Abstract
Remarkable progress of quantum information theory (QIT) allowed to formulate mathematical theorems for conditions that datatransmitting or dataprocessing occurs with a nonnegative entropy gain. However, relation of these results formulated in terms of entropy gain in quantum channels to temporal evolution of real physical systems is not thoroughly understood. Here we build on the mathematical formalism provided by QIT to formulate the quantum Htheorem in terms of physical observables. We discuss the manifestation of the second law of thermodynamics in quantum physics and uncover special situations where the second law can be violated. We further demonstrate that the typical evolution of energyisolated quantum systems occurs with nondiminishing entropy.
Introduction
In the 1870s, Ludwig Boltzmann published his celebrated kinetic equation and the Htheorem^{1,2} that gave the statistical foundation of the second law of thermodynamics^{3}. The Htheorem states that if f(x; v; τ) is the distribution density of molecules of the ideal gas at the time τ, position x and velocity v, which satisfies the kinetic equation, then entropy defined as is nondiminishing, i.e. that . Boltzmann’s kinetic equation rests on the molecular chaos hypothesis which assumes that velocities of colliding particles are uncorrelated and independent of position. Striving to bypass molecular chaos hypothesis, unjustified within the classical mechanics, John von Neumann proposed^{4} pure quantum mechanical origin of the entropy growth. He defined entropy through quantum mechanical density matrix as , and offered a proof of nondecreasing entropy resting on the final procedure of macroscopic measurement. As this proof yet invoked concepts going beyond pure quantum mechanical treatment, the nonstop tireless search for the quantum mechanical foundation of the Htheorem have been continuing ever since, see ref. 5 for a review. At the same time there have been a remarkable progress in quantum information theory (QIT), which formulated several rigorous mathematical theorems about the conditions for a nonnegative entropy gain^{6,7}. In this communication we show how the results of QIT apply to physical quantum systems and phenomena establishing thus nondiminishing von Neumann’s entropy in physics and formulate the conditions under which the evolution accompanied by nondiminishing entropy arises within pure quantum mechanical framework.
To describe quantum dynamics of an open system, the quantum information theory introduces the socalled quantum channel (QC) defined as a tracepreserving completely positive map, , of a density matrix^{6}. A remarkable general result of the QIT states that the entropy gain in a channel is^{8}
where is the identity operator. This formula was derived from the monotonicity property^{9} of the relative entropy under the quantum channel Φ : , where . There exists a wide class of channels, the socalled unital channels, defined by the relation , for which the right hand side of Eq. (1) vanishes, , so that the entropy gain is nonnegative, . Then within the framework of the QIT one can formulate the quantum Htheorem as follows: the entropy gain during evolution is nonnegative if the system evolution can be described by the unital channel. Moreover, for a quantum system endowed with the finite Ndimensional Hilbert space, the unitality condition becomes not only a sufficient, but also the necessary condition for nondiminishing entropy. Indeed, let us assume that for any initial state of a system with Ndimensional Hilbert space, the entropy gain in a channel Φ is nonnegative. It then follows that for the chaotic state that already has the maximal entropy, , the entropy cannot grow, . Thus , therefore, and the channel is unital. For an infinitedimensional quantum system the entropy is not continuous^{10}, and this situation requires special consideration. Finally, it is noteworthy that there exist certain classes of states that evolve with even if the channel is not unital^{11}.
To connect the general result (1) and the related mathematical Htheorem formulation to the realm of physics note that any quantum system interacting with the reservoir generates a quantum channel. Indeed, let us consider joint evolution of the grand system, comprising a given quantum system and a reservoir initially prepared in a disentangled state, , where is the density matrix of the reservoir. Let be the unitary operator describing the temporal evolution of the grand system. Then, according to the StinespringKraus dilation theorem^{6} is the quantum channel. Note that the evolution from an initially entangled state may be accompanied by the arbitrary gain in entropy. This demonstrates the necessity of the disentanglement condition. Examples of how the initially entangled system can evolve with the decreasing entropy are given e.g. in refs 12 and 13.
