Order by Disorder in Spin-Orbit Coupled Bose-Einstein Condensates

Order by Disorder in Spin-Orbit Coupled Bose-Einstein Condensates

Ryan Barnett, Stephen Powell, Tobias Graß, Maciej Lewenstein,, and S. Das Sarma Joint Quantum Institute and Condensed Matter Theory Center, Department of Physics, University of Maryland, College Park, Maryland 20742-4111, USA ICFO-Institut de Ciències Fotòniques, Mediterranean Technology Park, 08860 Castelldefels (Barcelona), Spain ICREA-Institució Catalana de Recerca i Estudis Avançats, Lluis Companys 23, 08010 Barcelona, Spain
July 5, 2019
Abstract

Motivated by recent experiments, we investigate the system of isotropically-interacting bosons with Rashba spin-orbit coupling. At the non-interacting level, there is a macroscopic ground-state degeneracy due to the many ways bosons can occupy the Rashba spectrum. Interactions treated at the mean-field level restrict the possible ground-state configurations, but there remains an accidental degeneracy not corresponding to any symmetry of the Hamiltonian, indicating the importance of fluctuations. By finding analytical expressions for the collective excitations in the long-wavelength limit and through numerical solution of the full Bogoliubov- de Gennes equations, we show that the system condenses into a single momentum state of the Rashba spectrum via the mechanism of order by disorder. We show that in 3D the quantum depletion for this system is small, while the thermal depletion has an infrared logarithmic divergence, which is removed for finite-size systems. In 2D, on the other hand, thermal fluctuations destabilize the system.

I Introduction and Overview

Multicomponent condensates of ultracold atoms offer rich physical systems due to the interplay between superfluidity and internal degrees of freedom Lewenstein et al. (2007). Recently, through the use of synthetic gauge fields, two-component bosons with spin-orbit (SO) coupling have been engineered in the ultracold laboratory Lin et al. (2011). SO coupling in solid-state materials has a long history and is responsible for a variety of interesting physical effects, with notable examples including the spin Hall effect Kato et al. (2004) and topological insulators Hasan and Kane (2010). In addition, SO-coupled materials have diverse applications including spintronics Zutic et al. (2004). The newer bosonic counterpart of SO-coupled systems using ultracold atoms have no analog in solid-state systems and are thus expected to exhibit genuinely new physics. SO-coupled cold atomic systems have also received considerable recent theoretical attention Wu et al. (2011); Zhang et al. (2008); Stanescu et al. (2008); Ho and Zhang (2011); Larson et al. (2010); Merkl et al. (2010); Wang et al. (2010); Yip (2011); Ozawa and Baym (2011); Sau et al. (2011); Jiang et al. (2011); van der Bijl and Duine (2011); Zhang et al. (2012); Gopalakrishnan et al. (2011); Hu et al. (2012); Sinha et al. (2011), investigating topics such as spin-striped states Ho and Zhang (2011); Wang et al. (2010); Yip (2011), fragmentation Stanescu et al. (2008); Gopalakrishnan et al. (2011), and the realization of Majorana fermions Zhang et al. (2008); Sau et al. (2011); Jiang et al. (2011).

Recent experiments Lin et al. (2011) have realized a special combination of Rashba Bychkov and Rashba (1984) and Dresselhaus Dresselhaus (1955) SO coupling in ultracold atoms. There are also promising proposals to realize more general non-Abelian gauge fields like pure Rashba (c.f. Dalibard et al. (2011)), or even SU gauge fields that provide a toolbox for topological insulators Mazza et al. (2012). The conceptually simple system of a Rashba SO-coupled Bose-Einstein Condensate with isotropic interactions (RBEC) has surprisingly rich physics. The non-interacting system has a macroscopic ground state degeneracy as shown in Fig. 1. Interactions at the mean-field level partially remove this degeneracy, but there remains an ‘accidental’ degeneracy not corresponding to any underlying symmetry of the system. Specifically, mean-field theory predicts a superposition of condensates of opposite momenta with their relative amplitudes and phases unspecified.

