Two component Bose-Hubbard model with higher angular momentum states

Two component Bose-Hubbard model with higher angular momentum states

Joanna Pietraszewicz, Tomasz Sowiński, Mirosław Brewczyk,
Jakub Zakrzewski, Maciej Lewenstein, and Mariusz Gajda
Institute of Physics Polish Academy of Sciences, Al. Lotników 32/46, 02-668 Warszawa, Poland
Wydział Fizyki, Uniwersytet w Białymstoku, ul. Lipowa 41, 15-424 Białystok, Poland
ICFO - Institut de Ciènces Fotòniques, Parc Mediterrani de la Tecnologia, E-08860 Castelldefels, Barcelona, Spain
ICREA - Institució Catalana de Recerca i Estudis Avançats, 08010 Barcelona, SpainInstytut Fizyki im. Mariana Smoluchowskiego, Uniwersytet Jagielloński, ul. Reymonta 4, 30-059 Kraków, Poland
July 12, 2019
Abstract

Bose-Hubbard Hamiltonian of cold two component Bose gas of spinor Chromium atoms is studied. Dipolar interactions of magnetic moments while tuned resonantly by ultralow magnetic field can lead to a transfer of atoms from the ground to excited Wannier states with a non vanishing angular orbital momentum. Hence we propose the way of creating of orbital superfluid. The spin introduces an additional degree of control and leads to a variety of different stable phases of the system. The Mott insulator of atoms in a superposition of the ground and vortex Wannier states as well as a superposition of the Mott insulator with orbital superfluid are predicted.

I Introduction

Ultracold atoms provide a playground for mimicking condensed matter and studying novel quantum many-body phenomena Bloch (); LewenR (). Recently, there has been particularly impressive progress in two areas of physics of ultracold atoms: the area of ultracold dipolar gases Baranov (); Lahaye (); Santos (); Sengstock () and the physics of orbital lattices LewenNP (). In this paper we combine these two areas and explore the effect of two-body dipolar interactions of magnetic atomic moments in a lattice potential. We study dipolar gases in their full complexity including spin as a dynamical variable (as opposed to be a conserved quantity), and magnetic dipolar interactions coupling different orbital states of involved magnetic components. That introduces additional physical processes into play and new degrees of control to the standard Bose-Hubbard model.

Spinor gases in a lattice have been studied in the context of Mott insulator (MI)- superfluid (SF) transition Kimura (). In general dipolar interactions lead directly to the dynamics of spin degree of freedom but up till now in lattice systems this phenomenon was neglected, i.e. it was assumed that spin is frozen Lahaye (). In such situations electric and magnetic dipoles are practically equivalent – they introduce long range correlations. On the other hand it is known from studies of gases confined in harmonic traps in the mean field limit Baranov (); Lahaye () that taking the dynamics of spin into account may modify properties of the ground state of the system.

Spin dynamics may result from contact or dipolar interactions. In the former case the total spin of interacting atoms remains unchanged (magnetization of the sample is constant). Qualitatively different phenomena take place when spin dynamics is triggered by the dipolar forces. The atomic magnetic moment originates from the spin which contributes to the total angular momentum of the system. When magnetic dipole changes due to the dipolar interactions, its variation must be accompanied by corresponding dynamics of the orbital angular momentum. Magnetic interactions can lead to a transfer of angular momentum from spin to orbital degrees of freedom. This phenomenon, discovered in ferromagnetic solid samples, is known as Einstein-de Haas effect Gawryluk (); Ueda (); Swistak1 (); Swistak_plakietki (). Not a long range character of magnetic dipolar interactions but rather their relation to the angular momentum plays a crucial role in this phenomenon. This makes a fundamental difference between magnetic and electric dipoles.

The main issue of our study is to account for the spin degree of freedom in the lattice environment. Spin flipping processes in the lattice could lead to an appearance of the orbital superfluid. Recently orbital superfluids were created in experiment Hammer (). The authors utilized a resonant tunneling in a particularly designed lattice potential.

In this paper we show another way of creating orbital superfluid by means of the resonant Einstein-de Haas effect. The atom which flips its spin has to gain some additional kinetic energy necessary to support its rotation. This energy is typically much larger than the energy of dipolar interactions and conservation of energy strongly suppresses the spin dynamics. The transfer of atoms between two spinor components can be enhanced by tuning energies of states involved via Zeeman effect Swistak1 (). We extend this idea to lattice gases. Dipolar effects significantly modify the MI-SF transition lead to new phases of the system with quantized vortices in MI or/and SF regimes.

