The Magnetic Spherical Pendulum
|
|
- Charla Rodgers
- 6 years ago
- Views:
Transcription
1 The Magnetic Spherical Pendulum R. Cushman L. Bates Abstract This article gives two formulae for the rotation number of the flow of the magnetic spherical pendulum on a torus corresponding to a regular value of the energy momentum mapping. One of these formulae is nonclassical and is based on an idea of Montgomery. In questo lavoro si danno due formule per il numero di rotazione del flusso del sferico pendolo magnetico su un toro che corrisponde a un valore regolare dell applicazione energia-momento. Una di queste formule è nonclassica ed è basata su un idea di Montgomery. In this article we look at the problem of computing a rotation number for the flow of the magnetic spherical pendulum. Mechanically, the magnetic spherical pendulum is the motion of a charged massive particle constrained to a sphere. The forces on the particle come from a gravitational field and a magnetic field due to a magnetic monopole located at the center of the sphere. At first sight this problem may seem obscure, if not baroque, but actually it is a mechanical model for the motion of the vertex of the Lagrange top (recall that the Lagrange top is the symmetrical top spinning in a gravitational field about a fixed point on its symmetry axis.) Geometrically, the magnetic spherical pendulum arises as a reduction of the Lagrange top by reducing out the symmetry about the body axis, and the value of angular momentum that we reduced by manifests itself as the strength of the magnetic field. We will give a fast heuristic derivation of this using Euler angles. It is interesting and more rigorous to do the calculation in an invariant manner, but we will not do so here for the sake of brevity. Keywords completely integrable system, particle mechanics
2 A Lagrangian for the top is L = 2 A( φ 2 + sin 2 φ θ 2 ) + 2 C( ψ + cos φ θ) 2 cos φ The notation is such that A and C are the moments of inertia, φ is the colatitude, θ is the longitude, and ψ is the rotation of the top about its symmetry axis. The Euler-Lagrange equations are d (A sin2 φ θ + C( ψ + cos φ θ) cos φ) = (A φ A sin φ cos φ θ 2 + C( ψ + cos φ θ) sin φ θ + sin φ = d (C( ψ + cos φ θ)) = Because of the third equation, set p ψ = L = j. Now j is a constant of ψ motion because ψ is an ignorable coordinate. Substitute this value of j into the first two Euler-Lagrange equations to obtain Note that the energy d (A sin2 φ θ + j cos φ) = A φ A sin φ cos φ θ 2 + j sin φ θ + sin φ = E = 2 A( φ 2 + sin 2 φ θ 2 ) + cos φ is a constant of motion for this reduced problem. Pushing everything over to the cotangent bundle by the Legendre transformation p θ = A sin 2 φ θ p φ = A φ we arrive directly at the Hamiltonian description with Hamiltonian h = 2A (p φ 2 + sin 2 φ p θ 2 ) + cos φ 2
3 and symplectic form ω = j sin φ dφ dθ + dθ dp θ + dφ dp φ. It is a simple calculation to check that the Hamiltonian equations of motion are what we get by pushing over the reduced Euler-Lagrange equations by the Legendre transformation. By inspection of the above two equations, one sees the validity of the mechanical interpretation of the motion of the vertex of the top which we gave at the beginning. Liouville integrability and reduction In this section we reduce out the axial symmetry of the magnetic spherical pendulum by using singular reduction []. We use this technique because it allows us to reduce at all values of the angular momentum. This means that our reduction captures those motions of the vertex of the top which pass through the north or the south pole as well as the motions corresponding to regular precession. These motions are physically interesting and are not susceptible to analysis using action angle variables. The reason for this is that the Liouville integrablility thorem, in its modern formulation by Arnol d [2], requires functional independence of the integrals. In addition, we explicitly realize each of the reduced spaces as an semialgebraic variety in R 3 with an explicit Poisson structure. As a byproduct of the invariant theoretic technique used in constructing the reduced space, we obtain a faithful geometric model of the singularities and how the reduced spaces fit together as the angular momentum is varied. We start by describing the magnetic spherical pendulum as a constrained Hamiltonian system. On R 3 let, be the Euclidean inner product and be the usual vector product. Define a 2-form Ω on the bundle π : T R 3 R 3 by Ω(x, y)((u, v), (r, s)) = dθ + µπt R3F () = v, r + s, u + µ x x 3, u r. Ω is the standard symplectic form dθ on T R 3 plus a term µf, which is the magnetic field of a monopole of strength µ located at the origin of R 3. It is 3
4 straightforward to check that Ω is symplectic. Suppose that H : T R 3 R is a smooth function. Then a short calculation shows that the Hamiltonian vector field X H associated to H is dx dy = H y = H x + µ x x 3 H y. (2) where On T R 3 define an S action Φ : S T R 3 T R 3 : (x, y) (R t x, R t y) (3) R t = cos t sin t sin t cos t. The infinitesimal generator of this S action is the vector field dx dy = x e 3 = y e 3. (4) Using (2), another short calculation shows that the Hamiltonian vector field X J corresponding to the Hamiltonian function J : T R 3 R : (x, y) x y, e 3 + µ x x, e 3 (5) is also given by (4). Thus J is the momentum mapping of the S action Φ. Consider the submanifold T S 2 T R 3 defined by F (x, y) = x, x = F 2 (x, y) = x, y =. Since the 2 2 matrix ({F i, F j } T S 2 ) = ( 2 2 ) 4