In this work we show how fluctuations remove this accidental degeneracy and select a unique ground state (up to overall symmetries) through the mechanism of ‘order by disorder’ Villain et al. (1980). Although the phenomenon of order by disorder has been theoretically accepted and discussed within the context of classical spin models Villain et al. (1980); Moessner and Chalker (1998), quantum magnetism Henley (1989); Bergman et al. (2007) and ultracold atoms Turner et al. (2007); Song et al. (2007); Zhao and Liu (2008); Tóth et al. (2010), experimental demonstrations are, at best, scarce cha (). In contrast to the original proposal Villain et al. (1980), the degeneracy lifting we find is primarily quantum driven. We determine the fluctuation spectrum by numerically solving the coupled Bogoliubov-de Gennes equations. The resulting modes are integrated over to obtain the free energy as a function of the relative condensate weights and temperature. With this we show that fluctuations select a state with all bosons condensing into a single momentum state in the Rashba spectrum. We estimate the energy splitting per particle due to fluctuations for typical experimental parameters to be on the order of 100 pK. While this splitting is smaller than typical condensate temperatures, it is the total energy which determines the ground state, so this effect should be readily observable provided the RBEC model can be realized.

Figure 1: (Color online) The non-interacting (Rashba) energy spectrum of the Hamiltonian Eq. (1) with . The red circle indicates the degenerate lowest-energy single-particle states.

Ii Definition of Hamiltonian and Mean-Field Ground States

The Hamiltonian describing non-interacting bosons in 3D with SO coupling reads

(1)

where is a two-component bosonic field operator, is the momentum operator, is the magnitude of the SO coupling, and is a vector composed of Pauli matrices as (we set ). The SO coupling in Eq. (1) is equivalent to the Rashba form Bychkov and Rashba (1984) through a spin rotation. The single-particle eigenstates of Eq. (1) have spins pointing either parallel or antiparallel to their momenta in the plane, and up to a constant have energies , where . Clearly, there is a ring in momentum space of degenerate lowest-energy states with and (Fig. 1). Correspondingly, there is a macroscopic number of ways non-interacting bosons can occupy this manifold of states.

For the interacting portion of the Hamiltonian we take the simplest SU(2) invariant form

(2)

where , is the chemical potential, and where is an effective scattering length. At the mean-field level one replaces the operators by c-numbers . The states that minimize the kinetic energy, Eq. (1), are in general given by

(3)

where are arbitrary coefficients and . Minimizing the interaction energy restricts the mean-field states of Eq. (3) to have a constant density, . Placing this constraint on states in Eq. (3), one finds that can have at most two nonzero coefficients occurring at opposite momenta. This can be shown by setting each non-zero wavevector component of to zero. Without loss of generality, we take the momenta to point along the -axis and thereby obtain the state

(4)

where . We can take and to be real and parametrized as and since changing the phases of and amounts to position displacements and overall phase shifts of in Eq. (4). The selection of as a result of spin-symmetry breaking interactions (which is resolved at the mean-field level) was worked out in Wang et al. (2010). In contrast, in this work there remains a degeneracy at the mean-field level.

Iii Calculation of Collective Excitations

The degeneracy with respect to is accidental, i.e. it does not correspond to any symmetry of the Hamiltonian We thus expect quantum fluctuations about the mean-field state Eq. (4) to remove this degeneracy and to select a unique ground state through the order-by-disorder mechanism. To this end, we write and perform a Bogoliubov expansion of to quadratic order in . Up to a constant the interaction Hamiltonian becomes where It proves useful to transform to the variables where for which the interaction Hamiltonian takes the simple form

The full Bogoliubov Hamiltonian, , can be written compactly in matrix form if we introduce the four-component vector

(5)

Then up to a constant independent of we find that , where

(6)

In this expression, all -dependence is included in and is the Kronecker product. This Hamiltonian can be diagonalized using a symplectic transformation Blaizot and Ripka (1986); Powell et al. (2010), which amounts to solving the Bogoliubov-de Gennes equations,

(7)

for positive eigenvalues , where , and is a four-component function. Because of the translational symmetries of , the eigenvalues are labelled with band index and momentum in the Brillouin zone (BZ) defined as and . As usual, the eigenvectors are normalized as . In practice, Eq. (7) is simplest to solve in momentum space. Since the momentum space representation of is an infinite matrix, in numerical calculations it must be truncated at high momentum and the eigenvalues of interest must be checked to be independent of the cutoff.