The paper is oranized as follows: in Section II we introduce the two component Bose-Hubbard model with dipolar interactions coupling different Wannier states, in Section III we present a phase diagram for the system while in Section IV we discusse validity and limiatations of the model.

Ii The model

We assume that Cr atoms are in a 2D optical square lattice. To fix the parameters we consider a realistic situation of the lattice described by the periodic potential Here is the wavelength of light beams creating the lattice and is the barrier height. A characteristic energy of the problem, i.e. the recoil energy is . We express all energies and lengths in units of and respectively. Confinement along the direction is provided by a harmonic potential of frequency . At each lattice site we choose two wave functions centered at the given site to form a single particle basis of the two component system. The basis allows to account for the resonant transfer of atoms between , and and states in the presence of magnetic field aligned along the z-axis. The lowest energy state is effectively coupled to the excited state with one quantum of orbital angular momentum . The state is a single site analogue of a hamonic oscillator state . and are the ground and the first excited Wannier states in a 1D periodic potential of the form . Single particle energies of the two essential states are denoted by and respectively.

Limiting the subspace of essential states is a crucial approximation in our study. It is possible only due to a weakness of dipolar interactions. In fact there are several channels of binary dipolar collisions leading to different excited Wannier states. However, we can choose the desired channel by a proper adjustment of the resonant external magnetic field Swistak1 (). Typically the energy difference between atoms in the ground and in the excited Wannier states is much larger then dipolar energy which is the smallest energy scale in the problem (except vanishing tunnelings case), . However, at resonant magnetic field , , the two energies are equal and the spin transfer between the components becomes efficient on a typical time scale s. Here is the Bohr magneton and is the Lande factor. Only then the system can dynamically redistribute particles between the two components without violating energy conservation. A characteristic width of the resonances is small Brewczyk (), of the order of , i.e. G. We assume that no other states can be effectively coupled (see a more detailed discussion of the validity of this model in Section IV).

In effect a two-component system is realized with -component corresponding to atoms in and state while atoms in -component have , . Single site basis states are , where is a number of atoms in -component (). The Hamiltonian of the system is:

(1)

The parameters depend only on lattice height and confining frequency in the z-direction. are the contact interaction energies plus the part of dipolar energy which has the same form as corresponding contact term, is the on-site dipolar coupling of the two components, while and are tunneling energies. The Hamiltonian (1) is an interesting modification of the standard Bose-Hubbard model.

The on-site contact interactions , and cannot change a total spin Ueda_review (); bruno (). Dipolar two body interactions are much smaller than the contact ones; we keep only those dipolar terms which lead to a spin dynamics. Moreover, only on-site dipolar effects are accounted for in the Hamiltonian (1). Dipolar potential, although long range, is so weak that we can ignore dipole-dipole interactions between atoms at neighboring sites in the considered range of small tunnelings.

Unlike tunneling between ground Wannier states , the tunneling energy of the excited state is negative because the wave function the is antisymmetric in and . Therefore the state with ‘antifferomagnetic’ order of phases between neighboring sites has lower energy than the state where phases of the exited Wannier functions are the same. For the opposite on-site phases of the excited Wannier states both and are positive. This case is considered here.

Iii Phase diagram of the model

We limit our study to a small occupation of a lattice site: not more than one particle per single site on average. The resonant magnetic fields equilibrates single particle energies of states and , i.e. . and depend on the lattice height thus the resonant magnetic field varies with , .

Even with a single particle per site the dipolar interactions couple ground and excited Wannier states due to the tunneling in a higher order process. The transfer between and states is a sequence of: adding an atom to the -component at a given single site via tunneling, followed by the dipolar transfer of both -species atoms to the excited Wannier state , and finally the tunneling which removes one -component atom from the site . The two considered states are therefore coupled provided that tunneling is nonzero.

Now, following the standard mean field approach of Fisher et al.Fisher () we find thermodynamically stable phases of the system in the choosen subspace. The Hamiltonian (1) is translationally invariant, we assume the same property is enjoyed by the lowest energy state. Introducing superfluid order parameters for both components: and as well as the chemical potential , the Hamiltonian of the system can be approximated by a sum of single site Hamiltonians

(2)
(3)

Notice we skipped indices enumerating sites. In (3) is a number of neighbors and depends on the lattice geometry. For a 2D square lattice . Hamiltonian does not conserve number of particles: it describes a single site coupled to a particle reservoir. Order parameters and vanish in the MI phase and hopping of atoms is suppressed. Only in the SF regime number of particles per site can fluctuate. Close to the boundary, on the SF side, and can be treated as small parameters of the perturbation theory.