5 is invertible (see table for the structure matrix of {, } T R 3), T S 2 is a symplectic submanifold of T R 3. Therefore Ω T S 2 is a symplectic form on T S 2. The magnetic spherical pendulum is the Hamiltonian system (T R 3, Ω, H) with Hamiltonian H : T R 3 R : (x, y) 2 y, y + γ x, e 3 (6) constrained to (T S 2, Ω T S 2 ). In other words, it is the Hamiltonian system (T S 2, Ω T S 2, H T S 2 ). Using the Dirac prescription [3] we compute X H T S 2 as follows. Let H = H 2 {H, F 2} T R 3F + 2 {H, F } T R 3F 2 = 2 y, y + γ x, e 3 + 2( y, y γ x, e3 )( x, x ) x, y 2. Then using (2), X H dx dy on (T R 3, Ω) is = y + y( x, x ) 2 x, y x = γ e γ e 3( x, x ) ( y, y γ x, e 3 )x + 2 x, y y + µ x x 3 ( y + y( x, x ) 2 x, y x ). Since {H, F } T R 3 T S 2 = {H, F 2 } T R 3 T S 2 =, T S 2 is an invariant manifold of X H. Consequently, X H T S 2 = X H T S 2 is given by dx dy = y = γ e 3 + (γ x, e 3 y, y )x + µ x y. (7) Since H and T S 2 are invariant under Φ, L XJ T S 2 H T S 2 = {H, J } T R 3 T S 2 =, that is, J T S 2 is an integral of the magnetic spherical pendulum. Therefore, the magnetic spherical pendulum is Liouville integrable and has energy momentum mapping EM : T S 2 T R 3 R 2 : (x, y) (H T S 2 (x, y), J T S 2 (x, y)). 5
6 To remove the S symmetry defined by the S action Φ and reduce the magnetic spherical pendulum to a one degree of freedom Hamiltonian system, we use the technique of singular reduction []. To start with, the algebra of S invariant polynomials on T R 3 is generated by which satisfy the relation σ = x 3 σ 3 = y 2 + y2 2 + y3 2 σ 5 = x 2 + x 2 2 σ 2 = y 3 σ 4 = x y + x 2 y 2 σ 6 = x y 2 x 2 y σ σ 2 6 = σ 5 (σ 3 σ 2 2) σ 3 & σ 5. (8) Thus the space of S orbits T R 3 /S is the semialgebraic variety W defined by (8). Since T S 2 T R 3 is S invariant, the S orbit space T S 2 /S is the semialgebraic variety U defined by (8) together with σ 5 + σ 2 = σ 4 + σ σ 2 =. (9) Solving (9) for σ 4 and σ 5 and then substituting the result into (8) shows that the variety U is defined by σ 2 σ σ 2 6 = ( σ 2 )(σ 3 σ 2 2), σ & σ 3. () Since the S action has momentum mapping J T S 2, the reduced phase space M j = (J T S 2 ) (j)/s is the semialgebraic variety of U defined by () and σ 6 + µ σ = j. In other words, M j is the semialgebraic variety of R 3 defined by σ 3 ( σ 2 2 ) (j µσ ) 2 σ 2 2 =, σ & σ 3. () When j ±µ, the reduced space M j is diffeomorphic to R 2, being the graph of the function σ 3 = G(σ, σ 2 ) = (j µσ ) 2 + σ2 2, σ σ 2 <. When j = ±µ, M ±µ is not the graph of a function, because it contains a vertical line {(±,, σ 3 ) R 3 σ 3 } (see figure ). However M ±µ is still homeomorphic to R 2. 6
7 Figure. The reduced phase space M j. Since H T S 2 is S -invariant, it induces the Hamiltonian H j M j on the reduced space M j where H j : R 3 R : (σ, σ 2, σ 3 ) 2 σ 3 + γσ (2) This completes the reduction of the magnetic spherical pendulum to a one degree of freedom Hamiltonian system. What remains to be done is find Hamilton s equations for the reduced Hamiltonian H j M j. To do this we compute the Poisson structure on C (M j ) as follows. From the definition of the symplectic form Ω on T R 3 we obtain a Poisson bracket {, } T R 3 on C (T R 3 ), which is given by {f, g} T R 3 = i,j f g {ζ i, ζ j } T R 3, ζ i ζ j where (ζ,..., ζ 6 ) = (x, x 2, x 3, y, y 2, y 3 ) are coordinates on T R 3 and ({ζ i, ζ j }) is the skew symmetric structure matrix {, } T R 3 half of which is given in table. 7
8 {A, B} x x 2 x 3 y y 2 y 3 B x x 2 x 3 y µ x 3 x 3 µ x x 3 y 2 µ x 2 x 3 y 3 A Table. Structure matrix for {, } T R 3 Let (σ,..., σ 6 ) are coordinates on R 6. A straightforward calculation using table shows that C (R 6 ) has a Poisson bracket {, } R 6 half of whose skew symmetric structure matrix is given in table 2. {A, B} σ σ 2 σ 3 σ 4 σ 5 σ 6 B σ 2σ 2 2µ µ σ 2 σ x 3 6 σ x 3 5 2µ σ 3 σ x 3 σ 6 + 2σ2 2 2σ 3 4σ 4 2µ (σ x 3 σ 4 + σ 2 σ 5 ) σ 4 2σ 5 µ σ x 3 σ 5 σ 5 σ 6 A Table 2. Structure matrix for {, } R 6 Here x = σ 2 + σ5 2 Using table 2 it is easily shown that C = σ σ 2 6 σ 5 (σ 3 σ 2 2) and C 2 = σ 6 + µσ are Casimir elements of (C (R 6 ), {, } R 6), that is, for every f C (R 6 ), {C, f} R 6 = {C 2, f} R 6 =. Since W, the space of S orbits on T R 3, is the semialgebraic variety defined by C =, σ 3 & σ 5, the Poisson bracket on W has the same 8
9 structure matrix as the Poisson bracket on R 6. Because {σ 5 + σ 2, σ 4 + σ σ 2 } R 6 U = 2, U, the space of S orbits on T S 2, is a symplectic subvariety of W. Consequently, the Poisson bracket {, } U on U may be computed using the Dirac prescription: namely, for every f, g C (R 6 ) where {f U, g U} U = {f, g } R 6 U f = f 2 {f, σ 4 + σ σ 2 } R 6(σ 5 + σ 2 ) + 2 {f, σ 5 + σ 2 } R 6(σ 4 + σ σ 2 ) and similarly for g. Half of the skew symmetric structure matrix for {. } U is given in table 3. {A, B} σ σ 2 σ 3 σ 6 B σ σ 2 2σ 2 σ 2 2µσ 6 2σ σ 3 µσ 5 σ 3 2µσ 2 σ 6 A Table 3. The structure matrix for {, } U. The reduced space M j is the subvariety of U defined by C 2 = j. Since C 2 is a Casimir in (C (U), {, } U ), the Poisson bracket {, } Mj on M j has the same structure matrix as that give in table 3 with the last row and column deleted and σ 6 replaced by j µσ. This completes the construction of the Poisson structure on M j. It is easier to calculate in the ambient space R 3 with coordinates (σ, σ 2, σ 3 ) instead of on the reduced space M j. On C (R 3 ) define a Poisson bracket {, } R 3 half of whose skew symmetric structure matrix is given in table 4. {A, B} σ σ 2 σ 3 B σ σ 2 2σ 2 σ 2 2µ(j µσ ) 2σ σ 3 σ 3 A Table 4. The structure matrix for {, } R 3. 9
10 An inspection of table 4 shows that {σ i, σ j } R 3 = k ε ijk ψ σ k (3) where ψ(σ, σ 2, σ 3 ) = σ 3 ( σ 2 ) σ 2 2 (j µσ ) 2 and ψ = is the defining equation of M j. Since ψ is a Casimir element of (C (R 3 ), {, } R 3), the Poisson bracket {, } Mj on C (M j ) is obtained by restricting {, } R 3. From (3) it follows that for every f, g C (R 3 ) {f, g} R 3 = f g, ψ. Consequently, for h C (R 3 ) Hamilton s equations are dσ i = {σ i, h} R 3 = ( h ψ) i (4) for i =, 2, 3. Using (2) and (4), Hamilton s equations for the reduced Hamiltonian H j M j are dσ dσ 2 dσ 3 = σ 2 = γ( σ 2 ) + µ(j µσ ) σ σ 3 = 2γσ 2 (5) restricted to M j. Note that ψ is an integral of (5). We return to studying the energy momentum mapping EM. For fixed µ, the set Σ µ of critical values of EM is the same as the set of critical values of H j M j. These values (h, j) occur when the family of lines h = 2 σ 3 + γσ (6) in R 2 with coordinates (σ,, σ 3 ) intersects the curve {σ 2 = } M j given by = σ 3 ( σ 2 ) (j µσ ) 2 σ & σ 3 (7) at a point with multiplicity greater than one (see figure 2).
