Lieb-Robinson bounds

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The Lieb-Robinson bound is a theoretical upper limit on the speed at which information can propagate in non-relativistic quantum systems. It demonstrates that information cannot travel instantaneously in quantum theory, even when the relativity limits of the speed of light are ignored. The existence of such a finite speed was discovered mathematically by Elliott Lieb and Derek William Robinson in 1972[1]. It turns the locality properties of physical systems into the existence of, and upper bound for this speed. The bound is now known as the Lieb-Robinson bound and the speed is known as the Lieb-Robinson velocity. This velocity is always finite but not universal, depending on the details of the system under consideration.

In the study of quantum systems such as quantum optics, quantum information theory, atomic physics, and condensed matter physics, it is important to know that there is a finite speed with which information can propagate. The theory of relativity shows that no information, or anything else for that matter, can travel faster than the speed of light. When non-relativistic mechanics is considered, however, (Newton's equations of motion or Schrödinger's equation of quantum mechanics) it had been thought that there is then no limitation to the speed of propagation of information. This is not so for certain kinds of quantum systems of atoms arranged in a lattice, often called quantum spin systems. This is important conceptually and practically, because it means that, for short periods of time, distant parts of a system act independently.

One of the practical applications of Lieb-Robinson bounds is quantum computing. Current proposals to construct quantum computers built out of atomic-like units mostly rely on the existence of this finite speed of propagation to protect against too rapid dispersal of information.[citation needed]

Review articles can be found in the following references, for example,[2][3][4]

Set up[edit]

To define the bound, it is necessary to first describe basic facts about quantum mechanical systems composed of several units, each with a finite dimensional Hilbert space.

Lieb-Robinson bounds are considered on a -dimensional lattice ( or ) , such as the square lattice .

A Hilbert space of states is associated with each point . The dimension of this space is finite, but this was generalized in 2008 to include infinite dimensions (see below). This is called quantum spin system.

For every finite subset of the lattice, , the associated Hilbert space is given by the tensor product

.

is a subspace of if .

An observable supported on (i.e., depends only on) a finite set is a linear operator on the Hilbert space .

When is finite dimensional, choose a finite basis of operators that span the set of linear operators on . Then any observable on can be written as a sum of basis operators on .

The Hamiltonian of the system is described by an interaction . The interaction is a function from the finite sets to self-adjoint observables supported in . The interaction is assumed to be finite range (meaning that if the size of exceeds a certain prescribed size) and translation invariant. These requirements were lifted later[5][6].

Although translation invariance is usually assumed, it is not necessary to do so. It is enough to assume that the interaction is bounded above and below on its domain. Thus, the bound is quite robust in the sense that it is tolerant of changes of the Hamiltonian. A finite range is essential, however. An interaction is said to be of finite range if there is a finite number such that for any set with diameter greater than the interaction is zero, i.e., . Again, this requirement was lifted later[5][6].

The Hamiltonian of the system with interaction is defined formally by:

.

The laws of quantum mechanics say that corresponding to every physically observable quantity there is a self-adjoint operator . For every observable with a finite support Hamiltonian defines a continuous one-parameter group of transformations of the observables given by

Here, has a physical meaning of time. (Technically speaking, this time evolution is defined by a power-series expansion that is known to be a norm-convergent series , see,[7] Theorem 7.6.2, which is an adaptation from.[8] More rigorous details can be found in.[1])

The bound in question was proved in[1] and is the following: For any observables and with finite supports and , respectively, and for any time the following holds for some positive constants and :

 

 

 

 

(1)

where denotes the distance between the sets and . The operator is called the commutator of the operators and , while the symbol denotes the norm, or size, of an operator . It is very important to note that the bound has nothing to do with the state of the quantum system, but depends only on the Hamiltoninan governing the dynamics. Once this operator bound is established it necessarily carries over to any state of the system.

A positive constant depends on the norms of the observables and , the sizes of the supports and , the interaction, the lattice structure and the dimension of the Hilbert space . A positive constant depends on the interaction and the lattice structure only. The number can be chosen at will provided is chosen sufficiently large. In other words, the further out one goes on the light cone, , the sharper the exponential decay rate is. (In later works authors tended to regard as a fixed constant.) The constant is called the group velocity or Lieb-Robinson velocity.