To compare how do the classical and quantum Htheorems work, note that for the former to hold, the classical distribution function of the system involved should obey the kinetic equation. The constraint imposed on the evolution of the density matrix of the quantum system is that the corresponding quantum channel is unital. This defines our task as to find out the necessary conditions under which the temporal dynamics of a quantum system endowed with the specific interaction with environment can be modeled by the unital quantum channel. Below, we formulate these conditions for the so called quasiisolated quantum systems with the negligible energy exchange with environment and demonstrate how do they apply to generic exemplary physical realizations.
Quantum Htheorem
In physics the positive entropy gain, according to the second law of thermodynamics, is ensured by the energy isolation of the evolving system. In contrast to the classical formulation of the second law where any isolated classical system evolves with the nondiminishing entropy, its literal extension onto the quantum case is meaningless since the entropy of any isolated quantum system does not change, . Hence, to bring the thermodynamic meaning to the consideration of quantum evolution one has to allow an interaction with the environment and establish the notion of the quasiisolated system. However, letting an arbitrarily systemenvironment interaction causes immediate problem. The energy exchange ΔE between the system and environment at temperature T and its entropy gain are related in classical thermodynamics as ΔS = ΔE/k_{B}T. One would expect that in a quantum case the similar relation also might hold provided the quantum system interacted with the macroscopic reservoir during the sufficiently long time. Moreover, long time evolution of a quantum system which exchanges energy with an environment can not, in general, be described by the unital channel at all. Indeed, consider a finite dimensional quantum system with N discrete nondegenerate energy states E_{n}〉 initially prepared in the chaotic state . Then the longtime interaction with the low temperature environment drives the system into the low energy states and hence the resulting quantum channel becomes nonunital, . Therefore, one has to restrict allowable interactions to the class of interactions that provide the system’s entanglement with the environment, but yet keep the energy exchange with the environment negligible. Such an interaction, for example, is realized for a specific environment of nuclear spins which possesses a highly energydegenerate ground state. For a general situation of the environment endowed with the lowenergy excitations, one can employ the concept of the quasiisolated system provided there is a time separation between the the dephasing time T_{2} of the offdiagonal elements of the density matrix and the relaxation time of its diagonal elements, T_{1}. Then in the intermediate time evolution regime the system gets entangled with its environment but its energy exchange remains still negligible. Accordingly, in what follows we discuss the systems energyisolated from the reservoir. Furthermore, we will be assuming that our systems are initially disentangled from the reservoir.
Let us consider a fixed energy subspace E of the system Hilbert space spanned by the orthonormal basis states ψ_{i,E}〉, , where index i denotes all the remaining nonenergy system’s degrees of freedom and is the system Hamiltonian. It is convenient to present the evolution operator, , of the grand system (a system plus reservoir) as
where s_{ji,E} are the components of the scattering matrix corresponding to the transition amplitude between the system’s quantum states ψ_{i,E}〉 → ψ_{j,E}〉 (without taking into account interaction with the reservoir) and operators are the family of operators acting in the reservoir Hilbert space, with the subscripts i, j, and E specifying the system’s states (for details see Supplementary Section S1). The factorization into s_{ji,E} and is not unique, so we will be choosing the most suitable one for each particular case.
For an energyisolated quantum system the quantum states at different energies transform independently. To determine whether the evolution belongs in the class of the unitality channel, one has to check if the system obeys the relation. Using the unitarity of , one finds
where 〈…〉 is averaging with respect to the initial state of the reservoir, and (the proof is presented in Supplementary Section S2). This relation is our central result. It establishes the criterion for unitality of the energyisolated system in terms of physical operators describing the interaction of the quantum system with the reservoir. Combining the concept of unitality and relation (3) we reformulate quantum Htheorem as follows.
Let the quantum system interacting with the reservoir be initially disentangled from it and be energyisolated during the evolution. Let , where operators and coefficients s_{ji,E} are defined as in Eq. (2), for energies E at which the system can be found with a finite probability, i.e. . Then the resulting quantum channel is unital in the subspace spanned by the states ψ_{E,i}〉 with a finite and hence the quantum system evolves with a nonnegative entropy gain .