11 Figure 2. The critical points and values of H j {σ 2 = } M j. Solving (6) for σ 3 and then substituting the result into (7) shows that (h, j) Σ µ if and only if the polynomial V (σ ) = 2(h σ )( σ 2 ) (j µσ ) 2 (8) has a multiple root in [, ]. In other words, Σ µ is a µ = const. slice of a piece S of the discriminant locus of V. The piece S also occurs in the treatment of the Lagrange top [4], [5]. Now suppose that (h, j) is a regular value of EM and that EM (h, j) is nonempty. The line defined by (6) intersects M j {σ 2 = } in two geometrically distinct nonsingular points, whose abscissas are σ ± = x ± 3. Thus, in R 3 with coordinates (σ, σ 2, σ 3 ) the plane defined by (6) intersects M j in a smooth manifold (H j M j ) (h), which is diffeomorphic to a circle. From the reduction process we know that the (h, j)-level set of EM is an S bundle over the h-level set of H j M j. Because this level set bounds a 2-disc on M j, which is contractible, the bundle is trivial. Hence EM (h, j) is diffeomorphic to a 2-torus Th,j. 2 By construction, Th,j 2 is invariant under the flow of X H T S 2 and X J T S 2. A good way to vizualize Th,j 2 is to view it as some sort of bundle over its image under the projection π T S 2 : T S 2 T R 3 S 2 R 3 : (x, y) x
12 (see figure 3). In the following discussion we construct this bundle. By definition T 2 h,j T R 3 is given by the equations x 2 = x 2 + x x 2 3 = x y + x 2 y 2 + x 3 y 3 = 2 (y2 + y2 2 + y3) 2 + γx 3 = h x y 2 x 2 y + µ x 3 x Substituting the above equations into the identity gives = j. (9) (x y 2 x 2 y ) 2 + (x y + x 2 y 2 ) 2 = (x 2 + x 2 2)(y 2 + y 2 2) y 2 3 = V (x 3 ) = 2(h γx 3 )( x 2 3) (j µx 3 ) 2 (2) where x 3. Consequently, x 3 [x 3, x + 3 ] where V (x ± 3 ) = and < x 3 < x + 3 <, because (h, j) is a regular value of EM. Therefore the image of Th,j 2 under π T S 2 is contained in the annular piece A of S 2 defined by {x S 2 R 3 x 3 x 3 x + 3 }. Given x A, from (2) we find that y 3 = η V (x 3 ) where η 2 =. Solving for (y, y 2 ) gives x y 2 x 2 y = j µx 3 x y + x 2 y 2 = x 3 y 3 = ηx 3 V (x 3 ) y = [x x 2 2 (j µx 3 ) + ηx x 3 V (x 3 )] 3 y 2 = [ x x 2 2 (j µx 3 ) + ηx 2 x 3 V (x 3 )]. 3 Therefore for every x int A there are two points p ± T 2 h,j such that π T S 2(p ± ) = x; while for every x A, there is exactly one point p so that π T S 2(p ) = x. In other words, T 2 h,j is a pinched S bundle over A with bundle 2
13 projection π T S 2 Th,j. 2 The above argument shows that π T S 2 Th,j 2 has a fold singularity at every point on the two curves C ± = π T S ({x S 2 x 2 3 = x ± 3 }). Note that C + and C are each an orbit of X J T S 2 Th,j. 2 Figure 3. Image of T 2 h,j under π T S 2. 2 Two formulae for the rotation number In this section we derive two formulae for the rotation number of the flow of X H T S 2 on the 2-torus Th,j. 2 First we recall the definition of rotation number. Since (h, j) is a regular value of EM, d(h T S 2 ) and d(j T S 2 ) are linearly independent at every point of Th,j 2 = EM (h, j). Therefore X H T S 2 and X J T S 2 are linearly independent at every point of Th,j. 2 The curve C + on Th,j, 2 which is the image of the integral curve t ϕt (p) of X J T S 2 through p π T S ({x 2 3 = x + 3 }), is a cross section for the flow ϕt of X H T S 2 on Th,j 2 because 3
14 ) if q C +, then X H T S 2(q) is transverse to C + at q; and 2) since X H T S 2 does not vanish on Th,j, 2 there is a smallest T = T (p) > such that ϕt (p) C +. Let θ h,j be the smallest positive time such that ϕ θ h,j (p) = ϕ T (see figure 4). Then θ h,j is the rotation number of the flow of X H T S 2 on Th,j. 2 The rotation number does not depend on the choice of point p on C +. For if q C +, q p, then there is a smallest time S > such that ϕs (p) = q. Thus ϕ T (q) = ϕ = ϕ = ϕ T S S (ϕ S (p)) (p) (ϕt (p)), since [X H T S 2, X J T S 2] = (ϕ θ h,j (p)) = ϕ θ h,j which proves the claim. We now derive the classical formula for the rotation number of X H T S 2 on Th,j. 2 Using the map π T S 2 Th,j, 2 project the integral curve Γ : t ϕt (p) of X H T S 2 on Th,j 2 onto the curve γ : t γ(t) in the annular region A of S 2. Let x i A be coordinates on A with (x, x 2, x 3 ) being coordinates on R 3. Furthermore, let θ = tan x 2 and x 3 x (q), be coordinates on the universal covering space à of A. The following reasoning shows that a lift γ of γ to à satisfies the differential equations dθ dx 3 = j µx 3 (2) x 2 3 = ± V (x 3 ). (22) How the sign in (22) is chosen will be discussed below. By definition of Lie derivative, we find that dθ = L XH T S 2 θ 4
15 = x 2 + x 2 2 dx 2 (x x dx 2 ) = x y 2 x 2 y, using (7) x 2 + x 2 2 = j µx 3, using the definition of J T S 2 and the fact that x 2 3 Γ(t) (J T S 2 ) (j). Also, dx 3 = L XH T S 2 x 3 = π j (L XHj M j σ ) = πj (σ 2 ) using (5) = ±πj ( σ 3 ( σ) 2 (j µσ ) 2 ) since ψ is an integral of X Hj = ±πj ( 2(h γσ )( σ) 2 (j µσ ) 2 ), = η V (x 3 ), η 2 =. since Γ(t) (H T S 2 ) (h) The sign ambiguity in (22) is handled as follows. Suppose that γ(t ) = x ± 3 and at t ε > the value of η is known, then at time t + ε the value of η is the negative of η at t ε. Since Γ crosses C ± transversally at Γ(t ) and the mapping π T S 2 Th,j 2 has a fold singularity at Γ(t ), the curve γ has second order contact with C ± at γ(t ). The above sign convention ensures that the solutions of (2) and (22) in à are real analytic. Now consider the curve s ϕs (p) for s [, θ h,j ). Then the projected curve s π T S 2(ϕs (p)) is an arc of the small circle {x 3 = x + 3 } on S 2 which joins two successive points of intersection γ() and γ(t ) of γ [, T ] with {x 3 = x + 3 }. Let ϑ h,j be the angle between γ() and γ(t ) as measured from the center of the small circle {x 3 = x + 3 }. Then ϑ h,j is equal to the rotation number θ h,j, because ϑ h,j = = ϑh,j θh,j dθ L XJ T S 2 θ ds, by definition of rotation number 5
16 = θh,j ds, using (4) and the definition of θ = θ h,j. (23) Since V (x 3 ) > for x = (x, x 2, x 3 ) int A, from (22) we find that dx 3. Hence for t (, T/2) (T/2, T ) we may parametrize γ by x 3. Choose η = in (22) for t = ε. Then θ h,j = θh,j = = 2 Using (2) and (22) we get x 3 x + 3 x + 3 x 3 x + 3 θ h,j = 2 x 3 L XH T S 2 θ dθ x + 3 dx 3 + dx 3 x 3 dθ dx 3 dx 3. dθ dx 3 dx 3 j µx 3 ( x 2 3) V (x 3 ) dx 3, (24) which is the classical formula for the rotation number. To find a second formula for the rotation number we proceed as follows. Let C = {ϕs (p) s θ h,j } and C 2 = {ϕt (p) t T } be curves on Th,j 2 and let C be the curve C 2 C. Now θ T S 2 is the canonical -form on T S 2, θ being the canonical -form on T R 3. Then clearly we have C θ T S 2 = θ T S 2 C 2 θ T S 2. C (25) According to [6], calculating both sides of (25) will give a second formula for θ h,j. We shall do this, starting with evaluating the first term of the right hand side of (25). We find that C 2 θ T S 2 = = T T (θ T S 2 ) ( ϕ t (p) ) ( ( (θ T S 2 )(X H T S 2) )( ϕ dϕh T S2 t t (p) ) (p) ). 6
