where 4.3 u := 1 N We also recall that M g is defined in 3.1. The lemma below is proved in [9, Lemma 5.1]. Lemma 4.1. For any smooth curve qt in Q and every p R 3N, the following identity holds: M g q p u1 + t u 1 2 u dx = Mqq p + Γq, q, q p, Fq where M is given in 3.4 and Γq is the connection associated with q Mq. u. Fq Before moving on we recall that the definitions of Eq, ω and Aq, ω are given in the previous section. As u 2 = u 2 τ on the boundary, by an integration by parts, we have the following. Lemma 4.2. For every q Q and every p R 3N, the following identity holds: 1 2 u 2 2 u dx = Eq, ω p, where u is given by 4.3. Fq

8 8 OLIVIER GLASS, CHRISTOPHE LACAVE, ALEXANDRE MUNNIER, AND FRANCK SUEUR On the other hand, we have the following result regarding the crossed term. Lemma 4.3. For any smooth curve qt in Q and every p R 3N, the following identity holds: u 2 t + u 1 u 2 u dx = Aq, ω, γq p, where u is given by 4.3. Fq Proof. By an integration by parts, u Fq t u dx = ν S νq t ψ ω,γq, u τ ds. Now we use the following lemma where we set C ω,γ,ν := C ω,ν + N =1 γ C,ν. Lemma 4.4. For any smooth curve qt in Q, for any ν, on S ν q: t ψ ω,γq, = ψ ω,γ ϕν q, q, q ν + C ω,γ,ν q q + δc ω,ν ω q q δω t. Let us stress that δcω,ν ω δω q t denotes the functional derivative of C ω,ν with respect to ω, so that the last term is constant on S ν q as a function of x. Proof of Lemma 4.4. By Kelvin s theorem, we consider only solutions such that γ t = 0, and we start with the observation that 4.5 t ψ ω,γq, = ψ ω,γ q + δψ ω,γ ω q, q δω t. By differentiating with respect to t the identity: ψ ω,γ q, Rθ ν X h ν,0 + h ν = C ω,γ,ν q, for X S ν,0, and by setting x = Rθ ν X h ν,0 + h ν, we obtain for every x S ν q, 4.6 ψ ω,γ q q, x q + δψ ω,γ ω q, x δω t + xψ ω,γ q, x w ν q, x = C ω,γ,ν q q q + δc ω,ν δω ω q t, where w ν q, x = θ νx h ν + h ν. Since ψ ω,γ q, is constant on S ν q, its tangential derivative is zero. Besides, on S ν q we have w ν q, n = ϕ ν q, q ν. Thus we get 4.7 ψ ω,γ q, x w ν q, x = ψ ω,γ q, x ϕ ν q, x q ν for x S ν q. By combining 4.5, 4.6 and 4.7 we conclude the proof of Lemma 4.4. By 4.4 and Lemma 4.4, we get u 2 N N 4.8 t u dx = Fq =1 ν=1 S νq ψ ω,γ ϕ ϕ ν ds q ν p. Let us stress here that the last two terms in the equality of Lemma 4.4 are constant so that their contribution in 4.4 vanish since S νq u τ ds = 0. On the other hand, since u is divergence-free, we have the Stokes formula: u 1 u 2 u dx = u 1 u 2 u n ds. Fq By , we have on S q, Fq u 1 u 2 = u 1 τu 2 τ = N ν=1 ϕ ν ψ ω,γ q ν,

