# Defect in the Joint Spectrum of Hydrogen due to Monodromy

###### Abstract

In addition to the well known case of spherical coordinates the hydrogen atom separates in three further coordinate systems. Separating in a particular coordinate system defines a system of three commuting operators. We show that the joint spectrum of the Hamilton operator, and the -components of the angular momentum and quantum Laplace-Runge-Lenz vectors obtained from separation in prolate spheroidal coordinates has quantum monodromy for energies sufficiently close to the ionization threshold. This means that one cannot globally assign quantum numbers to the joint spectrum. Whereas the principal quantum number and the magnetic quantum number correspond to the Bohr-Sommerfeld quantization of globally defined classical actions a third quantum number cannot be globally defined because the third action is globally multi valued.

What could possibly be said about the Hydrogen atom that is new? The hydrogen atom is conceivably the best studied system in quantum mechanics, alongside its classical counterpart the Kepler problem in classical mechanics. These systems are of paramount importance for our fundamental understanding of atomic physics and astronomy, respectively. Using their separability in spherical coordinates these systems are solved in any introductory physics course. Separable systems are special examples of integrable systems. A quantum integrable system (QIS) is a collection of independent commuting operators where say is the Hamilton operator. In addition we require that the classical limits of these operators have pairwise vanishing Poisson bracket, and thus constitute a Liouville integrable system with each a constant of motion (or integral for short). Geometrically this means that defines the energy momentum map, from the -dimensional classical phase space to and that the pre-image of a regular value of this map is a union of -dimensional tori (if compact) in the neighbourhood of which one can construct action angle variables following the Liouville-Arnold theorem Arnold (1978). The semiclassical Bohr-Sommerfeld quantization of actions shows that the joint spectrum where for with joint eigenstate , locally has the structure of a lattice and can hence be locally labelled by quantum numbers.

Due to defects this local lattice may not be extendable to a global lattice and hence a global assignment of quantum numbers to quantum states may be impossible Sadovskií and Zĥilinskií (1999); Vũ Ngọc (2000); Zĥilinskií (2006). This is the quantum mechanical manifestation of an obstruction to the global construction of action angle variables referred to as Hamiltonian monodromy and first introduced by Duistermaat Duistermaat (1980) and then studied quantum mechanically jointly with Cushman Cushman and Duistermaat (1988). Now many examples of (quantum) monodromy are known, see, e.g., Zĥilinskií (2011) and the references therein, and generalisations have been discovered Nekhoroshev et al. (2006); Sadovskií and Zĥilinskií (2007). Quantum monodromy explains, e.g., problems in assigning rovibrational spectra of molecules Cushman et al. (2004); Child (2008); Assémat et al. (2010) or electronic spectra of atoms in external fields Cushman and Sadovskií (1999); Efstathiou et al. (2007) and it provides a mechanism for excited-state quantum phase transitions Cejnar et al. (2006); Caprio et al. (2008). The generalization of monodromy to scattering systems leads to similar defects in the lattice of transparent states in planar central scattering Dullin and Waalkens (2008). It has been shown that monodromy can also play a role in spatiotemporal nonlinear wave systems Sugny et al. (2009). Dynamical manifestations of monodromy have recently been studied in Chen et al. (2014).

Both the Hydrogen atom and the Kepler problem have the property that they can be separated in four coordinate systems: spherical, parabolic, prolate spheroidal (which contains the first two as singular limiting cases) and sphero-conical coordinates, see, e.g., Cordani (2003). Each separating coordinate system gives a set of different separation constants which in turn define different sets of three commuting operators. In the case of spherical coordinates this gives the very well known QIS which has the joint spectrum with quantum numbers , and . Here is the -component of the angular momentum operator and, as in the rest of this paper, we use atomic units. In the case of separation in prolate spheroidal coordinates a different QIS is obtained as with where is the -component of the quantum Laplace-Runge-Lenz or eccentricity vector and the positive parameter is half the distance between the focus points of the prolate spheroidal coordinates, see, e.g., Morse and Feshbach (1953).

