Superfluid and supersolid phases of lattice bosons with ring-exchange interaction

Superfluid and supersolid phases of lattice bosons with ring-exchange interaction

Robert Schaffer Department of Physics and Astronomy, University of Waterloo, Ontario, N2L 3G1, Canada    Anton A. Burkov Department of Physics and Astronomy, University of Waterloo, Ontario, N2L 3G1, Canada    Roger G. Melko Department of Physics and Astronomy, University of Waterloo, Ontario, N2L 3G1, Canada
July 14, 2019
Abstract

We examine the superfluid phase of a hard-core boson model with nearest-neighbor exchange and four-particle ring-exchange at half-filling on the square lattice. At zero temperature we find that the superfluid in the pure- model is quickly destroyed by the inclusion of negative- ring-exchange interactions, favoring a state with a ordering wavevector. Minimization of the mean-field energy suggests that a supersolid state with coexisting superfluidity, charge-density wave, and valence-bond-like order is formed. We also study the behavior of the finite- Kosterlitz-Thouless phase transition in the superfluid phase, by forcing the Nelson-Kosterlitz universal jump condition on the finite- spin wave superfluid density. Away from the pure point, decreases rapidly for negative , while for positive , reaches a maximum at some in agreement with recent quantum Monte Carlo simulations.

I Introduction

The road to discovering new quantum phenomena such as exotic phases or unconventional quantum phase transitions is paved by the understanding of quantum Hamiltonians with competing microscopic interactions. Recent work has shown that competing kinetic energy terms, particularly four-particle “ring-exchange”, is a fertile venue for the study of valence-bond solids and unconventional quantum phase transitions.Paramekanti et al. (2002); Sandvik et al. (2002); Balents and Paramekanti (2003); Rousseau et al. (2005)

Long relegated to toy models of easy-plane spin systems or simple boson theories, the understanding of U(1) Hamiltonians has resurfaced as critical for the engineering of exotic quantum phases of ultracold atoms in optical lattices. Buchler et al.Büchler et al. (2005) presented the design of a ring-exchange interaction for bosonic cold atoms in two-dimensional (2D) square optical lattices. There, a conventional nearest-neighbor hopping term competes with a four-particle ring-exchange, which arises out of the hopping of boson pairs on the corners of square lattice plaquettes to an intermediate molecular state and back to the (opposite) plaquette corners. The Hamiltonian proposed in Ref. Büchler et al., 2005 can be written,

(1)

where the first term is the usual boson hopping, and the second is the ring-exchange interaction. Here, and are neighboring sites, lying opposite to sites and (respectively), which together form the basic square plaquette of the 2D lattice. This model has drawn significant attention recently from proposals that it may harbor an exotic quantum liquid phase that possesses d-wave correlations – a so-called d-wave Bose liquid (DBL) phaseMotrunich and Fisher (2007) – including extensive numerical investigation using exact diagonalization and the density matrix renormalization group.Sheng et al. (2008)

The main difficulty with the Hamiltonian Eq. (1) that prevents an exact solution in 2D for large systems (or the thermodynamic limit) is the presence of the prohibitive “sign-problem” in quantum Monte Carlo (QMC) simulations for the parameter regime . In fact, the same model in the parameter regime without the sign problem, , has been solved by QMC previously both at half-fillingSandvik et al. (2002) and in the presence of a symmetry-breaking chemical potential.Melko et al. (2004a) In this model, it was demonstratedSandvik et al. (2002) that the superfluid phase that dominates for large is destroyed by increasing the magnitude of the ring-exchange interaction, which realizes first a valence-bond solid (VBS) for , and a charge-density-wave (CDW) for . The intermediate superfluid to VBS quantum phase transition was studied intenselySandvik and Melko (2006) as one of the first candidates for a deconfined quantum critical point.Senthil et al. (2004) However, other interesting behavior occurs in the model, in particular in the experimentally relevant regime of finite-temperatures, where relatively little attention have been paid.Sandvik and Melko (2006)

In order to elucidate the mechanism by which the superfluid phase, which occurs for dominant in Eq. (1), is destroyed by the four-site interaction, we explore in this paper the behavior of the model using linear spin-wave (SW) theory. First, we calculate the dispersion and superfluid density at , where its behavior as a function of indicates the realization of a phase with symmetry for . Exploring the ordering nature of this phase in mean-field theory suggests a modulated in-plane order parameter, the mean-field indicator of a supersolid state, where superfluidity is expected to coexist with both CDW and also valence-bond-like order. In the superfluid phase, we also calculate the superfluid density at finite-temperature, and estimate the position of the Kosterlitz-Thouless (KT) transition using the universal jump condition. Interestingly, for the linear spin-wave theory reproduces the QMC resultSandvik and Melko (2006) that the maximum temperature of the KT transition does not occur when , rather it happens at some intermediate value of .