The bound (1) is presented slightly differently from the equation in the original paper.[1] This more explicit form (1) can be seen from the proof of the bound[1]

Lieb-Robinson bound shows that for times the norm on the right-hand side is exponentially small. This is the exponentially small error mentioned above.

The reason for considering the commutator on the left-hand side of the Lieb–Robinson bounds is the following:

The commutator between observables and is zero if their supports are disjoint.

The converse is also true: if observable is such that its commutator with any observable supported outside some set is zero, then has a support inside set .

This statement is also approximately true in the following sense:[9] suppose that there exists some such that for some observable and any observable that is supported outside the set . Then there exists an observable with support inside set that approximates an observable , i.e. .

Thus, Lieb-Robinson bounds say that the time evolution of an observable with support in a set is supported (up to exponentially small errors) in a -neighborhood of set , where with being the Lieb-Robinson velocity. Outside this set there is no influence of . In other words, this bounds assert that the speed of propagation of perturbations in quantum spin systems is bounded.

Improvements of the Lieb-Robinson bounds[edit]

In[10] Robinson generalized the bound (1) by considering exponentially decaying interactions (that need not be translation invariant), i.e., for which the strength of the interaction decays exponentially with the diameter of the set. This result is discussed in detail in,[11] Chapter 6. No great interest was shown in the Lieb-Robinson bounds until 2004 when Hastings[12] applied them to the Lieb–Schultz–Mattis theorem. Subsequently, Nachtergaele and Sims[13] extended the results of[10] to include models on vertices with a metric and to derive exponential decay of correlations. From 2005–2006 interest in Lieb–Robinson bounds strengthened with additional applications to exponential decay of correlations (see[5][6][14] and the sections below). New proofs of the bounds were developed and, in particular, the constant in (1) was improved making it independent of the dimension of the Hilbert space.

Several further improvements of the constant in (1) were made.[15] In 2008 the Lieb-Robinson bound was extended to the case in which each is infinite dimensional.[16] In[16] it was shown that on-site unbounded perturbations do not change the Lieb-Robinson bound. That is, Hamiltonians of the following form can be considered on a finite subset :

where is a self-adjoint operator over , which needs not to be bounded.

Harmonic and Anharmonic Hamiltonians[edit]

The Lieb-Robinson bounds were extended to certain continuous quantum systems, that is to a general harmonic Hamiltonian,[16] which, in a finite volume , where are positive integers, takes the form:

where the periodic boundary conditions are imposed and , . Here are canonical basis vectors in .

Anharmonic Hamiltonians with on-site and multiple-site perturbations were considered and the Lieb–Robinson bounds were derived for them,[16][17] Further generalizations of the harmonic lattice were discussed,[18][19]

Irreversible dynamics[edit]

Another generalization of the Lieb–Robinson bounds was made to the irreversible dynamics, in which case the dynamics has a Hamiltonian part and also a dissipative part. The dissipative part is described by terms of Lindblad form, so that the dynamics satisfies the Lindblad-Kossakowski master equation.

Lieb-Robinson bounds for the irreversible dynamics were considered by[14] in the classical context and by[20] for a class of quantum lattice systems with finite-range interactions. Lieb-Robinson bounds for lattice models with a dynamics generated by both Hamiltonian and dissipative interactions with suitably fast decay in space, and that may depend on time, were proved by,[21] where they also proved the existence of the infinite dynamics as a strongly continuous cocycle of unit preserving completely positive maps.

Some applications[edit]

Lieb–Robinson bounds are used in many areas of mathematical physics. Among the main applications of the bound there is the existence of the thermodynamic limit, the exponential decay of correlations and the Lieb–Schultz–Mattis theorem.

Thermodynamic limit of the dynamics[edit]

One of the important properties of any model meant to describe properties of bulk matter is the existence of the thermodynamic limit. This says that intrinsic properties of the system should be essentially independent of the size of the system which, in any experimental setup, is finite.

The static thermodynamic limit from the equilibrium point of view was settled much before the Lieb–Robinson bound was proved, see[7] for example. In certain cases one can use a Lieb–Robinson bound to establish the existence of a thermodynamic limit of the dynamics, , for an infinite lattice as the limit of finite lattice dynamics. The limit is usually considered over an increasing sequence of finite subsets , i.e. such that for , there is an inclusion . In order to prove the existence of the infinite dynamics as a strongly continuous, one-parameter group of automorphisms, it was proved that is a Cauchy sequence and consequently is convergent. By elementary considerations, the existence of the thermodynamic limit then follows. A more detailed discussion of the thermodynamic limit can be found in[22] section 6.2.