17 But (θ T S 2 )(X H T S 2)(x, y) = θ(x, y)(y, γe 3 + (γ x, e 3 y, y )x + +µx y) T S 2 ), using (7) = y, y T S 2, using the fact that θ(x, y)(u, v) = y, u = 2(H T S 2 )(x, y) 2(V S 2 )(x). where V(x) = γ x, e 3 is the potential energy of the unconstrained system (T R 3, Ω, H). Hence C 2 θ T S 2 = 2 T = 2hT 2γ = 2hT 2γ = 2hT 2γ (H T S 2 )(ϕt (p)) 2 T π j (σ M j ) ( ϕ t T (πt S (p) ) S2 2V)(ϕH T (p)) since t ϕt (p) lies in Th,j 2 EM (h, j) T since π j ϕ T σ (ϕ H j M j t (π j (p))) t (J T S 2 ) (j) = ϕ H j M j t π j σ (t) (26) where t (σ (t), σ 2 (t), σ 3 (t)) M j R 3 is the integral curve of the reduced vectorfield X Hj M j, which parameterizes the h-level set of the reduced Hamiltonian H j M j. Therefore we may write (26) as C 2 θ T S 2 = 2h = 4 = 4 = 4 T σ + σ σ + σ σ + σ 2γ T σ (t) h γσ dσ, parameterizing by σ instead of t σ h γσ σ 2 dσ, using (5) h γσ V (σ ) dσ, since ψ is an integral of (5) and σ(t) Hj (h). t (27) 7
18 We now compute C θ T S 2. As before we find that But C θ T S 2 = = θh,j θh,j ( θ T S 2 (ϕ s (p) ) ( ( (θ T S 2 )(X J T S 2) )( ϕ dϕj T S2 s (p) ) ds ds s (p) ) ds (θ T S 2 )(X J T S 2)(x, y) = (θ T S 2 )(x, y)( x e 3, y e 3 ), using (3) = y, x e 3 T S 2, since θ(x, y)(u, v) = y, u = (x y 2 y 2 x ) T S 2 = (σ 6 T S 2 )(x, y), which is invariant under the flow ϕ C θ T S 2 = θh,j s. Consequently, (σ 6 T S 2 )(p) = θ h,j ( σ6 T S 2 (p) ) = θ h,j (j µσ (p)), since J T S 2 = ( e 3, x y + µx 3 ) T S 2 and p C (J T S 2 ) (j) = θ h,j (j µσ + ) since σ = x 3 = x + 3 = σ + on C. (28) Finally we compute the left hand side of (25). Montgomery s idea [6] is to use Stokes theorem to evaluate C θ T S2. To carry this out we need to know that C bounds a suitable domain D. (This point seems to be incorrect in [6]). Certainly C is not null homologous on Th,j. 2 Therefore we must construct a suitable space D (J T S 2 ) (j) containing Th,j, 2 in which C is null homotopic and hence null homologous. To find D, we first fix a regular value j of J T S 2. Next observe that the image of C under the reduction map π j is the smooth closed curve (H j M j ) (h), which bounds a closed disc h = (H j M j ) (I h ) in M j. Here I h = [h min, h], where h min is the minimum value of H j M j. Since h is contractible, the S bundle πj ( h ) over h is trivial, that is, πj ( h ) is diffeomorphic to h S. Note that πj ( h ) = Th,j 2 and that πj ( h ) (J T S 2 ) (j). Finally put D = πj ( h ). To show that C is null homotopic in D, we note that D is a pinched closed -disc bundle over the annulus A S 2 with bundle projection π T S 2 D. The proof of this fact goes 8
19 as follows. Since D = {T 2 h,j h I h }, the space D T R 3 is defined by x 2 + x x 2 3 = x y + x 2 y 2 + x 3 y 3 = 2 (y2 + y2 2 + y3) 2 + γx 3 = h, h Ih x y 2 x 2 y + µ x 3 x = j, j µ. For each h I h, repeating the argument which lead to (2), we obtain where y 3 ± ( h) = ± V (x ± 3 ( h), h) Ṽ (x 3, h) = 2( h γx 3 )( x 2 3) (j µx 3 ) 2 and < x 3 ( h) x + 3 ( h) < are roots of Ṽ, that is, Ṽ (x± 3 ( h), h) =. From the definition of x ± 3 = σ ± ( h) as the abscissae of the intersection of the line h = σ σ with the graph of the function σ 3 = (j µσ ) 2, σ σ 2 <, (29) it follows from the strict convexity of (29) that the functions h σ + ( h) = x + 3 ( h) and h σ ( h) = x 3 ( h) are strictly monotonic decreasing and increasing, respectively, with x 3 (h min ) = x + 3 (h min ). Using the implicit function theorem we find that both of the functions h σ ± ( h) are smooth on (h min, h]. For h (h min, h], y 3 + ( h) > and y3 ( h) < ; while for h = h min, y3 (h min ) = = y 3 + (h min ). Thus for x A and h I h, we have (π T S 2 T 2 h,j ) (x) = {y 3 ± ( h)}, which implies that (π T S 2 D) (x) = [ min h I h y 3 ( h), max h I h y + 3 ( h) ] is a closed -disc containing. Hence D is a pinched closed -disc bundle over A. Viewing A as the zero section of the bundle D, we see that C is homotopic in D to the curve π T S 2(C) in A. Next we show that the curves γ 2 = π T S 2(C 2 ) and γ = π T S 2(C ) are homotopic in A leaving their end points fixed. Since γ and γ 2 both have the same beginning and end points, we can 9
20 lift them to curves γ and γ 2 in Ã, the universal covering space of A. In à the curves γ and γ have the same starting points. However, their end points can have θ coordinates differing by an integer multiple of 2π. From (2) it follows that dθ, because x 3 (, ) and j ±µ. Therefore γ 2 may be parameterized by θ instead of t. In fact, γ 2 is a function of θ where θ ranges in [, θ h,j ]. By the argument leading to (23) we see that γ is also a function of θ on [, θ h,j ]. Thus the end points of γ and γ 2 have the same θ coordinate and hence are the same point on Ã. Therefore γ and γ 2 are homotopic in A. Consequently, π T S 2(C) is null homotopic in A and thus in D, which is what we wanted to show. Let D be the domain in D bounded by C. Applying Stokes theorem, we find that C θ T S 2 = = = D (J T S 2 ) (j) D (J T S 2 ) (j) D (J T S 2 ) (j) dθ T S 2 ( Ω T S 2 µ π T S 2F ), using () πj Ω j + µ π D (J T S 2 ) T S 2F (j) using πj Ω j = Ω (J T S 2 ) (j) where Ω j is the symplectic form on M j and ( ) follows from the reduction theorem. = Ω j + µ F S 2. (3) π j (D) M j π T S 2 (D) Recall that for a regular value j ±µ, the reduced space M j R 3 is defined by ψ(σ) = σ 3 ( σ 2 ) (j µσ ) 2 = where σ 3 and σ <. A short calculation shows that the symplectic form Ω j on M j is given by ( ) Ω j (σ)(v, w) = ψ(σ), v w / ψ(σ) 2 (3) where v, w T σ M j = ker dψ(σ). Because µf is the magnetic field strength on S 2 of a monopole located at its center and π T S 2(D) is the region of S 2 bounded by π T S 2(C ) and π T S 2(C 2 ), we see that F h,j = F S 2. (32) π T S 2 (D) 2
21 is the magnetic flux through π T S 2(D) of the magnetic field of the monopole. Substituting (32) into (3) and then combining this result with (27) and (28), we see that (25) becomes where σ + (j µσ + h γσ )θ h,j = 4 σ V (σ ) dσ + A h,j µf h,j, (33) A h,j = Ω j. π j (D) M j We now compute the term A h,j. For j ±µ the reduced space M j is also defined by ϑ(σ) = σ 3 ( (j µσ ) 2 + σ 2 2 σ 2 ) = σ3 G(σ, σ 2 ), (34) since σ <. Suppose that σ M j, then ψ(σ) and ϑ(σ) are linearly dependent, because they are both normal to the surface M j R 3 at σ. From and we find that ψ(σ) = ( 2σ σ 3 + µ(j µσ ), 2σ 2, σ 2 ) Substituting (35) into (3) gives ϑ(σ) = ( G σ, G σ 2, ), ψ(σ) = ( σ 2 ) ϑ(σ). (35) Ω j (σ)(v, w) = ϑ(σ), v w /( σ 2 ) ϑ(σ) 2 (36) for v, w T σ M j = ker dϑ(σ). Pulling Ω j back by the mapping g : (, ) R R 3 : σ = (σ, σ 2 ) (σ, σ 2, G(σ, σ 2 )), which is a parametrization of M j, gives g Ω j ( σ)(, ) = σ σ 2 2