In this article we show that the spectrum of joint eigenvalues of has quantum monodromy in the limit of sufficiently large principal quantum number . The joint spectrum of for a large but fixed principal quantum number is shown in Fig. 1. Locally the spectrum has a lattice structure. Globally however it has a defect as can be seen from moving a fundamental lattice cell about the isolated singular value of the energy momentum map marked by the red dot in Fig. 1. As a consequence globally defined quantum numbers cannot exist. Even though separability of the hydrogen atom in prolate spheroidal coordinates has been known for a long time, this is the first time that quantum monodromy in the Hydrogen atom is described.

Super-integrable Systems. Before we discuss the details of the Hydrogen atom we want to elucidate the general structure underlying our analysis. Given a Hamiltonian operator it is exceptional to be able to find a QIS that contains – most Hamiltonians are non-integrable. It is even more exceptional to be able to find non-trivially distinct QIS and that both contain the same . This implies, but is not equivalent to, that the system is superintegrable, see, e.g., the review Evans (1990). Important examples are systems that are separable in different coordinate systems. Schwarzschild Schwarzschild (1916) was the first to point out that if the Hamilton-Jacobi equation of can be separated in more than one coordinate system, the quantum energy eigenvalues of are degenerate. Such a Hamiltonian operator is called multiseparable, and is hence included in non-equivalent QIS’s and . The simplest multiseparable systems are the free particle, the harmonic oscillator, and the Kepler problem. A multiseparable system is superintegrable, because if both and contain , then we have found more than operators that commute with . An important class of 3-dimensional superintegrable and multiseparable systems is classified in Kalnins et al. (2006).

The classical geometry of superintegrable systems is well understood. Fixing the integrals defines tori of lower dimension than in the Liouville-Arnold theorem and Nekhoroshev showed that one can construct lower dimensional action angle coordinates in a kind of generalization of the Liouville-Arnold theorem Nekhoroshev (1972). More global aspects have been studied in Miščenko and Fomenko (1978); Dazord et al. (1987). From the classical geometric point of view considering tori with half the dimension of phase space in a super-integrable system appears somewhat arbitrary. However, from the quantum point of view it is prudent to study all possible sets of commuting observables, because these tell us what can be measured simultaneously as the uncertainty principle is trivial in this case. Thus we are going to study a particular set of collections of Kepler ellipses that form 3-tori in phase space, and we will show that the joint quantum spectrum associated to these tori has quantum monodromy.

The Kepler problem and the hydrogen atom. To fix our notation let be the position of the electron in and its momentum. The nucleus is at the origin. The Hamiltonian is where , the angular momentum is , and the Laplace-Runge-Lenz vector is . The components of and all have vanishing Poisson brackets with , but are not all independent because of the relations and . Hence there are five independent integrals and the system is maximally superintegrable, i.e. fixing the five integrals on the six-dimensional phase space of the Kepler problem for negative energies defines one-dimensional tori. These one-dimensional tori simply are the periodic orbits given by the Kepler ellipses. Introducing where (assuming ) the components of and satisfy the commutator relations of the algebra with Casimirs and . In the quantum version similarly operators , and are defined and satisfy the same commutation relations of the algebra. We note that the symmetry was already used by Pauli in his 1926 paper Pauli (1926) to determine the spectrum of hydrogen.

Separation in Prolate Spheroidal Coordinates and Monodromy. Prolate spheroidal coordinates with focus points at on the -axis are defined by , where and and is the angle about the -axis. The surfaces of constant and are prolate ellipsoids and two-sheeted hyperboloids, respectively, with focus points . For , spherical coordinates are recovered, while for , parabolic coordinates are found. Assuming the hydrogen nucleus to be located at the focus point , the separation of the Schrödinger equation with the ansatz leads to three separated equations. The equation for gives the angular momentum eigenvalues , and the equations for and give the same equation

(1) |

where is the polynomial

(2) |

For , Eq. (1) is considered on the interval and for , Eq. (1) is considered on . The separation constant is the eigenvalue of the operator

(3) |

where is the -component of the quantum Laplace-Runge-Lenz vector which in position representation reads

(4) |

In (3) and (4) and are the standard momentum and angular momentum operators defined relative to the point . The operators , and mutually commute, i.e. defines a QIS.

