Suppression of transport in non-disordered quantum spin chains due to confined excitations

Suppression of transport in non-disordered quantum spin chains
due to confined excitations

P. P. Mazza SISSA – International School for Advanced Studies & INFN, via Bonomea 265, 34136 Trieste, Italy    G. Perfetto SISSA – International School for Advanced Studies & INFN, via Bonomea 265, 34136 Trieste, Italy    A. Lerose SISSA – International School for Advanced Studies & INFN, via Bonomea 265, 34136 Trieste, Italy    M. Collura The Rudolf Peierls Centre for Theoretical Physics, Oxford University, Oxford, OX1 3NP, United Kingdom    A. Gambassi SISSA – International School for Advanced Studies & INFN, via Bonomea 265, 34136 Trieste, Italy
Abstract

The laws of thermodynamics require any initial macroscopic inhomogeneity in extended many-body systems to be smoothed out by the time evolution through the activation of transport processes. In generic, non-integrable quantum systems, transport is expected to be governed by a diffusion law, whereas a sufficiently strong quenched disorder can suppress it completely due to many-body localization of quantum excitations. Here we show that the confinement of quasi-particles can also lead to transport suppression even if the dynamics are generated by homogeneous Hamiltonians. We demonstrate this in the quantum Ising chain with transverse and longitudinal magnetic fields in the paradigmatic case of the evolution of domain-wall states. We perform extensive numerical simulations of the dynamics which turn out to be in excellent agreement with an effective analytical description valid within both weak and strong confinement regimes. Our results show that the energy flow from “hot” to “cold” regions of the chain is suppressed for all accessible times. We argue that this phenomenon is connected with the presence of atypical states in the many-body energy spectrum which violate the eigenstate thermalization hypothesis, as recently reported in the literature.

pacs:

Introduction— Recent times have witnessed an increasing attention in the non-equilibrium dynamics of isolated quantum many-body systems Noneq (); Noneq1 (); Noneq2 (). This interest has been prompted by an impressive advance in experimental techniques with cold atoms that made it possible to maintain coherent quantum dynamics for sufficiently long times exp1 (); exp2 (); exp3 (); exp4 (); exp5 (); exp6 (); exp7 (); exp8 (); exp9 (); exp10 (); exp11 (); exp12 (); exp13 (); exp14 (); exp15 (). The simplest protocol to drive a system out of equilibrium is the so-called quantum quench quench1 (); quench2 (); quench3 (), in which the dynamics of the system are monitored after a sudden change of a parameter of its Hamiltonian.

In this context, a fundamental question concerns whether and how the transport of globally conserved physical quantities such as particle and energy densities arises in these non-equilibrium quantum many-body systems transexp1 (); transexp2 (). The spatial spreading of local inhomogeneities in isolated systems is generically expected to obey a diffusion law, whose microscopic origin is usually traced back to the occurrence of inelastic collisions mesoscopic1 (); mesoscopic2 ().

These transport processes can be conveniently studied via inhomogeneous quenches inhomogeneous1 (); inhomogeneous2 () in which two subsystems initially prepared in two different equilibrium states, are joined by means of a local interaction. In this framework, transport may be enhanced by the existence of stable quasi-particles traveling ballistically with certain characteristic velocities, as in the case of integrable systems. Indeed, around the junction, a non-equilibrium stationary state may arise, supporting ballistic transport and thus finite currents at long times. These current-carrying states have been investigated in conformal field theories cft1 (); cft2 (); cft3 () and in non-interacting models, where, in addition, exact expressions can be obtained for the non-equilibrium profiles of local quantities in the so-called hydrodynamic scaling limit, showing the emergence of a light cone trans1 (); trans2 (); trans3 (); trans4 (); trans5 (); trans6 (); trans7 (); trans8 (); trans9 (); trans10 (); trans11 (); trans12 (); trans13 (). Such a hydrodynamic approach has been recently extended to interacting integrable models, leading to a set of generalized hydrodynamical equations for local conserved quantities ghd1 (); ghd2 (); ghd3 (). These equations can predict non-ballistic transport when the underlying spectrum is gapped ghd4 (), but they cannot describe the diffusive regime observed numerically in Refs. diffusive1 (); diffusive2 (); diffusive3 (); diffusive4 (); diffusive5 (); diffusive6 () and analytically in Ref. kormos ().