There may be two major scenaria by which the right hand side of the Eq. (3) can vanish: (i) The ‘microscopic’ scenario where the reservoir operators commute individually, ; and (ii) The ‘macroscopic’ scenario where only the averaged commutators vanish, , while individual operators do not. Below we demonstrate that the scenario (i) is realized for the electron interacting with the phonon bath, under the condition of the quasielastic scattering, see Eq. (12). Here the unitality of the quantum channel appears already on a microscopic level for every electronphonon collision event. The scenario (ii) realizes, for example, for an electron interacting with the random ensemble of 3D nuclear spins, so that the vanishing of the averaged commutators occurred at the macrolevel in the thermodynamic limit of the large spin ensemble. Importantly, the above formulation of the Htheorem applies also to a situation where vanishing of the weighted commutators occurs only within certain energy range and does not hold for the arbitrary energies of the system. For example, in case of the electronphonon interaction the dynamics of an electron can be described by the unital channel only at high electron energies exceeding the Debye energy, see below.
The obtained formulation of the quantum Htheorem enables us to reveal a fundamental difference in how the second law of thermodynamics manifests itself in quantum and classical physics. In classical thermodynamics the energyisolated system inevitably evolves with nondiminishing entropy. We find that in quantum physics the situation is different. To demonstrate that, we construct an energyisolated quantum system for which and which thus evolves with the negative entropy gain. Let us consider a charged particle moving in a threelead conductor and interacting with the spin via the induced magnetic field, see Fig. 1, and, according to our general framework, initially disentangled from the spin. In the absence of the external magnetic field the energy exchange is absent and the particle is energyisolated. The joint scattering states of the particle and spin have the form
where is the particle’s incoming/outgoing state in the lead α, s_{βα} are the components of the scattering matrix of the three lead set up, σ_{0}〉 is the initial state of the spin and is the unitary spin1/2 rotation of the spin due to outgoing (incoming) electron in the lead α. Then the operators of Eq. (3) are defined as .
Let us recall now that rotations of a spin about different axis in general do not commute. We choose spin1/2 rotations as , and , where and are the Pauli matrices, so that . Accordingly, , and the resulting quantum channel is nonunital. The explicit calculation gives (for details of derivation Supplementary Section S3)
Let the initial state of the spin be a pure state , so that all the in the Eq. (5) are equal to 1/3. Hence all offdiagonal elements of appear finite. Taking all s = 2/3, at some energy E_{0}, we construct the normalized initial state of the particle as , with f(E) being the normalized to unity distribution function centered around E = 0 and rapidly decaying as E → ∞, and obtain ΔS ≈ −0.05k_{B}. We thus demonstrated that even the energy isolation does not guarantee the evolution with the nondiminishing entropy. Note that in the discussed example the reservoir acts as some quantum analogue of the classical Maxwell demon. Namely, having been prepared in a special state, the reservoir is able to decrease the entropy of the system without the energy exchange with it, and can be referred to as a ‘quantum Maxwell demon’ discussed in ref. 14 in the context of the work extraction in nanodevices. An extension of the Second Law, accounting for the classical correlation between the system and an information reservoir, i.e. classical Maxwell demon, has recently been considered in refs 15 and 16. In what was discussed above, an electron interaction with the quantum spin does not induce any correlations between the electron and the spin and, therefore, no classical correlations are present. Hence an important distinction between how do quantum and classical Maxwell’s demons operate.
Elastic scattering
As a first example of a system satisfying quantum Htheorem, we consider an electron elastically scattered by the onedimensional (1D) potential barrier, see Fig. 2. Let the electron reflection be accompanied by the change of the reservoir state (e.g. let the reflection to imply emission of the low energy photon via braking radiation, or scattering of the photon), see Fig. 2b, and the electron transmission to retain the state of the reservoir, see Fig. 2a. Accordingly, the joint scattering states of the particle with the fixed energy assume the form,
where indices {L, R} denote the incident (scattered) states in the left and right leads, respectively, n〉 is the initial reservoir state, and n′〉 and n″〉 are the reservoir states resulting from the backscattering to the left and to the right, respectively. The unitality of the corresponding channel follows now from general Eq. (3). However, for illustrative purpose we derive unitality straightforwardly using the explicit form of Eqs (6) and (7) (for details please see Supplementary Section S4). Namely, calculating in the basis of left and right scattering channels, i, j ∈ {L, R}, we obtain
and taking into account the unitarity of the overall transformation, we arrive at . Since this condition holds for any E, then for any state the system evolves with . The above consideration with some minor modifications holds for the grand system where the role of the reservoir is taken up by a single spin located near the scatterer. Then the spin remains intact if the particle is reflected and is rotated by the magnetic field induced by the transmitted particle.
