ISRN Mathematical Physics

Volume 2013 (2013), Article ID 639424, 10 pages

http://dx.doi.org/10.1155/2013/639424

## Classical Analog of Extended Phase Space SUSY and Its Breaking

Byurakan Astrophysical Observatory, Aragatsotn District, 378433 Byurakan, Armenia

Received 21 April 2013; Accepted 12 May 2013

Academic Editors: Z. Qiao and P. Roy

Copyright © 2013 Gagik Ter-Kazarian. This is an open access article distributed under the Creative Commons Attribution License, which permits unrestricted use, distribution, and reproduction in any medium, provided the original work is properly cited.

#### Abstract

We derive the classical analog of the extended phase space quantum mechanics of the particle with odd degrees of freedom which gives rise to ()-realization of supersymmetry (SUSY) algebra. By means of an iterative procedure, we find the approximate ground state solutions to the extended Schrödinger-like equation and use these solutions further to calculate the parameters which measure the breaking of extended SUSY such as the ground state energy. Consequently, we calculate a more practical measure for the SUSY breaking which is the expectation value of an auxiliary field. We analyze nonperturbative mechanism for extended phase space SUSY breaking in the instanton picture and show that this has resulted from tunneling between the classical vacua of the theory. Particular attention is given to the algebraic properties of shape invariance and spectrum generating algebra.

#### 1. Introduction

An interesting question of keeping the symmetry between canonical coordinates and momenta in the process of quantization deserves an investigation. From its historical development, this aspect of statistical quantum mechanics, unfortunately, has attracted little attention. However, much use has been made of the technique of ordering of canonical coordinates () and momenta () in quantum mechanics [1, 2]. It was observed that the concept of an *extended* Lagrangian in phase space allows a subsequent extension of Hamilton’s principle to actions minimum along the actual trajectories in -, rather than in -space. This leads to the phase space formulation of quantum mechanics. Consequently this formalism was developed further in [3] by addressing the extended phase space stochastic quantization of Hamiltonian systems with first class holonomic constraints. This in a natural way results in the Faddeev-Popov conventional path-integral measure for gauge systems. Continuing along this line in the present paper we address the classical analog of the extended phase space ()-SUSY quantum mechanics [4] of the particles which have both bosonic and fermionic degrees of freedom, that is, the quantum field theory in -dimensions in -space, exhibiting supersymmetry (for conventional SUSY quantum mechanics see [5–12]). We analyze in detail the non-perturbative mechanism for supersymmetry breaking in the instanton picture ([13]). This paper has been organized as follows. In the first part (Sections 2 and 3), we derive the classical analog of the extended phase space SUSY quantum mechanics and obtain the integrals of motion. Consequently, we describe the extended phase space ()-SUSY algebra. In the second part (Sections 4 and 5), by means of an iterative scheme, first, we find the approximate ground state solutions to the extended Schrödinger-like equation and then calculate the parameters which measure the breaking of extended SUSY such as the ground state energy. We calculate a more practical measure for the SUSY breaking, in particular in field theories, which is the expectation value of an auxiliary field. We analyze nonsperturbative mechanism for extended phase space SUSY breaking in the instanton picture and show that this has resulted from tunneling between the classical vacua of the theory. Section 6 deals with the independent group theoretical methods with nonlinear extensions of Lie algebras from the perspective of extended phase space SUSY quantum mechanics and, further, shows how it can be useful for spectrum generating algebra. The concluding remarks are given in Section 7. Unless otherwise stated we take the geometrized units (). Also, an implicit summation on repeated indices is assumed throughout this paper.

#### 2. The Integrals of Motion

For the benefit of those not familiar with the framework of extended phase space quantization, enough details are given in the following to make the rest of the paper understandable. The interested reader is invited to consult the original papers [1, 2] for further details. In the framework of the proposed formalism, the extended Lagrangian can be written as
where a dynamical system with degrees of freedom described by the independent coordinates and momenta which are not, in general, canonical pairs. A Lagrangian is given in -representation and the corresponding in -representation. A dot will indicate differentiation with respect to . The independent nature of and gives the freedom of introducing a second set of canonical momenta for both and through the extended Lagrangian
One may now define an extended Hamiltonian
where is the conventional Hamiltonian of the system. In particular, vanishing of /or is the condition for and to constitute a canonical pair. In the language of statistical quantum mechanics this choice picks up a pure state (*actual path*). Otherwise, one is dealing with a mixed state (*virtual path*). One may, however, envisage that the full machinery of the conventional quantum mechanical dynamics is extendible to the extended dynamics as alluded to the above. Here and will be considered as independent -number operators on the integrable complex function . One of the key assumptions of extended phase space quantization [1, 2] is the differential operators and commutation brackets for and borrowed from the conventional quantum mechanics as follows:
Note also the following:
By the virtue of (4) and (5), is now an operator on . Along the trajectories in -space, however, it produces the state functions, , via the following Schrödinger-like equation:
Solutions of (6) are
where , positive definite, , and and are solutions of the conventional Schrödinger equation in - and -representations, respectively. They are mutually Fourier transforms. Note that the and are not, in general, eigenindices. The normalizable () is a physically acceptable solution. The exponential factor is a consequence of the total time derivative, , in (1) which can be eliminated. Actually, it is easily verified that
and so on. Substitution of (8) in (6) gives
provided by the reduced Hamiltonian, . From now on we replace by and by , respectively, and retain former notational conventions.