The joint spectrum of can be computed numerically using a shooting method for the system of Fuchsian equations formed with and in (1). We follow however a more efficient algebraic approach that is briefly described in the methods section. A standard WKB ansatz shows that the joint spectrum can be computed semi-classically from a Bohr-Sommerfeld quantization of the actions according to , and with and non-negative quantum numbers and . Here the momenta and are given by where is again the polynomial in Eq. (2) which implies that the actions and are given by elliptic integrals. It turns out that and are not smooth functions of the eigenvalues – from a study of the elliptic integrals in the complex plane it can be shown that they have a discontinuous derivative at (this can be seen as a special case of the computation in Waalkens et al. (2004)). This is an indication that the lattice of eigenvalues formed by the joint spectrum might have a defect. Using the calculus of residues one finds that the sum of the actions is equal to and hence is in particular smooth for energies . In fact the quantization of the sum can be identified with the principal quantum number from which we then obtain . The magnetic quantum number and the principal quantum number are the only good quantum numbers – no third quantum number can be globally defined for the QIS . This is what we see in Fig. 1 which shows a layer of the lattice of the joint spectrum of constant principal quantum number . The defect is caused by a singular value of co-dimension two of the classical energy momentum map which is located on the axis at .

For at this singularity, the polynomial in Eq. (2) has a double root at . Because of this, the separated classical motions in the and degrees of freedom both have a turning point at . The corresponding orbits in configuration space are given by a two-parameter family of Kepler ellipses which have a common mutual intersection point at the focus point . In the left panel of Fig. 2 we show the one-parameter subfamily of these ellipses contained in the plane. The full two-parameter family is obtained from rotation about the -axis. In phase space the two-parameter family topologically forms a pinched 2-torus times a circle. In fact in order to prove monodromy it is sufficient to show that the corresponding classical system has a pinched torus Vũ Ngọc (2000) and this is what we do in the methods section. The two-parameter family of these Kepler ellipses contains the degenerate ellipse consisting of the line segment given by the interval on the -axis. This is a periodic collision orbit that runs along the symmetry axis and bounces back and forth between the nucleus at and the turning point on the -axis. For greater than which is the value of the potential energy at the focus point , the turning point of this periodic orbit on the -axis is below the focus point . This is the condition for the isolated value for the energy momentum map to come into existence as we will show in the methods section. This means that the layers of the joint spectrum for constant principal quantum number have a defect for and no defect for , which is illustrated in Fig. 3.

Conclusions

We have shown that the joint spectrum associated with the separation of the hydrogen atom in prolate spheroidal coordinates has a lattice defect due to quantum monodromy. The quantum integrable system obtained from this separation has two global quantum numbers and , but a third global quantum number does not exist due to the lattice defect. This raises the fascinating question whether an experiment can be designed which measures simultaneously the values of the the three observables of .

Spherical and parabolic coordinates can be considered to be limiting case of prolate ellipsoidal coordinates for and , respectively. In Fig. 3 the left and right images are close to these limiting situations. For , the condition cannot be satisfied, so there is no monodromy. For , the focus point collides with the boundary, and after extracting the square root of the diagram we recover the standard spectrum of again without monodromy. This leaves the sphero-conical coordinate system. Preliminary computations show that this QIS does not have monodromy. However, the spectrum does have an unexpected structure in that there is an additional separatrix.

A similar type of analysis can be done in other multiseparable systems. In particular we have already obtained preliminary results for the isotropic harmonic oscillator which again show that there is a QIS that contains this Hamiltonian for which the joint spectrum has monodromy. This will be presented in a forthcoming paper.

Methods

Proof of monodromy. As mentioned in the main text we can prove the presence of monodromy by studying the analytic properties of the elliptic integrals that give the actions associated with the separation in prolate spheroidal coordinates. It turns out that these integrals do not have a smooth dependence on the values of the constants of motion and no smooth single valued continuation of the actions is possible. The computations are very similar to the ones for Euler’s two-center problem in Waalkens et al. (2004).