Let us generalize the above consideration onto the particle propagating along the twodimensional array of scatterers and spins (comprising the reservoir) located in the xyplane. The magnetic field induced by the propagating particle is perpendicular to the plane, and all spins experience the commuting unitary rotations around the perpendicular zaxis. All the rotations commute, hence the condition of the quantum Htheorem is satisfied and .
Remarkably, the property of unitality of the grand system with the spin reservoir preserves in the 3D case. As we mentioned above, the rotations experienced by an individual spin may appear, in general, noncommuting. Note, however, that operators in Eq. (3) acquire the form
where is a unitary rotation of a spin a by the electron experienced a scattering process from the state i〉 to the state j〉. Then
where is the total number of spins. For most of the spins, the factors that appear upon averaging Eq. (10) are small, . We arrive at the estimate
therefore, as N → ∞. We see that in the macroscopic limit of the number of spins, the averaged commutators appearing in the condition for the Htheorem vanish in spite of the fact that the commutators for the individual spins could remain finite. Thus the evolution of the considered 3D system occurs with .
To proceed further, we note, that if one can find a basis in the reservoir Hilbert space where all operators are diagonal, then the operators commute. Below we present two generic physical examples where this basis can be found explicitly: (i) an electron interacting with adiabatic twolevel impurities and (ii) electronphonon interaction in solids.
Scattering on twolevel systems
Consider the electron scattering on impurities that fluctuate between two positions with nearly equal energies. To be concrete we focus on the random walk of the electron along the ensemble of TLS (see the description of the similar systems in refs 17 and 18) as shown in Fig. 3. Assume for simplicity that (i) the dynamics of a TLS is slow hence its state does not change during the interaction with the electron and that (ii) each TLS which is in the state ↑〉 (↓〉), scatters the electron via elastic unitary matrix . Then the global unitary transformation is given by where describes the scattering on the nth impurity. Denote the scattering state of the electron moving in a direction k by k〉. Then the reservoir operator with , see Eq. (2), commute with each other and, therefore, the second term in Eq. (3) vanishes. Hence, in each particular scattering event the entropy of the particle is nondiminishing.
The question that now arises is whether the nondiminishing entropy maintains for the sequence of scatterings. Recall that in order for the entropy to grow monotonously, an electron should be disentangled from the TLS with which it is going to interact. Since in the course of the evolution an electron may return to the TLS on which it have scattered and, with which, therefore, it could have been getting entangled in the past, these returns would violate this ‘initial nonentanglement condition.’ Thus to guarantee the evolution with nondiminishing entropy the TLS should have interacted with some other degrees of freedom that would lead to the memory loss of this TLS prior to the possible return of the electron. This memory loss is the manifestation of the socalled monogamy of entanglement^{19} which is a specific property of the entanglement distribution between quantum systems: if a TLS is already entangled with an electron and later it becomes entangled with another degree of freedom then the initial entanglement with the electron vanishes. Thus the process of sequential scattering of an electron satisfies the Htheorem if the typical entanglement time for the TLS is less than the typical return time of an electron to the particular TLS.
The interaction of a quantum system with a memoryless environment can be described by Markovian (or equivalently Lindblad) master equation^{20}. The system’s dynamics governed by Lindblad master equation can be described within the so called collision model^{21} where a quantum system (electron) interacts locally in time with the different environmental degrees of freedom or subenvironments. In a situation, where different subenvironments are initially uncorrelated and the system interacts with the given subenvironment at most once, the resulting quantum channel possesses a divisibility property: , where Φ_{i} is a quantum channel corresponding to the scattering on ith TLS followed by a free unitary evolution. In a more realistic situation, the TLSs may retain the partial entanglement with the electron that induces finite time memory effects in the environment. In this situation while the quantum channel is not divisible and hence cannot be described by the Lindblad master equation any more, it still can be described within in the collision model framework^{22,23,24}. This may result, in general, in a nonmonotonic entropy evolution. This issue requires a separate study and will be a topic of a forthcoming work.