It is certainly desirable to derive the classical analog of the extended phase space quantum mechanics of the particle with odd degrees of freedom directly from what may be taken as the first principle. Therefore, following [10–12], let us consider a nonrelativistic particle of unit mass with two () odd (Grassmann) degrees of freedom. The classical extended Lagrangian equation (1) can be written provided by . Here , , and are arbitrary piecewise continuously differentiable functions given over the -dimensional Euclidean space . The are two odd (Grassmann) degrees of freedom. The nontrivial Poisson-Dirac brackets of the system (10) are The extended Hamiltonian (3) reads which, according to (8), reduces to The Hamiltonian equation (13) yields the following equations of motion: A prime will indicate differentiation with respect either to or . Thus, is the integral of motion additional to . Along the trajectories and in -spaces, the solution to equations of motion for odd variables is Hence the odd quantities are nonlocal in time integrals of motion. In trivial case , we have and . Suppose that the system has even complex conjugate quantities , whose evolution looks up to the term proportional to like the evolution of odd variables in (14). Then local odd integrals of motion could be constructed in the form Let us introduce the oscillator-like bosonic variables in - and -representations as follows: In the expressions (18), and are the piecewise continuously differentiable functions called SUSY potentials. In particular case if , for the evolution of we obtain Consequently, This shows that either or when and or and , respectively. Therefore, when the functions and , are related as where are constants, then odd quantities are integrals of motion in addition to and . According to (3) and (13), let us present in the form , where Then, and together with the and form the classical analog of the extended phase space SUSY algebra as follows: with constants playing a role of a central charges in -spaces; is classical analog of the grading operator. Putting , we arrive at the classical analog of the extended phase space SUSY quantum mechanics given by the extended Lagrangian We conclude that the classical system (10) is characterized by the presence of two additional local in time odd integrals of motion equation (17) being supersymmetry generators. Along the actual trajectories in -space, (24) reproduces the results obtained in [6].

#### 3. The Path Integral Formulation

In the matrix formulation of extended phase space ()-SUSY quantum mechanics, the will be two real fermionic creation and annihilation nilpotent operators describing the fermionic variables. The , having anticommuting -number eigenvalues, imply They can be represented by finite dimensional matrices , where are the usual raising and lowering operators for the eigenvalues of which is the diagonal Pauli matrix. The fermionic operator reads , which commutes with the and is diagonal in this representation with conserved eigenvalues . Due to it the wave functions become two-component objects as follows: where the states , correspond to fermionic quantum number , respectively, in - and -spaces. They belong to Hilbert space . Hence the Hamiltonian of extended phase space ()-SUSY quantum mechanical system becomes a matrix as follows: To infer the extended Hamiltonian equation (27) equivalently one may start from the -number extended Lagrangian of extended phase space quantum field theory in -dimensions in - and -spaces as follows: In dealing with abstract space of eigenstates of the conjugate operator which have anticommuting -number eigenvalues, suppose that is the normalized zero-eigenstate of and as follows: The state is defined by then . Taking into account that , we get Now we may introduce the notation for the anticommuting eigenvalues of . Consistency requires The eigenstates of , can be constructed as and thus Then, the and eigenstates are obtained by Fourier transformation as follows: which gives The following completeness relations hold: The time evolution of the state is now given as follows: The kernel reads which can be evaluated by the path integral. Actually, an alternative approach to describe the state space and dynamics of the extended phase space quantum system is by the path integral [3], which reads In the path integral equation (40) the individual states are characterized by the energy and the fermionic quantum number . With the Hamiltonian , the path integral equation (40) is diagonal as follows: Knowing the path integral equation (41), it is sufficient to specify the initial wave function to obtain all possible information about the system at any later time , by with (26). In terms of anticommuting -number operators and defining , the path integral equation (41) becomes The functional integral is taken over all trajectories from to and to between the times and .

