Chaos in monopole sector 9 of the Georgi - Glashow model. 9 9 1 n T. Dobrowolski and J. Szcze¸sny a J Institute of Physics and Informatics WSP, 2 Podchora¸z˙ych 2, 30-084 Cracow, Poland 1 1 v 8 Abstract 0 0 A spherically symmetric excitations of the Polyakov - ’t Hooft 1 monopole are considered. In the framework of the geodesics deviation 0 9 equation it is found that in the large mass Higgs sector a signature of 9 chaos occurs. / n y d - o a h c : v i X r a 1 1 Introduction Because of extreme complication of the evolution of nonlinear dynamical systems a great career make methods originated in Poincare section method [1]. There is also growing pressure on evaluating Lapunov exponents and Hausdorff dimension which are the most restrictive (global) characteristics of the behavior of the dynamical system [2]. Simultaneously there is also a tendency to improve and find new local criterions of chaos which are much simpler in application than the global one. Historically the first criterion was based on the fact that in the neighbourhood of the fixed points the dynam- ics is dominated by the linear terms [3]. This method in more formal way could be expressed as a condition (Toda criterion) on the Gauss curvature of the potential energy surface [4]. The criterion based on the geodesics de- viation equation in space equipped in Jacobi metric [5] seems to be the best geometrically motivated one. On the other hand in particle physics [6], cosmology [7] and condensed matterphysics[8]thereis(causedbygrowingnumberofapplications)tremen- dous interest indynamics of theYang - Mills fields. Onclassical level, studies of this subject concentrate mainly on seeking for new solutions and their ex- citations [9]. In this paper extending approach of the paper [10] we apply local geo- metric criterion of chaos to monopole sector of the Georgi - Glashow model. Using the local criterion of chaos we investigate the neighbourhood of the core of the Polyakov - ’t Hooft monopole. We show that in the large mass Higgs sector of the model, excitations of the monopole behaves in chaotic way. On the other hand for sufficiently light Higgs fields trajectories do not diverge. In the next section we will remind basic facts about Georgi - Glashow model and monopole solutions. Then we will use the criterion of sensitive dependence on initial conditions based on geodesic deviation equation. The suitable form of this criterion is prepared in appendix. As a result we shall discover difference of the dynamics of the light and heavy Higgs mass sectors. Last section contains some remarks. 2 2 Spherical excitations of the core of the Polyakov - Thooft monopole. The Georgi - Glashow model is SO(3) gauge invariant system consisting of a Higgs multiplet φa (a = 1,2,3) transforming as a vector in the adjoint representation of the gauge group and the gauge fields A = Aa Ta. µ µ In the same representation of the gauge group generators take the form (Ta) = ifa , where fabc = ǫabc. They also satisfy the relation [Ta,Tb] = bc − bc ifabcTc. The lagrangian of the model is given by 1 1 = Fa Faµν + D φaDµφa V(φ), (1) µν µ L −4 2 − where F = ∂ A ∂ A +ie[A ,A ] (2) µν µ ν ν µ µ ν − are the field strengths, D φa = ∂ φa eǫabcAb φc (3) µ µ µ − are covariant derivatives of the Higgs fields and 1 V(φ) = λ(φ2 v2)2 (4) 4 − is a Higgs potential. The Euler - Lagrange equations for lagrangian (1) (D Fµν)a = eǫabcφb(Dµφ)c, (5) ν − D Dµφa = λφa(φ2 v2). (6) µ − − The field strengths also satisfy the Bianchi identities. Equations of motion have finite energy and time independent solutions. Existence and stability of these solutions is a result of nontrivial structure of the Higgs vacuum = φa : φaφa = v2 which has topology of a two sphere. The asymptotic N { } Higgs fields φr→∞ which are mappings from spatial infinity to the vacuum manifold of the Higgs fields could be divided into infinite number of inequiv- alent homotopy classes Π ( ) = Z. The transition (by continuos deforma- 2 N tion) from one to another class needs infinite amount of the energy what makes these solutions stable. 