Electronphonon interaction
Now we demonstrate that the electronphonon interaction leads to the electron evolution which satisfies the conditions of the quantum Htheorem. In a standard electronphonon interaction model, a representative test electron ‘sees’ a screened shortrange ionic potential. Since the resulting scattering time is short and the ion is much heavier than the electron, the position of a given ion remains nearly unchanged during the interaction with the electron, see Fig. 4. Then the standard consideration of the electronphonon interaction^{25} results in a conclusion that at high temperatures where the typical energy of an electron is relatively high (i.e. it exceeds the Debye energy, the maximal energy of phonons), the electronphonon collisions are quasielastic. This allows us to apply the same arguments as for the model of an electron interacting with twolevel impurities considered above. Indeed, the slow iondynamics preserves the classical distribution function, ρ_{ion}({r}), for the ions positions {r} = {r_{1}, r_{2}, …} and hence the induced operators are diagonal in the ion coordinate basis,
where s_{ji}({r}) are electron scattering matrix on the potential defined by the ions positions {r}. Therefore the conditions of the quantum Htheorem hold for electrons with energies exceeding the Debye energy. The initial disentanglement of the electron from the ionic reservoir is ensured either by the fact that a given ion did not participate in the previous collisions with the electron, or has already ‘forgotten’ about such an event due to the monogamy of entanglement.
It is noteworthy that unlike the other systems discussed in previous sections, the evolution of the electronphonon system does not occur in the unital channel. Nevertheless, it satisfies the condition of the Htheorem thus illustrating a mathematical result establishing that for some classes of initial states even the evolution defined by nonunital channels may occur with the nondiminishing entropy^{11}. The technical details and additional examples are given in the supplementary information.
Additional Information
How to cite this article: Lesovik, G. B. et al. Htheorem in quantum physics. Sci. Rep. 6, 32815; doi: 10.1038/srep32815 (2016).
References
 1.
Boltzmann, L. Weitere Studien über das Wärmegleichgewicht unter Gasmolekülen. Wiener Berichte 75, 62–100 (1872).
 2.
Boltzmann, L. Entgegnung auf die wärmetheoretischen Betrachtungen des Hrn. E. Zermelo. Annalen der Physik (Leipzig) 57, 773–784 (1896) [Translated and reprinted in S. G. Brush, Kinetic Theory 2, Pergamon Elmsford, New York (1966)].
 3.
Lebowitz, J. L. Statistical mechanics: A selective review of two central issues. Rev. Mod. Phys. 71, S346–S357 (1999).
 4.
Von Neuman, J. Beweis des Ergodensatzes und des HTheorems in der neuen Mechanik. Zeitschrift für Physik 57, 30–70 (1929) [Von Neumann, J., Proof of the ergodic theorem and the Htheorem in quantum mechanics. Eur. Phys. J. H 35, 201–237 (2010)].
 5.
Gemmer, J., Michel, M. & Mahler, G. Quantum thermodynamics. Springer (2009).
 6.
Nielsen, M. A. & Chuang, I. L. Quantum computation and quantum information. Cambridge Univ. Press (2011).
 7.
Holevo, A. S. Quantum systems, channels, information. A mathematical introduction. De Gryter (2012).
 8.
Holevo, A. S. The entropy gain of infinitedimensional quantum channels. Doklady Math. 82, 730–731 (2010).
 9.
Lindblad., G. Completely positive maps and entropy inequalities. Comm. Math. Phys. 40, 147 (1975).
 10.
Wehrl, A. General properties of entropy. Rev. Mod. Phys. 50, 221–260 (1978).
 11.
Amosov, G. G. Estimating the output entropy of a tensor product of two quantum channels. Theor. Math. Phys. 182, 397–406 (2015).
 12.
Argentieri, G., Benatti, F., Floreanini, R. & Pezzutto, M. Violations of the second law of thermodynamics by a non completely positive dynamics. Europhys. Lett. 107, 50007 (2014).
 13.
Lesovik, G. B. On the law of increasing entropy and the cause of the dynamics irreversibility of quantum systems. JETP Lett. 98, 184–189 (2013).
 14.
Lloyd, S. Quantummechanical Maxwell’s demon. Phys. Rev. A 56, 3374 (1997).
 15.
Deffner, S. & Jarzynski, C. Information Processing and the Second Law of Thermodynamics: An Inclusive, Hamiltonian Approach. Phys. Rev. X 3, 041003 (2013).