22 = Ω(g( σ)) ( = = G σ g( σ), G σ 2 g( σ) ) det ( ϑ(g( σ)), ( σ) ϑ(g( σ)) 2 2 σ 2 = dσ σ 2 dσ 2 (, ). σ σ 2 ϑ σ g( σ), ϑ σ 2 g( σ) ) Let D h,j be the projection of π j (D) along σ 3 -axis onto the σ -σ 2 plane. Then D h,j is the curve Therefore A h,j = = π j (D) D h,j σ + = 2 σ σ 2 2 = 2(h γσ )( σ 2 ) (j µσ ) 2 = V (σ ), for σ σ σ +. (37) Ω j = g Ω j, since g(d h,j ) = π j (D) D h,j σ 2 dσ σ 2 dσ 2 = dσ D h,j σ 2 by Stokes theorem V (σ ) σ 2 Substituting (38) into (33) gives σ + (j µσ + ) θ h,j = 2 σ dσ. (38) (j µσ ) 2 ( σ) V 2 (σ ) dσ µf h,j (39) which is the desired second formula for the rotation number θ h,j of the magnetic spherical pendulum. Substituting (25) into the right hand side of (39) gives the following quite surprising formula for the magnetic flux through π T S 2(D) σ + F h,j = 2 σ (σ + σ )(j µσ ) dσ. (4) ( σ) 2 V (σ ) 22
23 References [] Arms, J., Cushman, R., and Gotay, M., A Universal Reduction Procedure for Hamiltonian Group Actions, in: T. Ratiu (Ed.), Geometry of Hamiltonian Systems, Springer Verlag, New York, 99, pp [2] Arnol d, V., Mathematical Methods of Classical Mechanics, Springer Verlag, New York, 978. [3] Dirac, P.A.M., Lectures on Quantum Mechanics, Academic Press, New York, 964. [4] Cushman, R. and Knörrer, H., The momentum mapping of the Lagrange top, in: H. Doebner and J. Henning (Eds.), Differential Geometric Methods in Mathematical Physics, Lecture Notes in Mathematics, vol. 39, Springer Verlag, New York, 985, pp [5] Cushman, R. and van der Meer, J.-C., The Hamiltonian Hopf bifurcation in the Lagrange Top, in: Albert, C. (Ed.) Géométrie Symplectique et Mécanique, Lecture Notes in Mathematics, vol. 46, Springer Verlag, New York, 99, pp [6] Montgomery, R., How much does the rigid body rotate?, American Journal of Physics, 59 (99) R. Cushman L. Bates Mathematics Institute Department of Mathematics Rijksuniversiteit Utrecht University of Calgary Budapestlaan 6 25 University Drive, N.W. 358TA Utrecht Calgary, Alberta T2N N4 The Netherlands Canada 23
GEOMETRIC QUANTIZATION
GEOMETRIC QUANTIZATION 1. The basic idea The setting of the Hamiltonian version of classical (Newtonian) mechanics is the phase space (position and momentum), which is a symplectic manifold. The typical
More informationBACKGROUND IN SYMPLECTIC GEOMETRY
BACKGROUND IN SYMPLECTIC GEOMETRY NILAY KUMAR Today I want to introduce some of the symplectic structure underlying classical mechanics. The key idea is actually quite old and in its various formulations
More information[#1] R 3 bracket for the spherical pendulum
.. Holm Tuesday 11 January 2011 Solutions to MSc Enhanced Coursework for MA16 1 M3/4A16 MSc Enhanced Coursework arryl Holm Solutions Tuesday 11 January 2011 [#1] R 3 bracket for the spherical pendulum
More informationM3-4-5 A16 Notes for Geometric Mechanics: Oct Nov 2011
M3-4-5 A16 Notes for Geometric Mechanics: Oct Nov 2011 Text for the course: Professor Darryl D Holm 25 October 2011 Imperial College London d.holm@ic.ac.uk http://www.ma.ic.ac.uk/~dholm/ Geometric Mechanics
More informationMassachusetts Institute of Technology Department of Physics. Final Examination December 17, 2004
Massachusetts Institute of Technology Department of Physics Course: 8.09 Classical Mechanics Term: Fall 004 Final Examination December 17, 004 Instructions Do not start until you are told to do so. Solve
More informationLecture I: Constrained Hamiltonian systems
Lecture I: Constrained Hamiltonian systems (Courses in canonical gravity) Yaser Tavakoli December 15, 2014 1 Introduction In canonical formulation of general relativity, geometry of space-time is given
More informationarxiv: v1 [math.sg] 20 Jul 2015
arxiv:157.5674v1 [math.sg] 2 Jul 215 Bohr-Sommerfeld-Heisenberg Quantization of the Mathematical Pendulum. Richard Cushman and Jędrzej Śniatycki Department of Mathematics and Statistics University of Calgary,
More informationNoether Symmetries and Conserved Momenta of Dirac Equation in Presymplectic Dynamics
International Mathematical Forum, 2, 2007, no. 45, 2207-2220 Noether Symmetries and Conserved Momenta of Dirac Equation in Presymplectic Dynamics Renato Grassini Department of Mathematics and Applications
More informationHAMILTON S PRINCIPLE
HAMILTON S PRINCIPLE In our previous derivation of Lagrange s equations we started from the Newtonian vector equations of motion and via D Alembert s Principle changed coordinates to generalised coordinates
More informationPractice Qualifying Exam Questions, Differentiable Manifolds, Fall, 2009.
Practice Qualifying Exam Questions, Differentiable Manifolds, Fall, 2009. Solutions (1) Let Γ be a discrete group acting on a manifold M. (a) Define what it means for Γ to act freely. Solution: Γ acts
More informationLECTURE 5: SOME BASIC CONSTRUCTIONS IN SYMPLECTIC TOPOLOGY
LECTURE 5: SOME BASIC CONSTRUCTIONS IN SYMPLECTIC TOPOLOGY WEIMIN CHEN, UMASS, SPRING 07 1. Blowing up and symplectic cutting In complex geometry the blowing-up operation amounts to replace a point in
More informationChap. 1. Some Differential Geometric Tools
Chap. 1. Some Differential Geometric Tools 1. Manifold, Diffeomorphism 1.1. The Implicit Function Theorem ϕ : U R n R n p (0 p < n), of class C k (k 1) x 0 U such that ϕ(x 0 ) = 0 rank Dϕ(x) = n p x U
More informationarxiv: v1 [math.sg] 6 Nov 2015
A CHIANG-TYPE LAGRANGIAN IN CP ANA CANNAS DA SILVA Abstract. We analyse a simple Chiang-type lagrangian in CP which is topologically an RP but exhibits a distinguishing behaviour under reduction by one
More informationSolutions to the Hamilton-Jacobi equation as Lagrangian submanifolds
Solutions to the Hamilton-Jacobi equation as Lagrangian submanifolds Matias Dahl January 2004 1 Introduction In this essay we shall study the following problem: Suppose is a smooth -manifold, is a function,
More informationCurves in the configuration space Q or in the velocity phase space Ω satisfying the Euler-Lagrange (EL) equations,
Physics 6010, Fall 2010 Hamiltonian Formalism: Hamilton s equations. Conservation laws. Reduction. Poisson Brackets. Relevant Sections in Text: 8.1 8.3, 9.5 The Hamiltonian Formalism We now return to formal
More informationQualifying Examination HARVARD UNIVERSITY Department of Mathematics Tuesday, January 19, 2016 (Day 1)
Qualifying Examination HARVARD UNIVERSITY Department of Mathematics Tuesday, January 19, 2016 (Day 1) PROBLEM 1 (DG) Let S denote the surface in R 3 where the coordinates (x, y, z) obey x 2 + y 2 = 1 +
More informationEva Miranda. UPC-Barcelona and BGSMath. XXV International Fall Workshop on Geometry and Physics Madrid
b-symplectic manifolds: going to infinity and coming back Eva Miranda UPC-Barcelona and BGSMath XXV International Fall Workshop on Geometry and Physics Madrid Eva Miranda (UPC) b-symplectic manifolds Semptember,
More information1. Geometry of the unit tangent bundle
1 1. Geometry of the unit tangent bundle The main reference for this section is [8]. In the following, we consider (M, g) an n-dimensional smooth manifold endowed with a Riemannian metric g. 1.1. Notations
More informationHopf Fibrations. Consider a classical magnetization field in R 3 which is longitidinally stiff and transversally soft.