A completely different scenario emerges in strongly disordered quantum systems in the so-called many-body localized phase anderson (); basko (); huse (). In fact, the localization of excitations ros (); abanin () suppresses the energy and particle transport and therefore initial gradients of local quantities persist for arbitrarily long times during the evolution vipin1 (); vipin2 (); Moore ().

Disordered-induced localization, however, is not the sole mechanism which hinders the propagation of information in many-body interacting systems. Indeed, it has been recently shown that, even in the absence of disorder, the dynamical confinement of excitations can suppress the spreading of correlations Calabrese (). How can this be reconciled with the heuristic expectation that an initial inhomogeneous configuration has to be smoothed out by the evolution? In this work we address this issue and show that a non-integrable, non-disordered quantum spin chain with confined excitations, initially prepared in domain-wall states with a finite energy gradient, can exhibit suppression of energy transport.

Figure 1: Evolution of the energy density (left panel) and of the energy current density (right panel) profiles, governed by the Hamiltonian (1) starting from the inhomogeneous domain-wall state (2), obtained from TEBD simulations, for a range of increasing field values (), () and , varying as indicated by the axes. (Units are fixed such that .) The same qualitative behavior as that illustrated here persists up to long times . Note the oscillations of the profiles around the junction, with spatial amplitude and frequency , while there is no evidence for the activation of transport.

Model and protocol. —

We consider a ferromagnetic quantum Ising chain with a transverse and a longitudinal magnetic field, and , respectively:

(1)

Here are the Pauli matrices acting on the site , is the Ising exchange parameter, the (even) system size, and we consider open boundary conditions. For , the model is exactly solvable in terms of free fermions schultzmattislieb () which, in the ferromagnetic phase with , physically correspond to freely moving domain-walls (or kinks) connecting the two oppositely magnetized ground states with . A finite causes a non-perturbative modification of the spectrum of the elementary excitations: it selects as a ground state the one with along and raises the energy of configurations with domains of reversed spins by an amount proportional to their extension. This corresponds to a linear, V-shaped interaction potential between two consecutive kinks delimiting a domain, which therefore become confined into composite objects called mesons, in analogy with the low-energy limit of quantum chromodynamics. This modification of the spectrum has been studied both in the vicinity of the critical point exploiting field-theoretical methods McCoy (); Muss (); Zam (), and far away from it in the regime of low-density excitations for small Rut0 ().

Here we consider a domain-wall initial state with a single kink in the middle of the chain which reads, in terms of the eigenstates and of ,

(2)

and which is also an eigenstate of . The quench protocol consists in switching on the transverse field and studying the non-equilibrium evolution of the energy density profile as a function of , where

(3)

For , the initial energy density is equal on the two sides of the junction, due to the symmetry. However, in the presence of a non-vanishing , the chain acquires an initial macroscopic energy imbalance between the left (“cold”) part and the right (“hot”) part. In particular, the latter may be viewed as a “false vacuum” whose energy lies in the middle of the many-body spectrum, and may thereby be expected to decay into a finite density of traveling excitations upon activating the transverse field , leading to a meltdown of the initial imbalance after a transient Rut1 (). In the following we provide compelling evidence against this expectation.