Ii Linear spin wave theory at

In order to study the destruction of the superfluid phase by the competing ring-exchange interaction parameterized by , we begin by examining the behavior of the system at in a linear spin-wave analysis. To begin, it is helpful to write our hard-core boson Hamiltonian as the analogous two-dimensional spin-1/2 XY model using the standard mapping: and . This transforms the Hamiltonian Eq. (1) into

(2)

which can be written with and operators as

As mentioned above, the groundstate of the pure- Hamiltonian is a bosonic superfluid, or an in-plane ferromagnet in the spin language, with an order parameter at zero temperature. We therefore perform our spin-wave expansion around this ordered state, treating the term of the Hamiltonian as a perturbation. As first demonstrated by Gomez-Santos and Joannopoulos,Gomez-Santos and Joannopoulos (1987) the proper Holstein-Primakoff representation in the case of the XY model is

(4)

giving us a leading order approximation to the Hamiltonian in terms of bosonic spin-wave operators and . Writing the Hamiltonian in Fourier space gives the linear spin-wave Hamiltonian

(5)

Here, the mean-field energy is

(6)

while the coefficients and

(7)
(8)

are defined in terms of

(9)
(10)
(11)
(12)

where

(13)

This form for the SW Hamiltonian reduces to that obtained by Bernardet et. al. Bernardet et al. (2002) in the limit of the simple XY model () and the absence of an external magnetic field. Following Ref. Bernardet et al., 2002, we diagonalize Eq. (5) using a Bogoliubov transformation,

(14)

where and are destruction and creation operators for quasiparticles of momentum . The bosonic commutation relations are satisfied if

(15)

where is determined by the requirement that it diagonalizes our Hamiltonian. This yields

(16)
(17)

and thus the diagonalized spin-wave HamiltonianBernardet et al. (2002)

It is the diagonal SW Hamiltonian, in this generalized form, that we now proceed to use to analyze the behavior of our superfluid phase at zero temperature.

ii.1 Dispersion

We begin by studying the dispersion, which is obtained immediately from Eq. (II)

(19)

This can be examined as a function of for the Hamiltonian Eq. (2). For and , one reproduces the expected linear dispersion,Bernardet et al. (2002) a feature which survives for moderate (at least to first-order in the SW theory) – see Fig. 1. No soft modes develop in the dispersion until very large values of , which is well above the critical value of where a phase transition to a VBS is known from QMC.Sandvik et al. (2002) In contrast is the behavior of the dispersion in the regime, which is intractable to QMC methods due to the negative sign problem. In this case, the dispersion reveals the development of soft modes at . The value of tends towards 0 as approaches , as illustrated in Fig. 1. This indicates that an ordered phase with symmetry is realized for sufficiently large . The nature of this ordering is discussed in Section III.

Figure 1: (Color online) The dispersion , as a function of , for (top) and (bottom).

ii.2 The zero-temperature superfluid density

The most important quantity characterizing the superfluid phase is the superfluid density (or spin stiffness), defined as the second derivative of the free energy with respect to a uniform twist of the in-plane spin components across the system. At zero-temperature, one replaces the free energy by the groundstate energy, hence we use the definition

(20)

which is valid for . This is equivalent to finding the incremental energy per spin resulting from the twist,

(21)

Thus, we are faced with the task of finding . To do this, we consider the spins in a site-dependent rotated reference frame, defined via the standard rotation operator about the axis.Sandvik (1997) The relevant transformations become

(22)

which can also be written in terms of the spin raising and lowering operators,

(23)

We assume a uniform twist across the spins in the system, so that the twist , where and are nearest neighbors in the or direction. We find that, using the labeling of Eq. (1), , and thus the dependence of the ring-exchange term cancels. This gives for our twisted Hamiltonian

(24)

The linear components of the term proportional to cancel, so in linear spin wave theory the twist effectively scales the nearest neighbor exchange value . Thus, is obtained directly from the Hamiltonian Eq. (5), with the redefinition of

(25)
(26)
(27)

but with the coefficients , , , and unchanged from Eqs. (9-12). Expanding as , and noting that at zero temperature, the thermal expectation value is

(28)

we find that

Note that we have divided by a factor of two to account for the fact that Eq. (II) is defined with respect to a twist in a single lattice bond, while Eq. (22) considers a twist in each bond in the lattice, a total of 2N bonds.