Robinson was the first to show the existence of the thermodynamic limit for exponentially decaying interactions.[10] Later, Nachtergaele et al.[6][17][21] showed the existence of the infinite volume dynamics for almost every type of interaction described in the section "Improvements of Lieb–Robinson bounds" above.

Exponential decay of correlations[edit]

Let denote the expectation value of the observable in a state . The correlation function between two observables and is defined as

Lieb–Robinson bounds are used to show that the correlations decay exponentially in distance for a system with an energy gap above a non-degenerate ground state , see.[5][13] In other words, the inequality

holds for observables and with support in the sets and respectively. Here and are some constants.

Alternatively the state can be taken as a product state, in which case correlations decay exponentially without assuming the energy gap above the ground state.[6]

Such a decay was long known for relativistic dynamics, but only guessed for Newtonian dynamics. The Lieb–Robinson bounds succeed in replacing the relativistic symmetry by local estimates on the Hamiltonian.

Lieb-Schultz-Mattis theorem[edit]

Lieb-Schultz-Mattis theorem implies that the ground state of the Heisenberg antiferromagnet on a bipartite lattice with isomorphic sublattices, is non-degenerate, i.e., unique, but the gap can be very small.[23]

For one-dimensional and quasi-one-dimensional systems of even length and with half-integral spin Affleck and Lieb,[24] generalizing the original result by Lieb, Schultz, and Mattis,[25] proved that the gap in the spectrum above the ground state is bounded above by

where is the size of the lattice and is a constant. Many attempts were made to extend this result to higher dimensions, ,

The Lieb–Robinson bound was utilized by Hastings[12] and by Nachtergaele-Sims[26] in a proof of the Lieb–Schultz–Mattis Theorem for higher-dimensional cases. The following bound on the gap was obtained:

.

Discretisation of the Continuum via Gauss-Quadrature Rules[edit]

In 2015, it was shown that the Lieb-Robinson bound can also have applications outside of the context of local Hamiltonians as we now explain. The Spin-Boson model describes the dynamics of a spin coupled to a continuum of oscillators. It has been studied in great detail and explains quantum dissipative effects in a wide range of quantum systems. Let denote the Hamiltonian of the Spin-Boson model with a continuum bosonic bath, and denote the Spin-Boson model who's bath has been discretised to include harmonic oscillators with frequencies chosen according to Gauss Quadrature Rules. For all observables on the Spin Hamiltonian, the error on the expectation value of induced by discretising the Spin-Boson model according to the above discretisation scheme is bounded by[27]

 

 

 

 

()

where are positive constants and is the Lieb-Robinson velocity which in this case is directly proportional to , the maximum frequency of the bath in the Spin-Boson model. Here, the number of discrete modes play the role of a distance mentioned below Eq. (1). One can also bound the error induced by local Fock space truncation of the harmonic oscillators[28]

Experiments[edit]

The first experimental observation of the Lieb–Robinson velocity was done by Cheneau et al.[29]

References[edit]