Numerical analysis— In order to explore numerically the non-equilibrium evolution of the chain, we employ time-evolving block decimation (TEBD) simulations TEBD (). It turns out that the entanglement grows slowly up to moderate values of the field , which allows us to extend the simulations to long times with modest computational efforts, as in the case of Ref. Calabrese (). We investigate the behavior of [see Eq. (3)] and of the associated current , with

(4)

for various values of . The results of the simulations are illustrated in Fig. 1 only up to times , as no qualitative differences are observed up to . In both the “strong” () and “weak” () confinement regime, energy transfer between the two halves of the chain is suppressed even at late times. As shown in Fig. 1, the main dynamical effect of the quench is given by pronounced oscillations of the profiles around the position of the junction, with characteristic emergent amplitudes and frequencies which depend on the values of the fields. In particular, the energy current density does not vanish only around the junction, with an oscillating behavior which allows local instantaneous flows of energy against the macroscopic gradient. We emphasize that, within our protocol, an increase in the energy gradient between the two halves, caused by a stronger , does not result in the activation of transport: on the contrary, it turns out that the oscillations at the junction acquire an even smaller amplitude.

Figure 2: Comparison between the numerical results , , (symbols), and the analytical predictions , , (solid lines) for the magnetization (left panel), energy density (central panel) and energy density current (right panel) respectively, at the junction , as obtained from ED (with ) or TEBD (with or ), and from the effective single-particle model, respectively. These curves refer to , (top row), and , (bottom row). (Units are fixed such that .)

Effective dynamics— The oscillations of the profiles shown in Fig. 1 may be interpreted as the quantum motion of the isolated kink initially localized at the junction, triggered by the transverse field . In fact, the kinetic energy associated with this motion has a finite bandwith on the lattice, and therefore, because of energy conservation, the kink quasi-particle can travel, in the linear confining potential , at most a distance (confinement length scale), before bouncing back and oscillating. This phenomenon is analogous to the Wannier-Stark localization of electrons in a one-dimensional crystal subject to a constant electric field wannier ().

In order to rationalize the above intuition and make quantitative predictions on the evolution of the profiles, we propose a simple analytical approach based on dressing the meson quasi-particles perturbatively in the transverse field , with arbitrary . (This regime differs from the one , , of validity of the semiclassical technique of Ref. Rut0 ().) The approximation consists in neglecting the creation of new quasi-particles, which, in our setup, only affect the quantum fluctuations in the two homogeneous bulks away from the junction, as recognized in Refs. Calabrese (); Rut0 (). In fact, we show that the dynamics at the junction is very well captured within this scheme up to moderate values of .

In the spirit of an effective quasi-particle description of mesons cinesi (), we map the motion of the isolated kink onto the problem of a single quantum particle hopping on a one-dimensional lattice, by projecting the many-body Hilbert space onto the single-kink linear subspace SupplMat (). For and arbitrary 111 Note, however, that resonances occur at particular values of , commensurate with . Correspondingly, it costs no energy to break a single meson into multiple mesons by flipping individual spins. These transitions cause quantitative but not qualitative modifications to the evolution of the energy profile, which are not captured by the single-kink subspace projection discussed here. Evidence of this aspect can be found in the Supplemental Material. the dynamics essentially occurs within this subspace, spanned by the states with a single domain-wall located between sites and , with . The corresponding unperturbed energy eigenvalues are . The resulting matrix elements of the Hamiltonian (1) read , with and

(5)

We note that the off-diagonal perturbation produces an effective hopping amplitude for the kink quasi-particle. Accordingly, the effective Hamiltonian describes the dynamics in terms of a single particle hopping in a one-dimensional lattice in the presence of a linear potential, where the state of the particle is described by a vector with . The absolute value squared of the -th component of the wavefunction is equal to the probability that the particle is at site at time . Within this picture, the initial state in Eq. (2) maps to , corresponding to a particle completely localized at the junction between the two chains. Similarly, the magnetization at site and time can be expressed SupplMat () within this single-particle picture as

(6)

where is the time evolved state within the projected space.