Helmut Eschrig Leibniz-Institut für Festkörper- und Werkstofforschung Dresden Leibniz-Institute for Solid State and Materials Research Dresden Hopf Fibrations Consider a classical magnetization field in
More informationTHE EULER CHARACTERISTIC OF A LIE GROUP
THE EULER CHARACTERISTIC OF A LIE GROUP JAY TAYLOR 1 Examples of Lie Groups The following is adapted from [2] We begin with the basic definition and some core examples Definition A Lie group is a smooth
More informationSYMPLECTIC GEOMETRY: LECTURE 5
SYMPLECTIC GEOMETRY: LECTURE 5 LIAT KESSLER Let (M, ω) be a connected compact symplectic manifold, T a torus, T M M a Hamiltonian action of T on M, and Φ: M t the assoaciated moment map. Theorem 0.1 (The
More information1 Hamiltonian formalism
1 Hamiltonian formalism 1.1 Hamilton s principle of stationary action A dynamical system with a finite number n degrees of freedom can be described by real functions of time q i (t) (i =1, 2,..., n) which,
More informationPhysical Dynamics (SPA5304) Lecture Plan 2018
Physical Dynamics (SPA5304) Lecture Plan 2018 The numbers on the left margin are approximate lecture numbers. Items in gray are not covered this year 1 Advanced Review of Newtonian Mechanics 1.1 One Particle
More informationPreface On August 15, 2012, I received the following email message from Ryan Budney (ryan.budney@gmail.com). Hi Dick, Here s an MO post that s right up your alley. :) http://mathoverflow.net/questions/104750/about-a-letter-by-richard-palais-of-1965
More information1 Differentiable manifolds and smooth maps. (Solutions)
1 Differentiable manifolds and smooth maps Solutions Last updated: February 16 2012 Problem 1 a The projection maps a point P x y S 1 to the point P u 0 R 2 the intersection of the line NP with the x-axis
More informationHamiltonian flows, cotangent lifts, and momentum maps
Hamiltonian flows, cotangent lifts, and momentum maps Jordan Bell jordan.bell@gmail.com Department of Mathematics, University of Toronto April 3, 2014 1 Symplectic manifolds Let (M, ω) and (N, η) be symplectic
More informationDifferential Geometry qualifying exam 562 January 2019 Show all your work for full credit
Differential Geometry qualifying exam 562 January 2019 Show all your work for full credit 1. (a) Show that the set M R 3 defined by the equation (1 z 2 )(x 2 + y 2 ) = 1 is a smooth submanifold of R 3.
More informationHamilton-Jacobi theory on Lie algebroids: Applications to nonholonomic mechanics. Manuel de León Institute of Mathematical Sciences CSIC, Spain
Hamilton-Jacobi theory on Lie algebroids: Applications to nonholonomic mechanics Manuel de León Institute of Mathematical Sciences CSIC, Spain joint work with J.C. Marrero (University of La Laguna) D.
More informationPatrick Iglesias-Zemmour
Mathematical Surveys and Monographs Volume 185 Diffeology Patrick Iglesias-Zemmour American Mathematical Society Contents Preface xvii Chapter 1. Diffeology and Diffeological Spaces 1 Linguistic Preliminaries
More informationFiber Bundles, The Hopf Map and Magnetic Monopoles
Fiber Bundles, The Hopf Map and Magnetic Monopoles Dominick Scaletta February 3, 2010 1 Preliminaries Definition 1 An n-dimension differentiable manifold is a topological space X with a differentiable
More informationQuantum Theory and Group Representations
Quantum Theory and Group Representations Peter Woit Columbia University LaGuardia Community College, November 1, 2017 Queensborough Community College, November 15, 2017 Peter Woit (Columbia University)
More informationTHE LAGRANGIAN AND HAMILTONIAN MECHANICAL SYSTEMS
THE LAGRANGIAN AND HAMILTONIAN MECHANICAL SYSTEMS ALEXANDER TOLISH Abstract. Newton s Laws of Motion, which equate forces with the timerates of change of momenta, are a convenient way to describe mechanical
More informationGlobal Formulations of Lagrangian and Hamiltonian Dynamics on Embedded Manifolds
1 Global Formulations of Lagrangian and Hamiltonian Dynamics on Embedded Manifolds By Taeyoung Lee, Melvin Leok, and N. Harris McClamroch Mechanical and Aerospace Engineering, George Washington University,
More informationPhysical Dynamics (PHY-304)
Physical Dynamics (PHY-304) Gabriele Travaglini March 31, 2012 1 Review of Newtonian Mechanics 1.1 One particle Lectures 1-2. Frame, velocity, acceleration, number of degrees of freedom, generalised coordinates.
More informationExamples of Singular Reduction
Examples of Singular Reduction Eugene Lerman Richard Montgomery Reyer Sjamaar January 1991 Introduction The construction of the reduced space for a symplectic manifold with symmetry, as formalized by Marsden
More informationSeminar Geometrical aspects of theoretical mechanics
Seminar Geometrical aspects of theoretical mechanics Topics 1. Manifolds 29.10.12 Gisela Baños-Ros 2. Vector fields 05.11.12 and 12.11.12 Alexander Holm and Matthias Sievers 3. Differential forms 19.11.12,
More informationTwisted Poisson manifolds and their almost symplectically complete isotropic realizations
Twisted Poisson manifolds and their almost symplectically complete isotropic realizations Chi-Kwong Fok National Center for Theoretical Sciences Math Division National Tsing Hua University (Joint work
More informationA Cantor set of tori with monodromy near a focus focus singularity
INSTITUTE OF PHYSICS PUBLISHING Nonlinearity 17 (2004) 1 10 NONLINEARITY PII: S0951-7715(04)65776-8 A Cantor set of tori with monodromy near a focus focus singularity Bob Rink Mathematics Institute, Utrecht
More informationSmooth Structure. lies on the boundary, then it is determined up to the identifications it 1 2
132 3. Smooth Structure lies on the boundary, then it is determined up to the identifications 1 2 + it 1 2 + it on the vertical boundary and z 1/z on the circular part. Notice that since z z + 1 and z
More informationAction-angle coordinates and geometric quantization. Eva Miranda. Barcelona (EPSEB,UPC) STS Integrable Systems
Action-angle coordinates and geometric quantization Eva Miranda Barcelona (EPSEB,UPC) STS Integrable Systems Eva Miranda (UPC) 6ecm July 3, 2012 1 / 30 Outline 1 Quantization: The general picture 2 Bohr-Sommerfeld
More informationSymmetric Spaces Toolkit
Symmetric Spaces Toolkit SFB/TR12 Langeoog, Nov. 1st 7th 2007 H. Sebert, S. Mandt Contents 1 Lie Groups and Lie Algebras 2 1.1 Matrix Lie Groups........................ 2 1.2 Lie Group Homomorphisms...................
More informationarxiv: v1 [math.gt] 20 Dec 2017
SYMPLECTIC FILLINGS, CONTACT SURGERIES, AND LAGRANGIAN DISKS arxiv:1712.07287v1 [math.gt] 20 Dec 2017 JAMES CONWAY, JOHN B. ETNYRE, AND BÜLENT TOSUN ABSTRACT. This paper completely answers the question
More informationThe two body problem involves a pair of particles with masses m 1 and m 2 described by a Lagrangian of the form:
Physics 3550, Fall 2011 Two Body, Central-Force Problem Relevant Sections in Text: 8.1 8.7 Two Body, Central-Force Problem Introduction. I have already mentioned the two body central force problem several
More informationThe Geometry of Euler s equation. Introduction
The Geometry of Euler s equation Introduction Part 1 Mechanical systems with constraints, symmetries flexible joint fixed length In principle can be dealt with by applying F=ma, but this can become complicated
More informationfor changing independent variables. Most simply for a function f(x) the Legendre transformation f(x) B(s) takes the form B(s) = xs f(x) with s = df
Physics 106a, Caltech 1 November, 2018 Lecture 10: Hamiltonian Mechanics I The Hamiltonian In the Hamiltonian formulation of dynamics each second order ODE given by the Euler- Lagrange equation in terms
More informationSymplectic and Poisson Manifolds
Symplectic and Poisson Manifolds Harry Smith In this survey we look at the basic definitions relating to symplectic manifolds and Poisson manifolds and consider different examples of these. We go on to
More information1 Differentiable manifolds and smooth maps. (Solutions)
1 Differentiable manifolds and smooth maps Solutions Last updated: March 17 2011 Problem 1 The state of the planar pendulum is entirely defined by the position of its moving end in the plane R 2 Since
More informationÜbungen zu RT2 SS (4) Show that (any) contraction of a (p, q) - tensor results in a (p 1, q 1) - tensor.