Figure 2: (Color online) (a) The dispersions for the density and spin Goldstone modes for three values of for . (b) The average (arithmetic mean) of the density and spin modes. In both plots we have fixed .

In Fig. 2 we show the two gapless (Goldstone) modes for several values of , found numerically from Eq. (7). In experiments of Lin et al. (2011), , so we set these quantities to be equal. The dispersion is plotted along since, as can be seen from Eq. (7), the spectrum has no -dependence when . We refer to the dispersions as ‘density’ and ‘spin’ modes since they reduce to the known expressions and in the limiting case of , where is the free particle dispersion. One sees that upon increasing from zero to , the spin mode decreases in energy while the density mode increases. This gives, in a sense, a competing effect in terms of which configuration is selected from fluctuations. Noting this, in the right panel we plot the average of the spin and density modes for each value of . One sees that the average is always lowest in energy for . This indicates that the zero-point fluctuations from the Goldstone modes will select state though things become more subtle for . Such a state, as can be seen from Eq. (4), corresponds to all bosons condensing into a single momentum state of the RBEC system. The order-by-disorder mechanism will be considered more quantitatively below.

Analytical expressions for the dispersions and eigenvectors of Eq. (7) can be found perturbatively in the long-wavelength limit . In this limit one finds and for the density and spin modes respectively where and . These agree well with the numerical results shown in Fig. 2 for small except for two special cases which require more careful analysis. In particular, for , the density mode disperses quadratically along while for the spin mode disperses as along . Otherwise the density and spin mode have respectively linear and quadratic dispersions about their minima. It is interesting to compare these to the noninteracting energies shown in Fig. 1, which have quadratic and quartic dispersions about their minima.

Iv Quantum and Thermal Order by Disorder

Let us now consider the free energy due to quantum and thermal fluctuations described by . It is useful to separate out the contribution from zero-point fluctuations and write where

(8)
(9)

and is inverse temperature. Reminiscent of the zero-point photon contribution to the Casimir-Polder force Casimir (1948), the purely quantum contribution written as it is diverges. This divergence can be regularized by subtracting the free energy for a particular mean-field configuration which we take to have : . This regularized expression converges 111 After the -summation is performed, the summand has the asymptotic form proportional to for large as can be determined perturbatively, and no renormalization of the effective range of interactions is needed. The zero-point contribution to the free energy numerically computed as a function of is shown in Fig. 3(a) where the summation is performed over 26 bands (we emphasize that in order to obtain quantitatively correct results, including only the gapless modes is insufficient). One sees, indeed, that the state has the lowest energy and at such a state is unambiguously selected.

We now turn to the finite-temperature contribution to the free energy. Interestingly, one finds that the sign of the thermal contribution is negative and opposite to that of . Furthermore, the magnitude of the thermal contribution is always smaller than the contribution from zero-point fluctuations, in contrast to typical situations where thermal fluctuations enhance the degeneracy lifting and are larger in magnitude for modest temperatures (see, e.g. Turner et al. (2007)). Another instance of where quantum and thermal fluctuations select different states is in Ref. Tóth et al. (2010). The sign of at low can be understood by noting that the spin mode has the lowest energy for (Fig. 2).

Figure 3: (Color online) (a) The zero-point contribution to the free energy as a function of for three different values of . (b) The absolute value of the (negative) thermal free energy splitting between the and configurations as a function of temperature (solid line). This is seen to approach the quantum zero-point splitting at high temperatures (dashed line). In both panels the solid lines are fits to the numerically computed data points.

As seen in Fig. 3(b), the magnitude of approaches at high , so that in this limit. This behavior can be understood through a high expansion of the free energy

(10)

As the second term cancels the quantum contribution, we focus on the larger first term which can be written as

where are the eigenvalues of and we have used . The second summation above is over the reduced Brillouin zone which is restricted to positive values of . The eigenvalues are independent of the condensate configuration given by . This can be seen by noting that the -dependence of can be removed through the unitary transformation where 222The same transformation introduces -dependence into and so the eigenvalues of generally depend on , which determine the Bogliubov spectrum. . Thus to this order we find that . The next-order term in the high-temperature expansion has dependence which is evident in the numerical results shown in Fig. 3(b).