In order to test the accuracy of our approximation, we compare the dynamics obtained from the above effective single-particle problem with the exact dynamics generated by [see Eq. (1)] in the full many-body Hilbert space, starting from the domain-wall initial state of Eq. (2) as obtained via both exact diagonalization (ED) and TEBD techniques 222In this case, the simulations based on exact diagonalization of the Hamiltonian can be pushed until sufficiently late times because finite-size effects such as revivals are suppressed, due to the fact that excitations are confined Calabrese ().. The comparison between and is shown in Fig. 2. In particular, we observe that the agreement is fairly good up to moderate values of the transverse field .

Similarly, the relevant non-equilibrium profiles of the energy and energy current densities can be studied within the above effective single-particle description. This is achieved by projecting the energy density at site in Eq. (3) onto the single-kink subspace,

(7)

where the sign function equals for , for and for . From the continuity equation

(8)

we can infer the corresponding effective expression for the energy current density operator at site , i.e.,

(9)

The time-dependent expectation value of the energy density at site within this single-particle picture can therefore be simply written as

(10)

with an analogous expression for the current . In Fig. 2 we compare the time evolution of and with the corresponding exact quantities and as obtained from the TEBD simulations. The agreement is excellent for small values of the transverse field, whereas for larger values , small quantitative discrepancies appear, still retaining a fairly good qualitative agreement.

Conclusions— In a homogeneous quench, the confinement of excitations has been recently shown to hinder the spreading of correlations in the quantum Ising chains (1) with both transverse and longitudinal magnetic fields Calabrese (). In this work, we have shown that this phenomenon has significant consequences even in inhomogeneous setups, as it can lead to suppression of energy transport. This lack of transport in the presence of an initial gradient actually mirrors here a more general lack of approach to thermal equilibrium: the spatial inhomogeneity in the longitudinal magnetization persists at long times, meaning that the system fails to locally relax to the thermal ensemble, contrary to what is widely believed to be the case for non-integrable extended systems ETH ().

We emphasize that in the problem discussed here the specific choice of the class of inhomogeneous initial states plays an important role. As we have shown, the non-equilibrium dynamics are accurately captured by the oscillations of a single macroscopically large “meson”. Based on extensive numerical work, it has been recently suggested in Ref. Konik (), that the Hamiltonian (1) is characterized by a pattern of atypical energy eigenstates with non-thermal features carrying over to the thermodynamic limit, which violate the eigenstate thermalization hypothesis. In this light, our results may represent a dynamical manifestation of this phenomenon. In particular, if the initial states have significant overlap with those “single-meson” non-thermal eigenstates, the initial inhomogeneity would persist to infinite time. However, we argue that more general initial states, with magnetic domains separated by distances much larger than the confinement length scale, would also retain their inhomogeneity for a correspondingly long time.

We plan to extend this analysis to other related models, such as the XXZ spin chain in staggered field Rut2 (), as well as to long-range Ising chains, which are relevant to experiments with trapped ions Monroe (); Blatt () and with Rydberg atoms Lukin (). We finally observe that recent works have reported the occurrence of localization – and thereby of suppression of information spreading – within the context of lattice gauge theories, where confinement of elementary excitations arise as well Gauge-inv (); Montangero (). It would be interesting to investigate the possible connection between these findings and the results discussed here.

Acknowledgments— We acknowledge useful discussions with P. Calabrese, G. B. Mbeng, J. Moore, G. Pagano, N. Robinson, and S. B. Rutkevich. We thank G. Giudici for technical help with the numerical codes. The work of M. C. was supported by the European Union’s Horizon 2020 research and innovation programme under the Marie Sklodowska-Curie Grant Agreement No. 701221.

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Supplemental Material:

Suppression of transport in non-disordered quantum spin chains

due to real-time confinement

This supplemental material is organized as follows: in Sec. I we motivate the effective single-particle approach used in the main text, in Sec. II we define the restricted single-kink subspace and derive the effective Hamiltonian which governs the time evolution within this subspace, in Sec. III we study the corresponding dynamics of the energy and energy current densities, while in Sec. IV we briefly discuss the range of validity of this approach and its limitations.