Figure 2: (Color online) The superfluid density as a function of . The dashed line is the mean-field result, . The linear SW result for is , which can be compared to the best known exact results = 0.2696(2).Sandvik and Hamer (1999)

The superfluid density calculated in this linear SW theory, Eq. (II.2), is plotted in Fig. 2 for a range of . Note that, as in the above section, we have set to correspond to the usual definition of the XY spin model (when ). The superfluid density curve has its maximum at , with a value of , which can be compared to the best numerical estimate for the groundstate spin stiffness in the XY model using finite-size scaling quantum Monte Carlo techniques, = 0.2696(2).Sandvik and Hamer (1999) Away from this maximum at , the superfluid density declines monotonically with increasing . On the positive side, decreases relatively gradually, only becoming zero for an extremely large value of . This is consistent with the above results for the dispersion, which indicate that no soft modes develop for moderate values of positive . Again, exact QMC results have revealed a quantum phase transition to a valence-bond solid phase at ,Sandvik et al. (2002) reiterating the limitations of the linear SW theory calculation in this regime.

On the negative- side, where no QMC results are available, the value of drops rapidly as it approaches -2. In SW theory, there is a divergent negative contribution to at this value of . This is of course an artifact of linear SW theory. As explained in the next section, one actually expects to remain finite on the other side of the transition, where an ordered phase with symmetry is realized.

Figure 3: (Color online) The supersolid phase as dictated by mean-field theory, for . Solid (blue) arrows show the angles of deviation of the classical spin vectors from the direction (the out-of plane deviation is zero). Dashed (green) arrows are the corresponding bosonic charge currents , Eq (38).

Iii Supersolid phase for

Examining our linear SW theory results of the previous section, for we expect the development of a phase with as the ordering wavevector. We can further elucidate the nature of the ordering in this phase by minimizing the mean-field energy of the ring-exchange Hamiltonian, Eq. (1), under the constraint of order with symmetry. By representing the quantum spins as classical spin vectors,

(30)
(31)
(32)

we rewrite Eq. (II), which simplifies to the following Hamiltonian:

Note that the angle of the classical vector from the axis, , should not be confused with the phase twist variable defined in the previous section. Restricting ourselves to half-filling, we look for solutions to the angles and in the form

(34)
(35)

(where ) by minimizing the classical energy Eq (III). The solution is

(36)
(37)

This solution corresponds to a staggered canting of spins away from the axis, as illustrated in Fig. 3. In the boson language, we can map this to a charge current using the definition

(38)

This state would correspond to a staggered charge current as shown in Fig. 3.

In MFT, the above state does not contain any charge density modulation, since the out-of-plane angle is found to be zero. However, one expects (e.g. based on Landau-Ginzburg type symmetry arguments) such charge density modulation to appear once fluctuations are included. Such a state is therefore a bosonic supersolid phase, with coexistent superfluidity and CDW order. Interestingly, from the modulation of the boson current operator illustrated in Fig. 3, it is clear that the supersolid phase in this case has the curious additional feature of valence-bond-like order coexisting with CDW density modulation, a situation which does not typically occur in lattice supersolids arising from such simple Hamiltonians. It is also worth noting that the mechanism for formation of this supersolid is distinct from that of other hard-core boson supersolid phases at commensurate filling discussed previously,Wessel and Troyer (2005); Heidarian and Damle (2005); Melko et al. (2005, 2006) which are induced by the geometrical frustration of the lattice.

Iv Finite-temperature Kosterlitz-Thouless transition

We turn now to a discussion of the superfluid phase in the J-K model at finite temperatures. The goal of this section will be to map out the finite-temperature phase boundaries of the superfluid phase in our linear SW theory, to compare (at least in part) to the results obtained in other studies. In the QMC work of Ref. Sandvik and Melko, 2006, the phase boundary reported has a non-trivial shape, reaching a maximum for a positive value of . We are interested in whether this feature can be captured by our SW theory, therefore elucidating the physical mechanism by which this maximum at occurs. To do this, we first develop an expression for the superfluid density for (Section IV.1), then use it to estimate the SW Kosterlitz-Thouless transition through the universal jump condition (Section IV.2).

iv.1 The finite-temperature superfluid density

At finite temperatures, we may calculate the superfluid density by recalling its original definition as the response of the free energy with respect to a twist. Calculating the partition function from Eq. (II) we obtain the free energy

(39)

with the dispersion redefined as

(40)

As noted previously, the twist-dependent terms in are proportional to , so we can write for

(41)

which is properly normalized with being the number of lattice bonds. Therefore, we obtain for the superfluid density

(42)
(43)

where the important limits are evaluated as follows:

(44)
(45)
(46)

Thus, this calculation yields the following expression for the superfluid density at finite-:

(47)

This SW expression for as a function of temperature is plotted for several parameters in Fig. 4.