#### 4. Solution of the Extended Schrödinger Equation with Small Energy Eigenvalue

Adopting the technique developed in [13], first, we use the iterative scheme to find the approximate ground state solutions to the extended Schrödinger-like equation with energy . We will then use these solutions to calculate the parameters which measure the breaking of extended SUSY such as the ground state energy. The approximation, which went into the derivation of solutions of (44), meets our interest that the ground state energy is supposedly small. As we mentioned above the solutions for nonzero come in pairs of the form related by supersymmetry, where . The state space of the system is defined by all the normalizable solutions of (44) and the individual states are characterized by the energies and the fermionic quantum number . One of these solutions is acceptable only if and become infinite at both and , respectively, with the same sign. If this condition is not satisfied, neither of the solutions is normalizable, nor they can represent the ground state of the system. Equation (44) yields the following relations between energy eigenstates with fermionic quantum number : where and and are the eigenvalues of and , respectively. The technique now is to devise an iterative approximation scheme to solve (46) and (47) by taking a trial wave function for , substitute this into the first equation (46), and integrate it to obtain an approximation for . This can be used as an ansatz in the second equation (47) to find an improved solution for and so forth. As it was shown in [13], the procedure converges for well-behaved potentials with a judicious choice of initial trial function. If the and are odd, then since they satisfy the same eigenvalue equation. It is straightforward then, for example, to obtain The independent nature of and gives the freedom of taking which yield an expression for energies as follows: Suppose that the potentials and have a maximum, at and , and minimum, at and , respectively. For the simplicity sake we choose the trial wave functions as After one iteration, we obtain where and are the normalization factors. The next approximation leads to It can be easily verified that to this level of precision (52) is self-consistent solution. Actually, for example, for the exponential will peak sharply around and may be approximated by a -function ; similarly may be replaced approximately by for . The same arguments hold for the -space. With these approximations equations (53) reduce to (52). The normalization constant is The energy expectation value gives the same result as that obtained for odd potentials by means of (50) and (53). Assuming the exponentials and to be small, which is correct to the same approximations underlying (55), the difference is negligible and the integrals in both cases may be replaced by Gaussians around and , respectively. Hence, it is straightforward to obtain which gives direct evidence for the SUSY breaking in the extended phase space quantum mechanical system. Here we have reinstated , to show the order of adopted approximation, and its non-perturbative nature. We also denoted However, a more practical measure for the SUSY breaking, in particular, in field theories is the expectation value of an auxiliary field, which can be replaced by its equation of motion right from the start as follows: Taking into account the relation , with commuting with , which means that the intermediate state must have the same energy as , (58) can be written in terms of a complete set of states as According to (55), we have where , , , , and . From SUSY algebra it follows immediately that

By virtue of (61), (60) reads Using the matrix representations of , and and the wave functions equation (53), one gets [13] where and . Hence Along the actual trajectories in -space, (65) reproduces the results obtained in [13].

#### 5. An Extended SUSY Breaking in the Instanton Picture

In this Section our goal is to show that the expressions equations (64) and (65) can be obtained in the path integral formulation of the theory by calculating the matrix elements, that is, the effect of tunneling between two classical vacua by using a one-instanton background. That is, the matrix elements of , and can be calculated in the background of the classical solution and . In doing this we rewrite the matrix element equation (62) in terms of eigenstates of the conjugate operator as follows:
in the limit . This reduces to
which, in turn, can be presented by path integrals defined in terms of anticommuting -number operators and with Euclidean actions of the instantons in - and -spaces, respectively. Following [13], these functional integrals include an integration over * instanton time * which is due to the problem of zero modes of the bilinear terms in Euclidean actions. This arises from time-transformation of instantons and SUSY transformations on them, respectively. The existence of zero modes gives rise to non-Gaussian behaviour of the functional integral. Due to it the matrix elements above do not receive any contributions from either no-instanton or anti-instanton configurations. The zero mode problem is solved by introducing a collective coordinate replacing the bosonic zero mode [14]. Whereas; the functional integrals depend only on the difference . Note also that multi-instanton configurations could contribute in principle, provided they have not more than one normalizable fermionic zero mode. But as it was shown in [13], their contribution is clearly smaller with respect to and . In the case when the SUSY potentials in - and -spaces have more than two extrema and , , one can put conditions on the SUSY potentials as follows
and similar to , that the extrema are well separated as follows: , . Around each of the classical minima and of the potentials and , respectively, one can approximate the theory by a supersymmetric harmonic oscillator. Then there are ground states which have zero energy. These states are described by upper or lower component of the wave function, depending on whether and are odd or even. With this provision the functional integrals are calculated in [13], which allow us consequently to write
and so forth. Inserting this in (67), we arrive at (64)
and, thus, of (65) as its inevitable corollary. This proves that the extended SUSY breaking has resulted from tunneling between the classical vacua of the theory. The corrections to this picture are due to higher-order terms and quantum-tunneling effects.