Appendix A Motivation for the effective single-particle approach

As briefly outlined in the main text, we focus on the dynamics generated by in Eq. (1), within a perturbative expansion for and therefore we first discuss the structure of the spectrum of the unperturbed Hamiltonian . Its eigenstates can be written in terms of the eigenvectors , of the Pauli matrix . Examples of these eigenstates are reported in Fig. S1, where the various arrows correspond to the lattice sites of the chain.

Figure S1: Schematic representation of some excited states of , where the arrows indicate the eigenvectors , of at the various lattice sites of the chain while the red vertical bars indicate the occurrence of domain-walls or kinks.

In particular, the ground state of is

(S1)

for (a similar analysis can be done for ). The energy levels of the excited states can be characterized by two quantum numbers, namely the total number of kinks (or domain-walls) and the total number of reversed spins (i.e., arrows pointing downward), as

(S2)

with . Note that the corresponding eigenspaces are highly degenerate, because energy is unchanged upon separately shifting each domain with consecutively reversed spins (“meson”) by arbitrary distances, retaining the same number of kinks . Given this structure, we can pictorially arrange the energy levels of the excited states in bands labelled, e.g., by the number of kinks, as reported in Fig. S2.

Figure S2: Energy spectrum of the excited states of . From the initial state marked in red, belonging to the single-kink () band shaded in blue, the allowed transitions at first order in are indicated by the various arrows and they correspond to single spin flips. If , the transitions (dashed arrows) occurring outside the single-kink band are suppressed with respect to those (solid arrows) occurring within it.

When the perturbation

(S3)

is switched on, transitions between states and become possible, where () denotes a representative state in the eigenspace identified by and ( and ). For the single-kink () initial states considered in the main text, the possible transitions occurring up to the first order in are schematically shown in Fig. S2. In particular, they change by one, while can either remain constant or increase by two (in this discussion, for simplicity we disregard spin flips occurring at the boundary of the chain), i.e.,

  1. ;

  2. .

At the first order in perturbation theory, the associated long-time transition amplitudes are proportional to the matrix element of the perturbation between the two states divided by their energy difference (see, e.g., Ref. sakurai ()), i.e., to

  1. ;

  2. .

For , the probability amplitude of process 1 above is much larger than that of process 2. Accordingly, transitions between single-kink states dominate the dynamics, which therefore can be conveniently projected onto the subspace spanned by these states (see Fig. S2). If the value of is, instead, comparable to or larger than , the transitions discussed above are generically suppressed as long as the corresponding energy denominators do not vanish. For further details on the range of validity and on the limitations of the present single-particle approach, see Sec. IV.

Appendix B Effective dynamics within the single-kink subspace

Within the perturbative regime , the dynamics of the system prepared in the state involve only single-kink states. Accordingly, we can project it onto the -dimensional subspace spanned by the states with a single kink located between the lattice sites and , i.e.,

(S4)

As already stated in Sec. A, for simplicity we assume , such that the single “meson” in the state is given by a block of spins reversed with respect to the longitudinal field direction . Note that the initial state in Eq. (2) of the main text corresponds to . These states are eigenstates of the Hamiltonian ,

(S5)

where the ground state energy of is an additive constant which we neglect in what follows. The transverse field provides a kinetic energy to the kinks and, as a matter of fact, it allows transitions from the state to states : since (and ), one has

(S6)

where is defined in Eq. (S3). Accordingly, the effective Hamiltonian governing the evolution of the system in the single-kink subspace reads

(S7)

which is Eq. (5) in the main text. This Hamiltonian determines the time evolution of observables in the single-kink subspace and it can therefore be used to study the dynamics of the magnetization at each lattice site . Within the single-kink subspace spanned by the states in Eq. (S4), a generic vector can be written as

(S8)

with suitable coefficients . The average longitudinal spin component at site can therefore be written as

(S9)

where we have exploited the identity

(S10)

in which the unit step is defined such that and . Hence, the dynamics of the magnetization is readily obtained as

(S11)

in terms of the coefficients of the time-evolved state. In the problem considered in the main text, the initial state is a kink localized in the middle of the chain, corresponding to , and therefore .