Figure 1: Phase diagram for 2D square lattice at the resoance, . The regions are: – Mott insulator with one particle in equal superposition od and states, – superfluid in and components (-dominated) and Mott insulator in the orthogonal supperposition, – superfluid phase of superposition of and components, – superfluid in the -component. In the inset the diagram for together with chemical potential for a given number of particles obtained from the exact diagonalization. The lines, from bottom to top correspond to occupation equal to as indicated. For (light grey region) the ground state of the system is a two particle state, therefore in this regime, the phases shown are thermodynamically unstable. They are stable, however, with respect to one particle hopping.

The single site ground state becomes unstable if the mean field or are different than zero. The mean fields can be obtained numerically from the self-consistency condition:

(4)

where . In the lowest order of the perturbation in the order parameters, the set of equations (4) becomes linear and homogeneous. Vanishing of its determinant is a necessary condition for nonzero solutions for . This condition determines lobs shown in Fig. 1.

In the low temperature limit () the partition function reduces to a single lowest energy state contribution . The energy depends on the chemical potential . Moreover, for the only contribution to Eq.(4) comes from eigenstates of the Hamiltonian with zero, one and two particles. Our analysis is limitted to this case only.

For negative chemical potential, , the single site ground state is vacuum state (dark grey region in Fig. 1). With increasing tunneling (and fixed ) particles appear in the superfluid vortex -phase (). Only at larger tunnelings some atoms do appear in the -component and both: ‘standard’ and orbital superfluids coexist ().

Situation becomes more complicated for larger chemical potential . At the resonance, , the ground state is degenerate if tunneling is neglected: the states and have the same energy, . The degeneracy is lifted via tunneling in the second order of the perturbation. In addition a position of the resonance is shifted towards smaller magnetic field values. Analysis of the effective Hamiltonian (compare Grass ()) indicates that in the resonant region the single site ground state is a supperposition of both components . Exactly at resonance . While crossing the resonance the ground state switches from to . The width of the resonance can be estimated perturbatively to be for while for lower barriers, , the resonant region is broader . Due to its small width the resonance can be hardly accesible particularly for small tunnelings. Away from the resonance the standard phase diagrams for or component emerge.

In Fig. 1 we show regions of stability of different possible phases of the system at resonance i.e when . For small tunnelings the system is in the Mott insulating phase (M) with one atom per site. Every atom is in the superposition of the ground and the vortex Wannier state. At the blue line, the border of (M) lobe, Eqs.(4) allow for nonzero solutions for and . Eqs.(4) become diagonal if is expressed in terms of bosonic operators and where and both coefitients of the superposition depend on the tunellings and . The operators create an atom in two orthogonal superpositions of and states. At the border of the Mott phase (M) the mean value of the operator is different from zero and a nonvanishing superfluid component, , appears in the (MS) region. Our numerical results show that and the ratio is small at the edge of stability of the Mott insulator. Therefore , i.e. the superfluid is dominated by the orbital -component. The mean field corresponding to the operator is zero in the discussed region. The system is therefore in equal superposition of the Mott insulating and superfluid phases. The Mott phase is dominated by the -component and the superfluid phase is overwhelmed with the -species. Both components, however, contain a small minority of remaining species.

At larger tunneling the system undergoes another phase transition as Eqs.(4) allow for another nonzero mean field. Now the mean value of departs form zero defining the border of the ‘bigger’ lob. Mott component of the ground Wannier state becomes unstable. The additional mean field appears in the (S) region. Again and the maximal value of is small. The -species dominate the superfluid component. Both and superfluids exist in the (S) region.

All the above findings are supported by direct inspection of the true many body ground state obtained by exact digonalization of the many body Hamiltonian in a small rectangular plaquette with periodic boundary conditions for total number of particles . Note that each site has three neighbors, , in this case. Resonance condition is reached by finding the magnetic field for which both and species are equaly populated. Calculations for require much larger number of sites and are numerically unreachable. In the inset of Fig. 1 we compare the exact results with the mean field ones but for . The lines in the inset correspond to the constant number of particles per site obtained from the relation . They allow to trace the phases the system enters while adiabatically changing the tunneling at fixed particle number. The (M) and (MS) phases can be reached with one particle per site only (8 particles in the plaquette). Direct inspection of a structure of the many body ground state fully confirms the stable phases of the system described above. In particular the ground state in the (MS) region can be approximated (with the accuracy of about 4%) by , where is the vaccum state.