Übungen zu RT2 SS 2010 (1) Show that the tensor field g µν (x) = η µν is invariant under Poincaré transformations, i.e. x µ x µ = L µ νx ν + c µ, where L µ ν is a constant matrix subject to L µ ρl ν ση
More informationDierential geometry for Physicists
Dierential geometry for Physicists (What we discussed in the course of lectures) Marián Fecko Comenius University, Bratislava Syllabus of lectures delivered at University of Regensburg in June and July
More informationCritical points of the integral map of the charged 3-body problem
Critical points of the integral map of the charged 3-body problem arxiv:1807.04522v1 [math.ds] 12 Jul 2018 Abstract I. Hoveijn, H. Waalkens, M. Zaman Johann Bernoulli Institute for Mathematics and Computer
More informationTime-optimal control of a 3-level quantum system and its generalization to an n-level system
Proceedings of the 7 American Control Conference Marriott Marquis Hotel at Times Square New York City, USA, July 11-13, 7 Time-optimal control of a 3-level quantum system and its generalization to an n-level
More informationERRATA FOR INTRODUCTION TO SYMPLECTIC TOPOLOGY
ERRATA FOR INTRODUCTION TO SYPLECTIC TOPOLOGY DUSA CDUFF AND DIETAR A. SALAON Abstract. This note corrects some typos and some errors in Introduction to Symplectic Topology (2nd edition, OUP 1998). In
More informationEilenberg-Steenrod properties. (Hatcher, 2.1, 2.3, 3.1; Conlon, 2.6, 8.1, )
II.3 : Eilenberg-Steenrod properties (Hatcher, 2.1, 2.3, 3.1; Conlon, 2.6, 8.1, 8.3 8.5 Definition. Let U be an open subset of R n for some n. The de Rham cohomology groups (U are the cohomology groups
More informationTHEODORE VORONOV DIFFERENTIAL GEOMETRY. Spring 2009
[under construction] 8 Parallel transport 8.1 Equation of parallel transport Consider a vector bundle E B. We would like to compare vectors belonging to fibers over different points. Recall that this was
More informationB 1 = {B(x, r) x = (x 1, x 2 ) H, 0 < r < x 2 }. (a) Show that B = B 1 B 2 is a basis for a topology on X.
Math 6342/7350: Topology and Geometry Sample Preliminary Exam Questions 1. For each of the following topological spaces X i, determine whether X i and X i X i are homeomorphic. (a) X 1 = [0, 1] (b) X 2
More informationSmooth Dynamics 2. Problem Set Nr. 1. Instructor: Submitted by: Prof. Wilkinson Clark Butler. University of Chicago Winter 2013
Smooth Dynamics 2 Problem Set Nr. 1 University of Chicago Winter 2013 Instructor: Submitted by: Prof. Wilkinson Clark Butler Problem 1 Let M be a Riemannian manifold with metric, and Levi-Civita connection.
More informationSYMPLECTIC MANIFOLDS, GEOMETRIC QUANTIZATION, AND UNITARY REPRESENTATIONS OF LIE GROUPS. 1. Introduction
SYMPLECTIC MANIFOLDS, GEOMETRIC QUANTIZATION, AND UNITARY REPRESENTATIONS OF LIE GROUPS CRAIG JACKSON 1. Introduction Generally speaking, geometric quantization is a scheme for associating Hilbert spaces
More informationQualifying Exams I, 2014 Spring
Qualifying Exams I, 2014 Spring 1. (Algebra) Let k = F q be a finite field with q elements. Count the number of monic irreducible polynomials of degree 12 over k. 2. (Algebraic Geometry) (a) Show that
More informationROLLING OF A SYMMETRIC SPHERE ON A HORIZONTAL PLANE WITHOUT SLIDING OR SPINNING. Hernán Cendra 1. and MARÍA ETCHECHOURY
Vol. 57 (2006) REPORTS ON MATHEMATICAL PHYSICS No. 3 ROLLING OF A SYMMETRIC SPHERE ON A HORIZONTAL PLANE WITHOUT SLIDING OR SPINNING Hernán Cendra 1 Universidad Nacional del Sur, Av. Alem 1253, 8000 Bahía
More informationA loop of SU(2) gauge fields on S 4 stable under the Yang-Mills flow
A loop of SU(2) gauge fields on S 4 stable under the Yang-Mills flow Daniel Friedan Rutgers the State University of New Jersey Natural Science Institute, University of Iceland MIT November 3, 2009 1 /
More informationV = 1 2 (g ijχ i h j ) (2.4)
4 VASILY PESTUN 2. Lecture: Localization 2.. Euler class of vector bundle, Mathai-Quillen form and Poincare-Hopf theorem. We will present the Euler class of a vector bundle can be presented in the form
More informationA DANILOV-TYPE FORMULA FOR TORIC ORIGAMI MANIFOLDS VIA LOCALIZATION OF INDEX
A DANILOV-TYPE FORMULA FOR TORIC ORIGAMI MANIFOLDS VIA LOCALIZATION OF INDEX HAJIME FUJITA Abstract. We give a direct geometric proof of a Danilov-type formula for toric origami manifolds by using the
More informationPart II. Classical Dynamics. Year
Part II Year 28 27 26 25 24 23 22 21 20 2009 2008 2007 2006 2005 28 Paper 1, Section I 8B Derive Hamilton s equations from an action principle. 22 Consider a two-dimensional phase space with the Hamiltonian
More informationMath 225B: Differential Geometry, Final
Math 225B: Differential Geometry, Final Ian Coley March 5, 204 Problem Spring 20,. Show that if X is a smooth vector field on a (smooth) manifold of dimension n and if X p is nonzero for some point of
More informationDirac structures. Henrique Bursztyn, IMPA. Geometry, mechanics and dynamics: the legacy of J. Marsden Fields Institute, July 2012
Dirac structures Henrique Bursztyn, IMPA Geometry, mechanics and dynamics: the legacy of J. Marsden Fields Institute, July 2012 Outline: 1. Mechanics and constraints (Dirac s theory) 2. Degenerate symplectic
More information= 0. = q i., q i = E
Summary of the Above Newton s second law: d 2 r dt 2 = Φ( r) Complicated vector arithmetic & coordinate system dependence Lagrangian Formalism: L q i d dt ( L q i ) = 0 n second-order differential equations
More informationLecture 16 March 29, 2010
Lecture 16 March 29, 2010 We know Maxwell s equations the Lorentz force. Why more theory? Newton = = Hamiltonian = Quantum Mechanics Elegance! Beauty! Gauge Fields = Non-Abelian Gauge Theory = Stard Model
More informationMultiple Integrals and Vector Calculus (Oxford Physics) Synopsis and Problem Sets; Hilary 2015
Multiple Integrals and Vector Calculus (Oxford Physics) Ramin Golestanian Synopsis and Problem Sets; Hilary 215 The outline of the material, which will be covered in 14 lectures, is as follows: 1. Introduction
More informationDirac Structures and the Legendre Transformation for Implicit Lagrangian and Hamiltonian Systems
Dirac Structures and the Legendre Transformation for Implicit Lagrangian and Hamiltonian Systems Hiroaki Yoshimura Mechanical Engineering, Waseda University Tokyo, Japan Joint Work with Jerrold E. Marsden
More informationSOME EXERCISES IN CHARACTERISTIC CLASSES
SOME EXERCISES IN CHARACTERISTIC CLASSES 1. GAUSSIAN CURVATURE AND GAUSS-BONNET THEOREM Let S R 3 be a smooth surface with Riemannian metric g induced from R 3. Its Levi-Civita connection can be defined
More informationMorse Theory and Applications to Equivariant Topology
Morse Theory and Applications to Equivariant Topology Morse Theory: the classical approach Briefly, Morse theory is ubiquitous and indomitable (Bott). It embodies a far reaching idea: the geometry and
More informationA classical particle with spin realized
A classical particle wit spin realized by reduction of a nonlinear nonolonomic constraint R. Cusman D. Kemppainen y and J. Sniatycki y Abstract 1 In tis paper we describe te motion of a nonlinear nonolonomically
More informationSOLUTIONS TO THE GINZBURG LANDAU EQUATIONS FOR PLANAR TEXTURES IN SUPERFLUID 3 He
SOLUTIONS TO THE GINZBURG LANDAU EQUATIONS FOR PLANAR TEXTURES IN SUPERFLUID 3 He V. L. GOLO, M. I. MONASTYRSKY, AND S. P. NOVIKOV Abstract. The Ginzburg Landau equations for planar textures of superfluid
More informationMath 215B: Solutions 1
Math 15B: Solutions 1 Due Thursday, January 18, 018 (1) Let π : X X be a covering space. Let Φ be a smooth structure on X. Prove that there is a smooth structure Φ on X so that π : ( X, Φ) (X, Φ) is an
More informationMath 302 Outcome Statements Winter 2013
Math 302 Outcome Statements Winter 2013 1 Rectangular Space Coordinates; Vectors in the Three-Dimensional Space (a) Cartesian coordinates of a point (b) sphere (c) symmetry about a point, a line, and a
More informationGreen bundles : a dynamical study
Green bundles : a dynamical study Marie-Claude Arnaud December 2007 1 CONTENT 1) Hamiltonian and Lagrangian formalism 2) Lipschitz Lagrangian submanifolds, images of such manifolds and minimization properties
More informationsatisfying the following condition: If T : V V is any linear map, then µ(x 1,,X n )= det T µ(x 1,,X n ).