Instead we here prove the presence of monodromy by showing the existence of a pinched torus using the method of singular reduction Cushman and Bates (1997). Following Vũ Ngọc (2000) the existence of a pinched torus implies quantum monodromy. In the present case we can follow an approach similar to the reduction of Stark-Zeeman perturbations of the Kepler problem that have been analysed in detail in Cushman and Sadovskií (1999); Efstathiou et al. (2007). The first step is then symplectic reduction of the periodic Hamiltonian flow of the Kepler problem which leads to a four-dimensional phase space given by the product of two spheres, , where the two spheres have constant energy and are given by and . On this reduced space we then have an integrable Hamiltonian system with integrals and . The essential difference to Cushman and Sadovskií (1999); Efstathiou et al. (2007) is that our integral does not originate from a perturbation in their class. Reduction of the axial rotational symmetry generated by leads to a singular one-degree-of-freedom system which can be described using a Poisson structure in with variables , and . The variables have Poisson brackets , , with the Casimir where is a parameter Cushman and Sadovskií (1999). Our reduced second integral is . The two-dimensional phase space defined by and is singular when with singular points at , see Fig. 4. For the reduced phase space is diffeomorphic to a sphere, for it is a point at the origin and empty otherwise. When the surface intersects the surface in the singular point the system has an equilibrium point. When the intersection is otherwise empty it is an elliptic equilibrium. When the intersection contains non-singular points then we have a pinched torus and hence monodromy. To see when the latter case occurs we compare the slope of the Casimir surface at the singular point which is with the slope of at that point, which is , so that a bifurcation occurs for , see Fig. 4.. For , there is no monodromy, while for there is. This is demonstrated in Fig. 3.

The proof that the presence of a pinched torus implies quantum monodromy requires semiclassical techniques Vũ Ngọc (2000). For illustration, we show how the semiclassical limit develops by increasing the principal quantum number in Fig. 5. From the Bohr-Sommerfeld quantization rule it follows that the locally smooth lines resulting from the spectrum in the semiclassical limit can be identified with the contours of the action functions. From Fig. 5 it can be inferred that smooth actions are necessarily multi-valued.

Computation of the spectrum. The computation of the joint spectrum of the QIS obtained from separating the Hamiltonian of the Hydrogen atom in prolate spheroidal coordinates is most efficiently done using interbasis expansion. This has been discussed by Coulson & Robinson Coulson and Robinson (1958). Using an adaption of the separation in spherical coordinates they show that the spectrum can be computed exactly from eigenvalues of matrices of size . The matrix is tri-diagonal and symmetric, the entries are and where . For fixed and , this produces one vertical line of the joint spectrum shown in the figures. As discussed in Coulson and Robinson (1958), it is very special to have spheroidal wave functions that can be written as a finite combination of spherical harmonics. For the related Euler’s two-centre problem, no such representation is possible Coulson and Joseph (1967).