9 RIGID BODIES IN 2D EULER 9 hence we obtain by 4.1 that 4.9 u 1 u 2 u dx = Fq N =1 ν=1 N S q ψ ω,γ Gathering 4.8 and 4.9, we end the proof of Lemma 4.3. ϕ ϕ ν ds q ν p. Combining Lemmas 4.1, 4.2, 4.3, observing that ωu u dx = Dq, q, ω p Fq and taking 3.5 into account, we arrive at 1.2 since p can be arbitrarily chosen in R 3N. This concludes the proof of Theorem Computation of the Christoffel symbols This section is devoted to the proof of the following result regarding the computations of the Christoffel symbols. Proposition 5.1. For every integers i, j, k between 1 and 3N, M a i,j q ] = [ξ i ϕ i ξ j ϕ j ξ i ξ j ξ k n ds. q k S [k] q δ 3,i δ [k],[i] δ {1,2},k ϕ j ξ k τds δ 3,j δ [k],[j] δ {1,2},k S [k] q S [k] q ϕ i ξ k τds. Observe that the formula above does not involve the curvature of the fluid domain as opposed to [9, Lemma 6.3]. Proof. Let {1,..., N}, p = l t, r t R 3, q Q and ξ be a smooth divergence-free vector field such that ξ x = r x h + l in a neighborhood of S k q and ξ x = 0 elsewhere. Define the diffeomorphism T t, for t small as being the flow, corresponding to the Cauchy problem: T t t, x = ξ T t, x, T 0, x = x. Notice that we have: T t 0, x = ξ x. Define now the sets Ft := T t, Fq, S µ t := T t, S µ q for all µ = 1,..., N noting that S µ is fixed for µ and, for every t small and every i {1,..., 3N}, and the Kirchhoff potentials t ϕ i t, i=1,...,3n on Ft, see 2.1. The shape derivative of the Kirchhoff potential ϕ i i = 1,..., 3N at the point q in the direction p = l t, r t = 1,..., N, is then defined by ϕi p q q, := ϕ i0,. Lemma 5.2. For q Q and p = l t, r t R 3, the following Neumann condition on Fq: [ ϕi ϕi 5.1 p ξ i τ q, = [ ] q ϕi ξ n ϕi q p q, is harmonic in Fq and satisfies ] ξ n δ 3,i l τ if = [i], if [i],

10 10 OLIVIER GLASS, CHRISTOPHE LACAVE, ALEXANDRE MUNNIER, AND FRANCK SUEUR where ξ = r h + l. Proof. Differentiating with respect to t at every point x in Fq the identity ϕ i t, x = 0 we get ϕ i 0, x = 0. The boundary condition 2.1b can be rewritten, after a change of variables, as: 5.2 ϕ i t, T t, x nt, T t, x = K i t, T t, x nt, T t, x on S q, where nt, is the unit normal vector to Ft directed towards the exterior of Ft. Notice now that nt, T t, = Rtr n0, and hence that: 5.3 We deduce in particular that, when [i] = : 5.4a because on S and obviously, when [i] : 5.4b t 0, = r τ0, on S q. d dt K it, T t, nt, T t, t=0 = { r e i τ if i = 1, 2, 0 if i = 3, d T t, x T t, h t=0 nt, T t, dt = 0, d dt K it, T t, nt, T t, t=0 = 0. Differentiating now 5.2 with respect to t and using 5.3 and 5.4 we obtain: ϕ i 5.5 0, + D2 ϕ i 0, n ξ r ϕ 0 if [i] i 0, = r e i τ if = [i], i = 1, 2, 0 if = [i], i = 3. where D 2 ϕ i 0, is the Hessian matrix of ϕ i 0,. On the one hand, let us now decompose ξ into 5.6 ξ = ξ nn + ξ ττ on S q. On the other hand, computing the tangential derivative of the boundary condition 2.1b on S q, we get: 5.7 D 2 ϕ i 0, n τ = H ϕ 0 if [i] i 0, + He i τ if = [i], i = 1, 2, 1 H h τ if = [i], i = 3, where H is the local curvature of Fq defined by whence we deduce that: D 2 ϕ i 0, n n H ϕ i 0, + = Hτ on Fq. On Fq, we also have: 0, = ϕ i 0, = 0, ϕi 5.8 D 2 ϕ i 0, n n = H ϕ i 0, ϕi 0,.