  1. ^ a b c d e E. Lieb, D. Robinson, The finite group velocity of quantum spin systems, Commun. Math. Phys. 28, 251–257, (1972)
  2. ^ B. Nachtergaele, R. Sims, Much Ado About Something: Why Lieb-Robinson bounds are useful, IAMP News Bulletin, October 2010, 22–29, (2010)
  3. ^ M. Kliesch, C. Gogolin, J. Eisert, Lieb-Robinson bounds and the simulation of time evolution of local observables in lattice systems, arXiv:1306.0716, (2013)
  4. ^ M. B. Hastings, Locality in quantum systems, arXiv:1008.5137
  5. ^ a b c d M. Hastings, T. Koma, Spectral Gap and Exponential Decay of Correlations, Commun. Math. Phys. 256, 781, (2006)
  6. ^ a b c d e B. Nachtergaele, Y. Ogata, R. Sims, Propagation of Correlations in Quantum Lattice Systems, J. Stat. Phys. 124, 1–13, (2006)
  7. ^ a b D. Ruelle, Statistical mechanics. Rigorous results, Benjamin, New York, 1969
  8. ^ D. W. Robinson, Statistical mechanics of quantum spin systems II. Comm. Math. Phys. 7, 337–348, (1968)
  9. ^ S. Bachmann, S. Michalakis, B. Nachtergaele, R. Sims, Automorphic Equivalence within Gapped Phases of Quantum Lattice Systems, Commun. Math. Phys. 309, 835–871, (2012)
  10. ^ a b c D. W. Robinson, Properties of propagation of quantum spin systems, J. Austral. Math. Soc. 19 (Series B), 387–399, (1976)
  11. ^ O. Bratteli, D. W. Robinson, Operator algebras and quantum statistical mechanics, 1ed., vol. 2, Springer-Verlag, 1981 and 2 ed., vol. 2, Springer-Verlag, 1997
  12. ^ a b M. Hastings, Lieb–Schultz–Mattis in higher dimensions, Phys. Rev. B 69, 104431–10444, (2004)
  13. ^ a b B. Nachtergaele, R. Sims, Lieb-Robinson bounds and the exponential clustering theorem, Commun. Math. Phys., 265, 119–130, (2006)
  14. ^ a b M. Hastings, Locality in quantum and Markov dynamics on lattices and networks, Phys. Rev. Lett. 93, 140402, (2004)
  15. ^ B. Nachtergaele, R. Sims. Locality Estimates for Quantum Spin Systems, Sidoravicius, Vladas (Ed.), New Trends in Mathematical Physics. Selected contributions of the XVth International Congress on Mathematical Physics, Springer Verlag, 591–614, (2009)
  16. ^ a b c d B. Nachtergaele, H. Raz, B. Schlein, R. Sims, Lieb-Robinson bounds for harmonic and anharmonic lattice systems, Commun. Math. Phys. 286, 1073–1098, (2009)
  17. ^ a b B. Nachtergaele, B. Schlein, R. Sims, S. Starr, V. Zagrebnov, On the existence of the dynamics for anharmonic quantum oscillator systems, Rev. Math. Phys., 22, 207–231, (2010)
  18. ^ M. Cramer, A. Serafini, J. Eisert, Locality of dynamics in general harmonic quantum systems, arXiv:0803.0890, (2008)
  19. ^ J. Juenemann, A. Cadarso, D. Perez-Garcia, A. Bermudez, J. J. Garcia-Ripoll, Lieb–Robinson bounds for spin-boson lattice models and trapped ions, arXiv:1307.1992, (2013)
  20. ^ D. Poulin, Lieb–Robinson bound and locality for general Markovian quantum dynamics, Phys. Rev. Lett. 104, 190401, (2010)
  21. ^ a b B. Nachtergaele, A. Vershynina, V. Zagrebnov, Lieb-Robinson bounds and Existence of the thermodynamic limit for a class of irreversible quantum dynamics, AMS Contemporary Mathematics, 552, 161–175, (2011)
  22. ^ O. Bratteli, D. W. Robinson, Operator algebras and quantum statistical mechanics, 2 ed., vol. 2, Springer Verlag, 1997
  23. ^ E. Lieb, D. Mattis, Ordering energy levels in interacting spin chains, Journ. Math. Phys. 3, 749–751, (1962)
  24. ^ I. Affleck, E.H. Lieb, A proof of part of Haldane’s conjecture on quantum spin chains, Lett. Math. Phys. 12, 57–69, (1986)
  25. ^ E. Lieb, T. Schultz, D. Mattis, Two soluble models of an antiferromagnetic chain, Ann. Phys. (N.Y.) 16, 407–466, (1961)
  26. ^ B. Nachtergaele, R. Sims, A multi-dimensional Lieb–Schultz–Mattis theorem, Commun. Math. Phys. 276, 437-472, (2007)
  27. ^ M.P. Woods & M.B. Plenio, Dynamical error bounds for continuum discretisation via Gauss quadrature rules, --A Lieb-Robinson bound approach, J. Math. Phys. 57, 022105 (2016), ArXiv
  28. ^ M.P. Woods, M. Cramer & M.B. Plenio, Simulation Bosonic Baths with Error bars, Phys. Rev. Lett. 115, 130401 (2015) ArXiv
  29. ^ M. Cheneau, P. Barmettler, D. Poletti, M. Endres, P. Schauß, T. Fukuhara, C. Gross, I. Bloch, C. Kollath, S. Kuhr, Light-cone-like spreading of correlations in a quantum many-body system, Nature 481, 484–487, (2012)