In addition we calculated a hopping, i.e. the mean values of the following hopping operators : and . These operators annihilate a particle at a given site and put it in a neighboring site. They might be viewed as number conserving analogons of the mean fields and . In Fig. 2 we show the hopping for the case of one particle per site. For large tunnelings both and hopping are large – the components are in the superfluid phase. Entering the MS phase, , the hopping of -component rapidly falls down while hopping of -atoms remains big – the system enters -component dominated Mott insulator superimposed with -component dominated superfluid. At both hoppings tend to zero – the system enters the Mott phase with equal occupation of both species. This confirms results based on the Fisher method.

Figure 2: Hopping for the lowest energy state in a plaquette obtained from the exact diagonalization. Upper line – component, lower line – component.

Iv Validity of the model

Finally let us discuss possible limitations of the validity of the model discussed above. As we study a stability of the Mott phase we consider the case of deep optical lattices where tunneling is a small perturbation only. It is very natural to assume that dipolar interactions couple the ground Wannier state to the orbital state at each lattice site, and the system posseses the translational symmetry. Moreover, we have assumed that locally the potential at a given site has almost perfect axial symmetry with respect to the site center. Therefore, the local site Hamiltonian preservs projection of the total angular momentum, and the only state coupled to the ground Wannier one is of the type , where and are measured with respect to the site center. This state is the eigenstate of the projection of the orbital angular momentum on the -axis.

Three comments are in order.

iv.1 Role of anharmonicity.

Due to high selectivity of magnetic resonances we have a freedom of choosing a given channel of dipolar collision by a proper adjustment of the external magnetic field. In particular, we study the channel where the -comonent of the relative orbital angular momentum of interacting particles changes by two quanta, . Assuming that each of two colliding atoms are initially in the spherically symmetric ground state, the lowest energy final state of the two atoms has a form . Note that in the harmonic trap of radial frequency the state corresponds to a superposition of two states: and , where are particles coordinates. For one of colliding atoms aquires two quanta of rotation while the second atom remains in the spatial ground state, i.e. the energy of is . On the other hand represents the situation where each of two atoms gets one quantum of rotation resulting in the total energy . Evidently for equally spaced harmonic energy levels both states are degenerate, and both the conservation of angular momentum and the conservation of energy can be satisfied.

The situation becomes different in the optical lattice because of anharmonicity of the lattice potential. The state has energy of the second Wannier state, . This energy is smaller than twice the energy of the first excited Wannier of the state . Even for high barriers, i.e. the energy splitting is significantly larger then dipolar energy of Cr atoms, . Therefore, by means of magnetic field tuning one may select the resonant transfer of atoms due to dipolar interactions bringing both interacting particles to the state with one quantum of rotation while making the transfer to the second Wannier state nonresonant (and not efficient). This is a situation considered in the present paper. Note that a proper adjustment of the magnetic field may make the excitation of orbital resonant - the situation not considered here. Anharmonicity of the lattice potential, although small, plays thus an important role.

iv.2 Vorticity versus tunneling

The second issue is related to the tunneling of vortex-like states. As the lattice states have symmetry the angular momentum need not be conserved in the tunneling. With our choice of alternating phases of the excited Wannier states the tunneling coefficient in the excited band is positive, . Therefore tunneling of the right handed vortex to the vortex of the same vorticity at neighbouring site is equal to and is larger then tunneling with simulataneous change of the vorticity, i.e. to state, . The difference is small since tunneling in the lowest Wannier state but significant. The tunneling decreases the system energy thus the larger tunneling for the process preserving vorticity will decrease the system energy more and will be preferred. This observation allows for including only right handed vortex in our single particle basis and omitting the left handed one.