Appendix C Representation of transport observables in the single-kink subspace

The same procedure as the one described in Sec. II can be repeated for the energy density, Eq. (3) in the main text. In particular, by using the fact that (), we obtain

(S12)

which, together with Eq. (S10), yields Eq. (7) of the main text. The energy density operator at site obtained in this way is a well-defined density, since its sum over the lattice sites of the chain renders the projected Hamiltonian , i.e.,

(S13)

The energy current density at site in the single-kink subspace can be conveniently defined by writing the commutator between and as a divergence of a local current, as done in Eqs. (8) and (9) of the main text. Note that the energy current obtained in this way differs from the one which would have been obtained by projecting directly the current operator in Eq. (4) of the main text on the single-kink subspace, with an analogous prescription as the one followed above for . In fact, this procedure would have led to

(S14)

which differs from in Eq. (9) of the main text by terms of order . This can be realized by considering the continuity equation which defines the energy density and current at the operator level, i.e.,

(S15)

with , , given by Eqs. (1), (3) and (4), respectively, of the main text. By projecting this equation over the single-kink subspace spanned by the indices , one finds

(S16)

On the other hand, in the regime of validity of our approximation scheme, corresponding to , terms of order in Eq. (9) are negligible and there is actually no difference in using the definition of Eq. (S14) or the one in Eq. (9) of the main text. The latter, however, has been preferred in order to have an effective energy current operator which satisfies the continuity equation (8) of the main text.

Appendix D Range of validity and limitations

The agreement between the effective dynamics within the single-kink subspace discussed in the previous sections and the exact dynamics in the full many-body Hilbert space is fairly good for arbitrary values of , as shown in Fig. (2) of the main text and for a wider range of parameters in Fig. S3.

Figure S3: Comparison between the effective dynamics within the single-kink subspace (solid line) and the exact dynamics in the full many-body Hilbert space [symbols, determined via exact diagonalization (ED) with ] for both small (, left panel) and intermediate (, right panel) values of . Here and units are fixed such that . Although the data shown here refer to the average magnetization at the center of the chain, a similar agreement is observed for the average energy density and energy current density up to similar times.

However, if and are commensurable, degeneracies occur in the unperturbed energy spectrum in Eq. (S2). In particular, this happens when the energies and of two states and , respectively, are equal, i.e., when

(S17)

If two such states are connected by spin flips, then resonances occur at the -th order in perturbation theory, and therefore their effect becomes manifest only at a correspondingly long time scale.

For instance, at the first order in , the process 2 above is resonant when . In this case, it costs no energy to break the single initial meson into multiple mesons via single spin flips. During the evolution, a finite density of isolated reversed spins is thus generated, thereby lowering the average local magnetization. Since these states have , they no longer belong to the single-kink subspace and the effective single-particle description employed in the main text is therefore not expected to properly capture the resulting dynamics, as indeed demonstrated in Fig. S4. However, as long as the perturbation is small, these reversed domains have a low spatial density and therefore they all have zero momentum (cf. Ref. [63] of the main text). Accordingly, in this perturbative regime, transport is not expected to be activated by the presence of these resonances, as shown in Fig. S5.

Figure S4: Comparison between the numerical data [determined by exact diagonalization (ED) with ] of the magnetization at the junction and the corresponding analytical prediction . At variance with what is observed in Fig. S3, a qualitative discrepancy emerge between the two curves, due to resonances at first order in perturbation theory. These curves refer to and , where the units are fixed such that .
Figure S5: Energy density profile as a function of the coordinate along the chain [determined by exact diagonalization (ED) with ] and of time , for , and , where units are fixed such that . In spite of the resulting resonance at the first order in , no energy flow from right to left is observed.

References

  • (83) J. J. Sakurai, E. D. Commins, Modern quantum mechanics, Addison Wesley (1995).
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