3 A particular example of the monopole is given by Polyakov - ’t Hooft (P-T) ansatz φa = xaH(r) Φa, A a = ǫ xiK(r) W a, A a = 0, (7) k aki k 0 ≡ ≡ where H and K have the following asymptotic behaviour H r→0 H∗ = const, K −r→→0 K∗ = const and H r−→→∞ 1rv, K r−→→∞ −1er12. Monop−o→le of this form carries one unit of topological charge. From now we shall confine ourselves to n = 1 monopole sector of the Georgi - Glashow model. Following the approach of paper [10] we consider time deformations of the P-T ansatz φa = Φaf(t), A a = W ag(t), A a = 0, (8) k k 0 where f > 0 and g > 0 are unknown functions of time. Lagrangian density on this new ansatz takes the form 1 = ΦaΦaf˙2 +W aW ag˙2 V(f,g) (9) k k L 2 − (cid:16) (cid:17) where 1 1 1 V = λ(ΦaΦaf2 v2)2 + F aF ag2 eǫabcF aW bW cg3 sk sk sk s k 4 − 4 − 2 1 + e2[(W aW a)(W bW b) (W aW a)(W bW b)]g4 s s k k s k s k 4 − 1 + (∂ Φa)(∂ Φa)f2 eǫabc(∂ Φa)W bΦcgf2 k k k k 2 − 1 + e2[(W aW a)(ΦbΦb) (W aΦa)(W bΦb)]g2f2 (10) k k k k 2 − As the homogenous time dependent shift of the fields (7) in the whole space costs infinite amount of the energy it is unphysical. Therefore we confine our interest only to excitations of the core of the P-T monopole i.e. located in region surrounding zero of the Higgs fields. We implement locality of these excitations by taking zero (r 0) asymp- → totics of the shape functions H and K 1 = r2H∗2f˙2 +2r2K∗2g˙2 V(f,g), (11) L 2 − (cid:16) (cid:17) 4 where 1 3 V = 6K∗2g2 +2er2K∗3g3 + e2r4K∗4g4 + H∗2f2 + 2 2 1 +2er2H∗2K∗f2g +e2r4K∗2H∗2f2g2 + λ(r2H∗2f2 v2)2. (12) 4 − The effective lagrangian of the spherical excitations is in natural way defined by integration of the lagrangian density over a sphere of radius r which 0 contains the whole excitation L = d3x = 4π r0drr2 . Local (regular Sr0 L 0 L in time) excitations have been found for large amount of solitonic solutions R R [9]. We attempt to check possibility of existence not only regular but also chaotic solutions. After rescaling by the overall factor 4πr 5 the monopole 5 0 effective lagrangian q1 = f, q2 = g has the form 1 L = H∗2(q˙1)2 +2K∗2(q˙2)2 V(q1,q2), (13) 2 − h i 10 5 5 V = r 2K∗2(q2)2 +2eK∗3(q2)3 + 14e2r02K∗4(q2)4 + 2r 2H∗2(q1)2 + 0 0 5 +2eH∗2K∗(q1)2(q2)+ e2r02K∗2H∗2(q1)2(q2)2 + 7 1 5 5 +4λ 7r02H∗4(q1)4 −2v2H∗2(q1)2 + 3r 2v4 (14) (cid:18) 0 (cid:19) Now we shall use, based on the geodesic deviation equation, local criterion of chaos. Intwo dimensions system allows chaoticbehaviour ifthe Gausscurva- ture of the geometry determined by corresponding Jacobi metric is negative. If the Gauss curvature is positive and admissible for the physical trajectories region has no boundary then chaos does not occur. According to considera- tions of appendix (A8) the extrinsic curvature is 1 1 ∂2V 1 ∂2V 1 ∂V 2 1 ∂V 2 Kˆ = (E V) + + + 4(E V)3  − "H∗2∂(q1)2 2K∗2∂(q2)2# H∗2 ∂q1! 2K∗2 ∂q2!  −    (15)    In admissible for trajectories region of the configuration space (E V) > 0. − The second square bracket is also positive. Explicit differentiation of the po- tential(14)showsthat ∂2V > 0and ∂2V = 1M +P(q1,q2),whereM = ∂(q2)2 ∂(q1)2 −2 H H 5 2λv2 is a Higgs mass and P = r052H∗2+4eH∗2K∗(q2)+ 170e2r02K∗2H∗2(q2)2+ 175λr02H∗4(q1)2 > 0 is positive function. From equation (15) it follows that the sign of the Gauss curvature is controlled by the value of the Higgs mass. For small Higgs masses Kˆ is positive and excitations evolve in regular way. If mass of Higgs is sufficiently large then Kˆ became negative and chaos may occur. 3 Remarks Weconsidered spherically symmetric time-dependent deformationsoftheP- T monopole. This deformation could be obtained by the choice of the initial configuration which is deformed in the center and pure P-T monopole (7) at spatial infinity. In the heavy Higgs sector the local GDE criterion of chaos reveals chaotic behaviour of the fields. Because of the spherical symmetry we do not expect any radiation in this system which convince us that the excitation does not disappear. 4 Appendix Our purpose is to calculate the Gauss curvature Kˆ of the surface described by the Jacobi metric. Let us start from evaluating the components of the Riemann tensor. The most efficient way of evaluating the components of the curvature tensor has its origin in Cartan structural equations dΘa +ωa Θb = 0, (A.1) b ∧ Rˆa = dωa +ωa ωc , (A.2) b b c ∧ b whereΘa istheorthogonalco-base, i.e. suchthatgˆ= Θ1 Θ1+...+ΘN ΘN. ⊗ ⊗ The first equation ensures the torsionless of the connection and the second one is a definition of the curvature 2 - form. Let us confine to the two dimensional manifold equipped in metric gˆ = αdx dx+βdy dy, (A.3) ⊗ ⊗ 6 where α = α(q1,q2), β = β(q1,q2). In orthonormal co-base Θ1 = √αdq1, Θ2 = √βdq2 metric (A3) can be expressed in standard form gˆ = Θ1 Θ1 +Θ2 Θ2. (A.4) ⊗ ⊗ In two dimensions the definition of the curvature 2-form (A2) is even simpler Rˆa = dωa . (A.5) b b Evaluation of the curvature is extremely simple because the connection 1- form has the only one independent component (which follows from equation dgˆ = 0) ω1 = ω2 = ω = ω . The first Cartan structural equation 2 1 12 21 − − leads to 1 1 ∂α 1 ∂β ω1 = Θ1 Θ2 . (A.6) 2 2√αβ √α∂q2 − √β∂q1 ! On the other hand we use the fact that Rˆ1 component of the Riemann 2 curvature tensor can be expressed by Gauss curvature dω1 = Rˆ1 = KˆΘ1 Θ2. (A.7) 2 2 ∧ Now the Gauss curvature computation is a straightforward substitution of ω1 into equation (A7) 2 1 ∂2α ∂2β 1 ∂α ∂ ∂β ∂ Kˆ = + + (αβ)+ (αβ) . −2αβ ∂(q2)2 ∂(q1)2! 4α2β2 " ∂q2! ∂q2 ∂q1! ∂q1 # (A.8) 7 References [1] J.Guckenheimer, P.Holmes, ”Nonlinear Oscilations, Dynamical Systems and Bifurcations of Vector Fields,” Springer Verlag, 1983. L.E.Reichl, ”The Transition to Chaos,” Springer Verlag, 1992. [2] E.Ott, ”Chaos in Dynamical Systems,” Cambridge University Press, 1993. [3] L.Perko, ”DifferentialEquationsandDynamicalSystems,”SpringerVer- lag, 1992. [4] M.Toda, Phys. Lett. 48 A (1974) 5. [5] V.I.Arnold, ”Mathematical Methods of Classical Mechanics,” Springer Verlag, New York 1978. M.Szyd lowski, J.Szcze¸sny, Phys. Rev. D 50 (1994) 819. [6] I.Bars, A.Chodos, C.H.Tze, ”Symmetries in Particle Physics,” Plenum Press, New York and London 1984. [7] E.E.Donets, Preprint gr-qc 9807057 [8] S.C.Zhang, Science 275 (1997) 1098. E.Demler, S.C.Zhang, Preprint cond-mat 9805404. [9] H.Arod´z, Nucl.Phys. B 509 (1998) 273. H.Arod´z, L.Hadasz, Phys.Rev. D 55 (1997) 942. E.Braaten, S.Townsend, L.Carson, Phys.Lett. B 235 (1990) 147. T.Dobrowolski, Phys.Rev. D 50 (1994) 6503. C.Houghton, N.Manton, P.Sutcliffe, Nucl.Phys. B 510 (1998) 507. 8 [10] L.Salasnich, Preprint nucl-th 9707035. 9