#### 6. Spectrum Generating Algebra

An extended Hamiltonian equation (27) can be treated as a set of two ordinary two-dimensional partner Hamiltonians [4] as follows:
provided by partner potentials
A subset of the SUSY potentials for which the Schrödinger-like equations are exactly solvable share an integrability conditions of * shape-invariance* [15] as follows:
where and are a set of parameters that specify phase-space-independent properties of the potentials, and the reminder is independent of .

##### 6.1. Algebraic Properties of Shape Invariance

Using the standard technique, we may construct a series of Hamiltonians , where ( is the number of iterations). From (72) and (73) we obtain then coupled nonlinear differential equations which are the two recurrence relations of Riccati-type differential equations as follows: where we denote , , , and . Here we admit that for unbroken SUSY, the eigenstates of the potentials , respectively, are that is, the ground states are at zero energies, characteristic of unbroken supersymmetry. The differential equations (75) can be investigated to find exactly solvable potentials. The shape invariance condition equation (73) can be expressed in terms of bosonic operators as where - is the coordinate in -space denotes concisely either - or -representations (no summation on is assumed). To classify algebras associated with the shape invariance, following [16], we introduce an auxiliary variables and define the following creation and annihilation operators: where are an arbitrary real constants and are an arbitrary real functions. Consequently, the creation and annihilation operators in -spaces can be written as The operators and are the generalization of (77), where and . One can easily prove the following relations: and that If we choose a function such that , then we have identified , and . Similar relations can be obtained for the -representations. From (77) we obtain then Introducing the operators and and combining (79) and (82), we may arrive at a deformed Lie algebras as follows: where and define the deformations. Different functions in (82) define different reparametrizations corresponding to several models. For example, (1)the translational models () correspond to . If is a linear function of , the algebra becomes SO(2.1) or SO(3). Similar in many respects prediction is made in somewhat different method by Balantekin [17];(2)the scaling models () correspond to and so forth.

##### 6.2. The Unitary Representations of the Deformed Lie Algebra

In order to find the energy spectrum of the partner SUSY Hamiltonians
one must construct the unitary representations of deformed Lie algebra defined by (83) [16, 18]. Using the standard technique, one defines up to additive constants the functions and as follows:
The Casimirs of this algebra can be written as and accordingly . In a basis in which and are diagonal, and are lowering and raising operators (the same holds for -representations). Operating on an arbitrary state , they yield
where
Similar arguments can be used for the operators , , and , which yield similar relations for the states . The profile of (and, thus, of ) determines the dimension of the unitary representation. Having the representation of the algebra associated with a characteristic model, consequently we obtain the complete spectrum of the system. For example, without ever referring to underlying differential equation, we may obtain analytic expressions for the entire energy spectrum of extended Hamiltonian with * self-similar* potential. A scaling change of parameters is given as , , at the simple choice , where is a constant. That is,
which yields
This is a deformation of the standard SO(2.1) Lie algebra, and therefore one gets
For scaling problems [16] one has , which leads to . The unitary representation of this algebra for monotonically decreasing profile of the function , is infinite dimensional. Let the lowest weight state of the be , and then . One can choose the coefficients to be real. From (87), for an arbitrary , , we obtain
The spectrum of the extended Hamiltonian reads
with the eigenenergies
Similar expressions can be obtained for the and eigenenergies and () as
and that
Hence

#### 7. Conclusions

We addressed the classical analog of the extended phase space quantum mechanics of particle which have both bosonic and fermionic degrees of freedom, that is, the particle with odd degrees of freedom which gives rise to ()-realization of the supersymmetry algebra. We obtain the integrals of motion. We use the iterative scheme to find the approximate ground state solutions to the extended Schrödinger-like equation and calculate the parameters which measure the breaking of extended SUSY such as the ground state energy. The approximation, which went into the derivation of solutions of (44), meets our interest that the ground state energy is supposedly small. This gives direct evidence for the SUSY breaking. However, we calculate a more practical measure for the SUSY breaking, in particular in field theories which is the expectation value of an auxiliary field. We analyze in detail the nonperturbative mechanism for extended phase space SUSY breaking in the instanton picture and show that this has resulted from tunneling between the classical vacua of the theory. Finally, we present an analysis on the independent group theoretical methods with nonlinear extensions of Lie algebras from the extended phase space SUSY quantum mechanics. Using the factorization procedure we explore the algebraic property of shape invariance and spectrum generating algebra. Most of these Hamiltonians possess this feature and hence are solvable by an independent group theoretical method. We construct the unitary representations of the deformed Lie algebra.

#### Acknowledgments

The author would like to thank Y. Sobouti for drawing his attention to the extended phase space formulation of quantum mechanics. The knowledgable comments from the anonymous referees are much appreciated.

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