Figure 4: (Color online) The superfluid density, calculated from Eq. (47), as a function of the temperature. Lines are labeled by the parameter value . The universal jump (Eq. (48)) is illustrated as a dashed line. The exact value for the Kosterlitz-Thouless transition for is , from unbiased QMC calculations.Melko et al. (2004b)

iv.2 Estimation of the Kosterlitz-Thouless transition

The superfluid density of Eq. (47), plotted as a function of , decays slowly (see Fig. 4), crossing zero for relatively large temperatures. However, as is well known, the XY model realizes a Kosterlitz-ThoulessKosterlitz and Thouless (1973) (KT) transition in any two-dimensional lattice, which is manifest as a discontinuity in precisely at . This, of course, can not be captured by a simple spin wave theory. We can, however, take advantage of the fact that the expected discontinuity in in 2D models such as this obeys the so-called universal jump condition,

(48)

first found by Nelson and Kosterlitz.Nelson and Kosterlitz (1977) One can thus hypothesize a reasonable estimate of by solving , using from our spin-wave theory. An important test of this idea can be performed at and , the parameter values for the XY model. This is illustrated in Fig. 4, where the crossing point of the dashed line and the curve for is our SW theory solution to Eq. (48). The value of obtained by this procedure is 0.6507, remarkably close to the exact result of , obtained from unbiased QMC calculations.Melko et al. (2004b)

We thus generalize this procedure of calculating in our linear SW theory to nonzero values of . Results are plotted in Fig. 5. As is evident by studying Fig. 4 closely, the SW theory reproduces the remarkable trend that increases for small to moderate values of . In Fig. 4, the maximum in occurs at , before beginning to drop slowly. The phase boundary for the KT transition drops to zero for the large value of , well outside of the expected range of validity for the SW calculation. Clearly, a simple spin-wave theory cannot capture the physics of the superfluid-VBS quantum phase transition that is observed in QMC simulations.

On the negative- side, the phase boundary drops rapidly to zero as approaches , confirming the expectation from SW theory that a transition to a supersolid phase, discussed in the previous sections, happens at this point.

Figure 5: (Color online) The KT transition phase boundary as calculated in linear SW theory. A maximum of occurs at approximately .

V Discussion

We have studied through linear spin wave theory the various mechanisms which destroy the superfluid phase in the bosonic ring-exchange model Eq. (1) at half-filling, motivated as a candidate to realize exotic phases in cold atomic gases in optical lattices.Büchler et al. (2005) As is known from previous QMC results,Sandvik et al. (2002) sufficiently large ring-exchange promotes: first, a quantum phase transition to a valence bond solid state; second, a quantum phase transition to a charge-density wave (CDW) state, at large . In this paper, we have shown that a moderate value of is also sufficient to destroy the superfluid phase, promoting a ordered phase that is identified as a supersolid, or a phase with coexisting superfluidity, CDW, and valence-bond-like order.

It is interesting to combine the exact results from QMC and our current SW theory results to speculate on the phase diagram for all parameters at half-filling. The supersolid phase that we find at must be related to the CDW phase found by exact QMC simulations for , since in the limit , the Hamiltonian Eq. (1) for maps exactly onto the Hamiltonian with , via a rotation of spins on one of the sub lattices by around the axis. For a finite value of , two possibilities exist for the evolution of the supersolid state to the CDW; the state can remain supersolid for all finite , or there could be a quantum phase transition between the supersolid and the CDW solid at some critical . In either case, we have identified in this paper that a supersolid phase is possible at half-filling in the relatively simple Hamiltonian Eq. (1) that has already been identified as a candidate for construction in ultracold bosons in optical lattices.Büchler et al. (2005)

Further, we have studied the finite-temperature phase boundary of the superfluid phase in linear SW theory, by calculating the superfluid density and estimating the Kosterlitz-Thouless transition temperature by forcing it to obey the universal jump condition. We find that this procedure yields good numerical agreement with exact QMC results for . For , the phase boundary monotonically decreases to at , indicating promotion of the supersolid phase discussed above. Increasing from the XY-point, the phase boundary initially increases, reaching a maximum for before monotonically decreasing. This is in qualitative agreement with the trend identified with QMC simulations,Sandvik and Melko (2006) and allows us to attribute at least the initial increase in for small to the physics of non-interacting spin waves. It is remarkable that such nontrivial information about this model, namely the non-monotonic behavior of as a function of , and the existence of a novel supersolid phase, can be contained in such a simple analytical theory.

Vi Acknowledgments

We are indebted to P. Nikolic, A. Paramekanti, A. Sandvik and D. Scalapino for enlightening discussions. Support for this work was provided by NSERC of Canada.

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