 16.
Horowitz, J. M. & Esposito, M. Thermodynamics with Continuous Information Flow. Phys. Rev. X 4, 031015 (2014).
 17.
Aharonov, Y., Davidovich, L. & Zagury, N. Quantum random walks. Phys. Rev. A 48, 1687 (1993).
 18.
Childs, A. M., Farhi, E. & Gutmann, S. An example of the difference between quantum and classical random walks. Quant. Inf. Proc. 1, 35 (2002).
 19.
Coffman, V., Kundu, J. & Wootters, W. K. Distributed entanglement. Phys. Rev. A 61, 052306 (2000).
 20.
Lindblad, G. On the generators of quantum dynamical semigroups. Comm. Math. Phys. 48, 119 (1976).
 21.
Ziman, M. et al. Diluting quantum information: An analysis of information transfer in systemreservoir interactions. Phys. Rev. A 65, 042105 (2002).
 22.
Rybár, T., Filippov, S. N., Ziman, M. & Buzek, V. Simulation of indivisible qubit channels in collision models. J. Phys. B 45, 154006 (2012).
 23.
Ciccarello, F., Palma, G. M. & Giovannetti, V. Collisionmodelbased approach to nonMarkovian quantum dynamics. Phys. Rev. A 87, 040103 (2013).
 24.
Caruso, F., Giovannetti, V., Lupo, C. & Mancini, S. Quantum channels and memory effects, Rev. Mod. Phys. 86, 1203 (2014).
 25.
Pitaevskii, L. P. & Lifshitz, E. M. Physical Kinetics. ButterworthHeinenann (1981).
Acknowledgements
We are delighted to thank G. Blatter, G.M. Graf, M. McBreen, L. B. Ioffe and G. G. Amosov for illuminating discussions. The work was supported by the RFBR Grant No. 140201287 (G.B.L.), by the Pauli Center for Theoretical Studies at ETH Zurich (G.B.L.), by the US Department of Energy, Office of Science, Materials Sciences and Engineering Division (I.A.S. and V.M.V.), and by the Swiss National Foundation through the NCCR QSIT (A.V.L.).
Author information
Affiliations
L.D. Landau Institute for Theoretical Physics RAS, Akad. Semenova av., 1A, Chernogolovka, 142432, Moscow Region, Russia
 G. B. Lesovik
Theoretische Physik, WolfgangPauliStrasse 27, ETH Zürich, CH8093 Zürich, Switzerland
 G. B. Lesovik
 & A. V. Lebedev
Materials Science Division, Argonne National Laboratory, 9700 S. Cass Avenue, Argonne, Illinois 60637, USA
 I. A. Sadovskyy
 & V. M. Vinokur
Moscow Institute of Physics and Technology, Institutskii per. 9, Dolgoprudny, 141700, Moscow District, Russia
 M. V. Suslov
Authors
Search for G. B. Lesovik in:
Search for A. V. Lebedev in:
Search for I. A. Sadovskyy in:
Search for M. V. Suslov in:
Search for V. M. Vinokur in:
Contributions
All authors have contributed to essential portions of this work. The original idea was due to G.B.L. the work was conceived by G.B.L. and V.M.V. I.A.S. performed numerical simulations. All authors carried out analytical calculations, discussed the results, and contributed to the writing of the manuscript.
Competing interests
The authors declare no competing financial interests.
Corresponding author
Correspondence to V. M. Vinokur.
Supplementary information
PDF files
Rights and permissions
This work is licensed under a Creative Commons Attribution 4.0 International License. The images or other third party material in this article are included in the article’s Creative Commons license, unless indicated otherwise in the credit line; if the material is not included under the Creative Commons license, users will need to obtain permission from the license holder to reproduce the material. To view a copy of this license, visit http://creativecommons.org/licenses/by/4.0/
About this article
Further reading

Quantum Landauer erasure with a molecular nanomagnet
Nature Physics (2018)

Entropy Dynamics in the System of Interacting Qubits
Journal of Russian Laser Research (2018)
Comments
By submitting a comment you agree to abide by our Terms and Community Guidelines. If you find something abusive or that does not comply with our terms or guidelines please flag it as inappropriate.