11 RIGID BODIES IN 2D EULER 11 Plugging the decomposition 5.6 into 5.5 and using the equalities 2.1b, 5.7 and 5.8, we get: ϕ [ i 0, = ξ n ϕi 0, + r Hξ τ ϕ ] i 0, 0 if [i] + r + Hξ τe i τ He i nξ n if = [i], i = 1, 2, r + Hξ τ h k τ H h k nξ n l τ if = [i], i = 3. Observe now that: and the result follows. ξ n = r Hξ τ on S q, With the same notation as above, we can now compute the shape derivatives of the entries of the added mass matrix 3.3. Lemma 5.3. The following identity holds true for every i, j {1,..., 3N}, {1,..., N}: M a ij p q = ϕi ϕ j ϕ i ξ j ϕ j ξ i ξ q n ds S q δ 3,i δ,[i] ϕ j l τds δ 3,j δ,[j] ϕ i l τds. S q where we recall that p = l t, r t and ξ = r h + l. Proof. The quantity we are interested in is the derivative at t = 0 of: M a ijt := ϕ i ϕ j dx. Ft The proof relies on Reynold s transport theorem which reads: d dt Ma ij0 := ϕ i ϕ j + ϕ i ϕ j dx + Fq S q S q ϕ i ϕ j ξ nds. We now use the expression 5.1 and integrate by parts on the boundary. We obtain: d ϕ i ϕ j ϕ i dt Ma ij0 := ξ nds + ξ j τξ n ds We write ϕ i ϕ j and the conclusion follows. + S q S q δ 3,i δ,[i] ϕ j ξ i τξ nds + S q = ϕ i ϕ j ϕ i S q S q ϕ j l τds δ 3,j δ,[j] ϕ j, ϕ j ξ i τ = ϕ j ξ i ϕ j ξ i n, Using now the expressions in Lemma 5.3 we get Proposition 5.1. ϕ i ϕ j ξ n ds S q ϕ i l τds. ϕ i ξ j τ = ϕ i ξ j ϕ i ξ j n,

12 12 OLIVIER GLASS, CHRISTOPHE LACAVE, ALEXANDRE MUNNIER, AND FRANCK SUEUR 6. Proof of Proposition 3.1 This section is devoted to the proof of Proposition 3.1. We first observe that Lemma 4.4 can be adapted to determine the shape derivative of the stream function ψ m in terms of the shape derivatives of the constants C m,ν associated with the boundaries S ν, for ν in {1,..., N}. Lemma 6.1. For, µ in {1,..., N}, for any p in R 3 ψµ, q p q, is harmonic in Fq and satisfies for ν in {1,..., N}, 6.1 ψµ q p q, = C µ,νq p ψµ q ϕ q, p on S ν. Then, using the expression of E when ω = 0, see 3.2, we deduce Proposition 3.1 from the following lemma, whose proof relies on Lemma 6.1. Lemma 6.2. For every µ, ν, in {1,..., N}, for every p = l t, r t in R 3, Cµ,ν p ψ µ ψ ν q = q S q ξ n ds, where ξ = r h + l. Proof. We first observe that for every µ, ν in {1,..., N}, C µ,ν q = ψ µ ψ ν dx. Fq By Reynold s transport theorem, for every in {1,..., N}, for every p = l t, r t in R 3, Cµ,ν p q = ψ µ p q Fq q ψ ν + ψ µ ψ ν p q dx ψ µ ψ ν ξ nds, S q where ξ = r h + l. By integrations by parts and Lemma 6.1, since the first term in the right hand side term of 6.1 is constant, Cµ,ν p Cµ,ν q =2 p ψµ ϕ q + q, p ψ ν q q S q ds ψν ϕ + q, p ψ µ ds ψ µ ψ ν ξ n ds, S q S q and the conclusion follows. Acknowledgements. The authors are partially supported by the Agence Nationale de la Recherche, Project IFSMACS, grant ANR-15-CE The first, second and last authors are partially supported by the Agence Nationale de la Recherche, Project SINGFLOWS grant ANR-18-CE The fourth author is partially supported by the Agence Nationale de la Recherche, Project BORDS, grant ANR-16-CE , the Conseil Régionale d Aquitaine, grant CP, by the H2020- MSCA-ITN-2017 program, Project ConFlex, Grant ETN

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