ensities Although differential forms are natural objects to integrate on manifolds, and are essential for use in Stoke s theorem, they have the disadvantage of requiring oriented manifolds in order for
More information9 Radon-Nikodym theorem and conditioning
Tel Aviv University, 2015 Functions of real variables 93 9 Radon-Nikodym theorem and conditioning 9a Borel-Kolmogorov paradox............. 93 9b Radon-Nikodym theorem.............. 94 9c Conditioning.....................
More informationarxiv:gr-qc/ v2 6 Apr 1999
1 Notations I am using the same notations as in [3] and [2]. 2 Temporal gauge - various approaches arxiv:gr-qc/9801081v2 6 Apr 1999 Obviously the temporal gauge q i = a i = const or in QED: A 0 = a R (1)
More informationOn local normal forms of completely integrable systems
On local normal forms of completely integrable systems ENCUENTRO DE Răzvan M. Tudoran West University of Timişoara, România Supported by CNCS-UEFISCDI project PN-II-RU-TE-2011-3-0103 GEOMETRÍA DIFERENCIAL,
More informationThe Canonical Sheaf. Stefano Filipazzi. September 14, 2015
The Canonical Sheaf Stefano Filipazzi September 14, 015 These notes are supposed to be a handout for the student seminar in algebraic geometry at the University of Utah. In this seminar, we will go over
More informationVariational principles and Hamiltonian Mechanics
A Primer on Geometric Mechanics Variational principles and Hamiltonian Mechanics Alex L. Castro, PUC Rio de Janeiro Henry O. Jacobs, CMS, Caltech Christian Lessig, CMS, Caltech Alex L. Castro (PUC-Rio)
More informationLagrangian knottedness and unknottedness in rational surfaces
agrangian knottedness and unknottedness in rational surfaces Outline: agrangian knottedness Symplectic geometry of complex projective varieties, D 5, agrangian spheres and Dehn twists agrangian unknottedness
More informationGeodesic flow on three dimensional ellipsoids with equal semi-axes
Geodesic flow on three dimensional ellipsoids with equal semi-axes Chris M. Davison, Holger R. Dullin Department of Mathematical Sciences, Loughborough University Leicestershire, LE11 3TU, United Kingdom.
More informationarxiv:math-ph/ v1 20 Sep 2004
Dirac and Yang monopoles revisited arxiv:math-ph/040905v 0 Sep 004 Guowu Meng Department of Mathematics, Hong Kong Univ. of Sci. and Tech. Clear Water Bay, Kowloon, Hong Kong Email: mameng@ust.hk March
More informationPart IB GEOMETRY (Lent 2016): Example Sheet 1
Part IB GEOMETRY (Lent 2016): Example Sheet 1 (a.g.kovalev@dpmms.cam.ac.uk) 1. Suppose that H is a hyperplane in Euclidean n-space R n defined by u x = c for some unit vector u and constant c. The reflection
More informationGroup Actions and Cohomology in the Calculus of Variations
Group Actions and Cohomology in the Calculus of Variations JUHA POHJANPELTO Oregon State and Aalto Universities Focused Research Workshop on Exterior Differential Systems and Lie Theory Fields Institute,
More informationJ-holomorphic curves in symplectic geometry
J-holomorphic curves in symplectic geometry Janko Latschev Pleinfeld, September 25 28, 2006 Since their introduction by Gromov [4] in the mid-1980 s J-holomorphic curves have been one of the most widely
More informationDIRAC COTANGENT BUNDLE REDUCTION HIROAKI YOSHIMURA JERROLD E. MARSDEN. (Communicated by Juan-Pablo Ortega)
JOURNAL OF GEOMETRIC MECHANICS doi:10.3934/jgm.2009.1.87 c American Institute of Mathematical Sciences Volume 1, Number 1, March 2009 pp. 87 158 DIRAC COTANGENT BUNDLE REDUCTION HIROAKI YOSHIMURA Applied
More informationA645/A445: Exercise #1. The Kepler Problem
A645/A445: Exercise #1 The Kepler Problem Due: 2017 Sep 26 1 Numerical solution to the one-degree-of-freedom implicit equation The one-dimensional implicit solution is: t = t o + x x o 2(E U(x)). (1) The
More informationUniversity of Utrecht
University of Utrecht Bachelor thesis The bifurcation diagram of the second nontrivial normal form of an axially symmetric perturbation of the isotropic harmonic oscillator Author: T. Welker Supervisor:
More informationSymmetry Preserving Numerical Methods via Moving Frames
Symmetry Preserving Numerical Methods via Moving Frames Peter J. Olver University of Minnesota http://www.math.umn.edu/ olver = Pilwon Kim, Martin Welk Cambridge, June, 2007 Symmetry Preserving Numerical
More informationGauge Fixing and Constrained Dynamics in Numerical Relativity
Gauge Fixing and Constrained Dynamics in Numerical Relativity Jon Allen The Dirac formalism for dealing with constraints in a canonical Hamiltonian formulation is reviewed. Gauge freedom is discussed and
More informationTHE GEOMETRY OF B-FIELDS. Nigel Hitchin (Oxford) Odense November 26th 2009
THE GEOMETRY OF B-FIELDS Nigel Hitchin (Oxford) Odense November 26th 2009 THE B-FIELD IN PHYSICS B = i,j B ij dx i dx j flux: db = H a closed three-form Born-Infeld action: det(g ij + B ij ) complexified
More informationAVERAGING AND RECONSTRUCTION IN HAMILTONIAN SYSTEMS
AVERAGING AND RECONSTRUCTION IN HAMILTONIAN SYSTEMS Kenneth R. Meyer 1 Jesús F. Palacián 2 Patricia Yanguas 2 1 Department of Mathematical Sciences University of Cincinnati, Cincinnati, Ohio (USA) 2 Departamento
More informationChapter 3. Riemannian Manifolds - I. The subject of this thesis is to extend the combinatorial curve reconstruction approach to curves
Chapter 3 Riemannian Manifolds - I The subject of this thesis is to extend the combinatorial curve reconstruction approach to curves embedded in Riemannian manifolds. A Riemannian manifold is an abstraction
More informationWeek 1. 1 The relativistic point particle. 1.1 Classical dynamics. Reading material from the books. Zwiebach, Chapter 5 and chapter 11
Week 1 1 The relativistic point particle Reading material from the books Zwiebach, Chapter 5 and chapter 11 Polchinski, Chapter 1 Becker, Becker, Schwartz, Chapter 2 1.1 Classical dynamics The first thing
More informationPhysics 221A Fall 1996 Notes 12 Orbital Angular Momentum and Spherical Harmonics
Physics 221A Fall 1996 Notes 12 Orbital Angular Momentum and Spherical Harmonics We now consider the spatial degrees of freedom of a particle moving in 3-dimensional space, which of course is an important
More informationMonodromy in the hydrogen atom in crossed fields
Physica D 142 (2000) 166 196 Monodromy in the hydrogen atom in crossed fields R.H. Cushman a,, D.A. Sadovskií b a Mathematics Institute, University of Utrecht, Budapestlaan 6, 3508 TA Utrecht, The Netherlands
More informationAn Invitation to Geometric Quantization
An Invitation to Geometric Quantization Alex Fok Department of Mathematics, Cornell University April 2012 What is quantization? Quantization is a process of associating a classical mechanical system to
More information