iv.3 Single site anisotropy

In our model we have assumed that the single site potential is isotropic, i.e. the two particle state produced in the dipolar interactions has both the well defined energy and the relative angular momentum. In fact this is not strictly true. The single site potential cannot be approximated by a harmonic one if fine details are to be studied. In a sqaure 2D lattice every site has four neighbours and the square symmetry of the lattice influences the single site potential. The quartic terms in the expansion of potential are relevant. For this reason the two particle state, corresponding to is not the eigenenergy state of single particle plus contact interaction on-site Hamiltonian. It is a superposition of three two-particles states of different energy instead. The fine structure results both from the anharmonicity and the anisotropy of the trapping potential. The anisotropy of the trap cannot be reduced even for very high lattices. We checked that even for the energy splitting is significantly larger then dipolar interaction energy. Large magnetic moments, leading to larger dipolar energy could help to overcome this problem. Conservation of energy allows to tune independently only to the one of the three components of the state. Weak dipolar interactions resolve this fine structure of two-particle energy states. To observe the Einstein de Haas effect in optical lattices one should use the lattice geometry for which the anisotropy due to the lattice symmetry is substantially reduced. To this end a 2D triangular lattice with every site having 6 neighbours might be promissing. The other way out is to rotate every lattice site around its axis similarly as in the experiment Gemelke ().

V Conclusions and outlook

In this paper we studied the model Bose-Hubbard system with two Wannier states in optical lattice. We show that weak dipolar interactions can be resonantly tuned to couple the ground Wannier state to the excited one with higher orbital angular momentum. We have studied a case of at most one particle per site on average. Even in this case, we predict various novel phases of the system. The phase diagram of the system significantly depends on the magnetic field. On the resonance we predict three distinct phases of the system: i) the Mott insulator of superposition of ground and vortex states ii) the -component dominated Mott superimposed with -component dominated superfluid, iii) two superfluids in particular combination of both species. We also discuss some limitations of our approach stressing that harmonic approximation has to be used with caution when studying orbital physics in optical lattices.

Higher densities (more particles per site) are more favorable for dipolar transfer, the related physics will be discussed elsewhere. It is worth noting that our results may be direcly related to the very recent experiments, in which spin relaxation in an ultracold dipolar gas in an optical lattice was observed in a presence of ultra low magnetic field bruno (); bruno2 (). Although, so far, no vortices have been found, we hope that the present work will help to identify the regime of parameters, in which generation of superfluid and appearance of novel quantum phases occurs.

Vi Acknowledgements

The authors acknowledge discussions with M. Załuska-Kotur and J. Mostowski. This paper was supported by the EU STREP NAMEQUAM, IP AQUTE, ERC Grant QUAGATUA, Spanish MINCIN (FIS2008-00784, QOIT), Alexander von Humboldt Stiftung, Polish Ministry of Science for 2009-2012 (J.Z.) and for 2009-2011 (M.G.) period.

References

  • (1) I. Bloch, J. Dalibard, W. Zwerger, Rev. Mod. Phys. 80 885 (2008).
  • (2) M. Lewenstein et al., Advances in Physics 56, 243 (2007).
  • (3) M. A. Baranov, Phys. Rep. 464, 71 (2008).
  • (4) T. Lahaye et al., Rep. Prog. Phys. 72, 126401 (2009).
  • (5) K. Rodrigues et al., Phys. Rev. Lett 105 050402 (2010).
  • (6) P.Soltan-Panahi et al. Nature Phys. 7, 434, (2011).
  • (7) M. Lewenstein, W. V. Liu, Nature Physics 7, 101 (2011).
  • (8) T. Kimura, S. Tsuchiya, S. Kurihara , Phys. Rev. Lett. 94, 110403 (2005).
  • (9) K. Gawryluk et al., Phys. Rev. Lett. 99, 130401 (2007).
  • (10) Y. Kawaguchi, H. Saito, and M. Ueda, Phys. Rev. Lett 96, 080405 (2006).
  • (11) T. Świsłocki et al., Phys. Rev. A 83, 063617 (2011).
  • (12) T. Świsłocki et al., Phys. Rev. A 84, 023625 (2011).
  • (13) G. Wirth, M. Ölschläger, A. Hemmerich, Nature Physics 7, 147 (2011)
  • (14) K. Gawryluk, K. Bongs, and M. Brewczyk, Phys. Rev. Lett. 106 140403 (2011).
  • (15) M. Ueda and Y. Kawaguchi, arXiv:1001.2072 (2010).
  • (16) B. Pasquiou et al., Phys. Rev. Lett. 106, 015301 (2011).
  • (17) M. P. A. Fisher et al., Phys. Rev. B 40, 546 (1989).
  • (18) T. Grass et al., arXiv:1108.2672
  • (19) N. Gemelke, E. Sarajlic, and S. Chu, arXive:1007.2677 (2010).
  • (20) B. Pasquiou et al., Phys. Rev. Lett. 106, 255303 (2011).
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