V Condensate Depletion

Having established using the Bogoliubov expansion that fluctuations select , we now investigate the self-consistency of this approach. This is determined by the depletion or the number of particles excited out of the condensate considered as a fraction of the total particle number . Consistency of course requires that this be finite, while neglecting of terms beyond quadratic order in is quantitatively reliable only if . The quantum and thermal contributions to are, respectively, and , where is the Bose-Einstein distribution function. The only possible divergences of these expressions are in the infrared, and so can be studied analytically using the small- expansion.

In 3D at , is finite and so can be sufficiently small provided weak-enough interactions. Our numerical results in fact demonstrate that the depletion is small even for moderately strong interactions, including in the region of experimental relevance. For , the thermal contribution is instead found to have a logarithmic divergence in 3D. This divergence (similar to that occurring in quasi-2D scalar condensates) is naturally removed for finite-sized systems and the condensate will thereby satisfy the stability criterion. For 2D condensates with isotropic SO coupling, the situation is different. Here, the quantum depletion again converges, but the thermal depletion diverges as for small . Thus, at our theory is unstable in 2D, which is consistent with work suggesting fragmentation Stanescu et al. (2008); Gopalakrishnan et al. (2011). Our conclusions on the stability of the condensate are, remarkably, identical to those based on the simple application of the Einstein criterion to the noninteracting spectrum. This is particularly surprising since the low- region is strongly modified by the interactions, giving quasiparticle modes that disperse with different powers than in the noninteracting case.

Vi Experimental Feasibility

We now comment on the experimental feasibility of observing order by disorder in RBEC. We first consider the magnitude of the degeneracy lifting. As a prototypical example we take spin one Rb. For a typical density of and , we find (for the appropriate scattering lengths) that at zero temperature the free energy splitting per particle due to fluctuations is . One should note that this number should not be directly compared with the condensate temperature since the total energy determines the ground state. It is this energy which will determine experimental timescales for the relaxation to the ground state. Spin-one atoms also possess a spin-dependent interaction term which we have neglected. For Rb, however, this spin-dependent interaction is relatively small (.5% that of the spin-independent) and as a result the degeneracy lifting from fluctuations is typically larger. Alternatively, one could use fermionic homonuclear molecules that have a singlet ground state. More importantly, schemes to create SO coupling in bosonic systems typically rely on utilizing dressed states Dalibard et al. (2011); Lin et al. (2011); Zhang et al. (2012) which can induce anisotropic interactions. The magnitude of such terms and their effect on the order-by-disorder mechanism will be left to future work when it becomes clear which of the several proposed schemes is most promising to realize Rashba coupling.

Another entity of experimental relevance is the harmonic confining potential. The results of the current manuscript will hold if the conditions for the local density approximation (LDA) are satisfied Dalfovo et al. (2011). For our system this requires that the energy splitting of the single-particle states as recently found in in Hu et al. (2012); Sinha et al. (2011) be small compared to the interaction energy. This energy splitting becomes small for weak trapping and/or strong SO coupling, resulting in a large quasi-degenerate manifold of single-particle states. Conversely, in the weakly interacting limit (where LDA is inapplicable) recent work Hu et al. (2012); Sinha et al. (2011) has shown the ground states of the RBEC system in a trap can form vortex lattices.

Vii Conclusion

In conclusion we have investigated the system of Rashba SO-coupled bosons with isotropic interactions (RBEC). In general bosons with SO coupling offer a genuinely new class of systems which has not been addressed in the vast solid state literature on spintronics Zutic et al. (2004). In particular, we have established that fluctuations select the RBEC system to condense into a single momentum state. We have argued that such a configuration is stable in 3D but destabilized when in 2D. We expect bosons with Rashba SO coupling to be realized in the near future for which the predicted configuration will be observable in Stern-Gerlach experiments. In future studies it will be interesting to investigate more general combinations of Rashba and Dresselhaus SO coupling. Such systems also possess accidental mean-field degeneracies and thus fluctuations are expected to play an important role in determining their ground states. In addition it will be interesting to investigate RBEC systems in two dimensions.

Acknowledgements.
We thank Ian Spielman and Anna Maria Rey for discussions and J. T. Chalker for drawing our attention to Ref. cha (). This work was supported by JQI-NSF-PFC, JQI-ARO-MURI, ERC Grant QUAGATUA, Spanish MINCIN grant TOQATA, and KITP under grant NSF PHY05-51164, where this work was initiated.

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