## References

- Arnold (1978) V. I. Arnold, Mathematical Methods of Classical Mechanics, Graduate Texts in Mathematics, Vol. 60 (Springer, 1978).
- Sadovskií and Zĥilinskií (1999) D. A. Sadovskií and B. I. Zĥilinskií, Phys. Lett. A 256, 235 (1999).
- Vũ Ngọc (2000) S. Vũ Ngọc, Comm. Pure Appl. Math. 53, 143 (2000).
- Zĥilinskií (2006) B. Zĥilinskií, “Hamiltonian monodromy as lattice defect,” in Topology in Condensed Matter, edited by M. I. Monastyrsky (Springer Berlin Heidelberg, Berlin, Heidelberg, 2006) pp. 165–186.
- Duistermaat (1980) J. J. Duistermaat, Comm. Pure Appl. Math. 33, 687 (1980).
- Cushman and Duistermaat (1988) R. H. Cushman and J. J. Duistermaat, Bull. Amer. Math. Soc. 19, 475 (1988).
- Zĥilinskií (2011) B. Zĥilinskií, “Monodromy and complexity of quantum systems,” in The Complexity of Dynamical Systems: A Multi-disciplinary Perspective (John Wiley and Sons, Inc., 2011) pp. 159–181.
- Nekhoroshev et al. (2006) N. N. Nekhoroshev, D. A. Sadovskií, and B. I. Zĥilinskií, Annales Henri Poincaré 7, 1099 (2006).
- Sadovskií and Zĥilinskií (2007) D. Sadovskií and B. Zĥilinskií, Annals of Physics 322, 164 (2007), january Special Issue 2007.
- Cushman et al. (2004) R. H. Cushman, H. R. Dullin, A. Giacobbe, D. D. Holm, M. Joyeux, P. Lynch, D. A. Sadovskíi, and B. Zĥilinskiíi, Phys. Rev. Lett. 93, 024302 (2004).
- Child (2008) M. S. Child, “Quantum monodromy and molecular spectroscopy,” in Advances in Chemical Physics (John Wiley and Sons, Inc., 2008) pp. 39–94.
- Assémat et al. (2010) E. Assémat, K. Efstathiou, M. Joyeux, and D. Sugny, Phys. Rev. Lett. 104, 113002 (2010).
- Cushman and Sadovskií (1999) R. H. Cushman and D. A. Sadovskií, EPL (Europhysics Letters) 47, 1 (1999).
- Efstathiou et al. (2007) K. Efstathiou, D. Sadovskií, and B. Zĥilinskií, Proc. Roy. Soc. London Ser. A. 463, 1771 (2007).
- Cejnar et al. (2006) P. Cejnar, M. Macek, S. Heinze, J. Jolie, and J. Dobeš, Journal of Physics A: Mathematical and General 39, L515 (2006).
- Caprio et al. (2008) M. Caprio, P. Cejnar, and F. Iachello, Annals of Physics 323, 1106 (2008).
- Dullin and Waalkens (2008) H. R. Dullin and H. Waalkens, Phys. Rev. Lett. 101, 070405 (2008).
- Sugny et al. (2009) D. Sugny, A. Picozzi, S. Lagrange, and H. R. Jauslin, Phys. Rev. Lett. 103, 034102 (2009).
- Chen et al. (2014) C. Chen, M. Ivory, S. Aubin, and J. Delos, Physical Review E 89, 012919 (2014).
- Cordani (2003) B. Cordani, The Kepler Problem, Progress in Mathematical Physics, Vol. 29 (Springer, 2003).
- Morse and Feshbach (1953) P. Morse and H. Feshbach, Methods of Theoretical Physics (McGraw-Hill, New York, 1953).
- Evans (1990) N. Evans, Physical Review A 41, 5666 (1990).
- Schwarzschild (1916) K. Schwarzschild, Sitz. Ber. Kgl. Preuss. Akad. d. Wiss. Berlin 1916, 548 (1916).
- Kalnins et al. (2006) E. G. Kalnins, J. M. Kress, and W. Miller Jr, Journal of Mathematical Physics 47, 043514 (2006).
- Nekhoroshev (1972) N. N. Nekhoroshev, Tr. Mosk. Mat. Obs. 26, 181 (1972).
- Miščenko and Fomenko (1978) A. S. Miščenko and A. T. Fomenko, Functional Anal. Appl. 12, 113 (1978).
- Dazord et al. (1987) P. Dazord, T. Delzant, et al., J. Diff. Geom 26, 223 (1987).
- Pauli (1926) W. Pauli, Zeitschrift für Physik 36, 336 (1926).
- Waalkens et al. (2004) H. Waalkens, H. R. Dullin, and P. H. Richter, Physica D 196, 265 (2004).
- Cushman and Bates (1997) R. H. Cushman and L. M. Bates, Global Aspects of Classical Integrable Systems (Birkhäuser, Basel, Boston, Berlin, 1997).
- Coulson and Robinson (1958) C. A. Coulson and P. D. Robinson, Proceedings of the Physical Society 71, 815 (1958).
- Coulson and Joseph (1967) C. A. Coulson and A. Joseph, Proceedings of the Physical Society 90, 887 (1967).