Minimal evolution time and quantum speed limit of non-Markovian open systems.

We derive a sharp bound as the quantum speed limit (QSL) for the minimal evolution time of quantum open systems in the non-Markovian strong-coupling regime with initial mixed states by considering the effects of both renormalized Hamiltonian and dissipator. For a non-Markovian quantum open system, the possible evolution time between two arbitrary states is not unique, among the set of which we find that the minimal one and its QSL can decrease more steeply by adjusting the coupling strength of the dissipator, which thus provides potential improvements of efficiency in many quantum physics and quantum information areas.

As a fundamental bound for the evolution time of quantum systems, the quantum speed limit (QSL) (also referred to as quantum evolution time limit) plays an important role in tremendous areas of quantum physics and quantum information, such as quantum computation and communication12, quantum metrology3, cavity quantum electrodynamics4, quantum control5, etc. The derivation of QSL is most required for the purpose of simplification and/or optimization in theoretical analysis, since in most quantum-cases one only needs to derive a lower bound on the minimal time of evolution without solving the exact equation to see the dominant factors in evolution and/or optimize our demand. For closed quantum systems, two types of QSL have been derived at the start: the Mandelstam-Tamm (MT) bound 6 and the Margolus-Levitin (ML) bound 7. Since then, further investigations are launched into QSL89101112. As the energy of a closed system is conserved, the QSL of a closed system is decided by the variance of energy ΔE or the mean energy , related only to the unitary Hamiltonian. Recently, the QSL for quantum open systems13 draws wide attention with several bounds1415161718 being found. Because there is energy and/or coherence exchange between system and environment for quantum open systems, the evolution generator therein contains not only a time-dependent Hamiltonian H but also a dissipator (a trace-preserving term referring to dissipation behaviors)13. In quantum open systems, non-Markovianity is valuable in practice and highly emphasized for its particular characteristics of memory effect, negative energy/population flow and singularity of the state evolution1920. The latter two characteristics are commonly found in the strong-coupling regime, where the system and environment are strongly coupled and the non-Markovianity becomes a non-negligible strong effect21. Typically, a strong-coupling regime can be achieved and temporarily maintained in high-Q optical micro-cavities22 and quantum circuits23. In spite of recent breakthrough on measurement methods for non-Markovianity2425262728, the strong-coupling regime still remains as an open question. Also, QSL issue becomes more complicated than it was considered16, since in such a regime the possible evolution time between two arbitrary states is not unique, while only the QSL for the minimal one does matter. In addition to non-Markovianity, the evolution of mixed states in quantum open systems also attracts concern. It is therefore of great significance to derive a sharp bound on evolution time for general conditions, i.e., for mixed states in different non-Markovian coupling regimes.

In this report, we study the non-Markovian problem by using geometric methods and derive a sharp bound for the minimal evolution time for quantum open systems with initial mixed states. We define the minimal evolution time for non-Markovian quantum open systems as the minimal possible evolution time between two arbitrary states before we study its relevant QSL using new mathematical inequality tools. A steeper decrease of QSL than previous result16 caused by strong non-Markovianity is observed in the examples of two-level models, indicating that a much smaller evolution time can be achieved in the strong-coupling regime. It is implied that the evolution of quantum physical process and computation involving strong-coupling interactions can be more effective.

Results

Geometric fidelity

To quantify the geometric distance between two general quantum states, the Bures fidelity29 with the Bures angle was usually used, where ρ is the density operator of a general quantum state. Here, however, we introduce the relative-purity fidelity with . This one derived from the so-called relative purity30 is more useful in studying QSL31. It is easy to prove that , and, if ρ2 is a pure state, then one has .

From the von Neumann trace inequality32,

Hence, we have and is valid. In addition, compared with another recently used fidelity18 , can guarantee a perfect and simple linear relationship (as we shall see later) at the expense of good symmetry between ρ1 and ρ2.

Minimal evolution time

The minimal evolution time of a quantum evolution is defined in the following: given a predefined quantum evolution , then, a predetermined state ρ, one has , where stands for the set of all the actual possible driving time τ that the evolution from ρ0 to ρ may take. One should notice that τ is not unique, especially in the non-Markovian strong-coupling regime.

Quantum speed limit

In order to derive a lower bound as the QSL for driving time τ, the square of the relative-purity fidelity

is used, which is simply linear with ρ. The same linear relationship for is not true unless ρ0 is a pure state. Taking time derivatives of yields

The dynamical map of a general quantum system reads 13, where the renormalized Hamiltonian contains a time-dependent Lamb shift term . For a Markovian system, the super-operator takes a Lindblad form and is time-independent, hence , where obeys the adjoint master equation15. However, this is invalid for a non-Markovian system13. To derive the lower bound for a non-Markovian case, we divide into two parts using the triangle inequality

The absolute trace inequality32 reads . Since , one has

As H and ρ are both positive (by shifting the ground energy of H) and Hermitian operators, we take the commutator inequality33, i.e., , where and N is the rank of the operator. For convenience, we denote . It is worth noting that this inequality is sharp, e.g., if and , then and . Since , for simplicity we have . Substituting it into Eq. (1) and integrating t from 0 to τ then yield

where . It is manifested that Eq. (2) is determined by both the renormalized Hamiltonian H (system) and the dissipator (environment). Also, this bound can reduce to the previous result16 when ρ0 is a pure state and .

Non-Markovianity

To investigate the minimal evolution time in more detail, we use the damped Jaynes-Cummings model as an example, which describes the coupling between a two-level system and a single cavity mode with the background of cavity-QED13. Within a resonant Lorentzian spectral density of environment that , the exact Hamiltonians read13

where ħω0 is the energy difference and are Pauli operators. The exact dissipator reads

with , in which λ is the spectral width, γ0 the coupling strength, and . When γ0 < λ/2, the system and environment are weakly coupled and evolve subexponentially; the degree of non-Markovianity 24. When γ0 > λ/2, D is real; the system and environment are strongly coupled with oscillatory characteristics13 and (see Fig. 2). The initial environment is chosen to be a vacuum state and the initial system fully excited to make the model simpler. Consequently, we only need to consider the dissipator , for the exact solution13 implies ρ a diagonal operator so that in Eq. (1). It is useful to introduce a special minimal evolution time , , i.e., is the minimal evolution time for the maximum of Θ. It is worth noting that depends strongly on different coupling regimes (see Fig. 1): in the weak-coupling regime, we have , but in the strong-coupling case, is finite, which is caused by the oscillatory characteristics of the population. Like , it is worth noting for itself that it will be smaller in the strong-coupling regime than that in the weak-coupling regime16. Although is equal to the only possible driving time when it is weakly coupled, it is not the case for the strong-coupling regime. From numerical solution of we find that has a first derivative singular point at and a steep decrease in the strong-coupling regime, which cannot be implied from (see Fig. 2). A decrease of the QSL for was also suggested in the previous result16, but the decreasing slope with γ0 deviates from the minimal evolution time as shown in Fig. 2.

Figure 2

Minimal evolution time (red solid line) of the same model and its different QSL bounds (black lines) as a function of γ0.

The bounds are derived from the previous result16 (dotted), Eq. (4) (solid), and Eq. (5) (dashed). Also indicated here is the degree of non-Markovianity24 (blue solid line). We set λ = 1 and τ = 10.

Figure 1

Solutions of the population of the damped Jaynes-Cummings model13 in the weak- (black line) and strong-coupling regime (red line), with γ0 = 0.4 and γ0 = 10, respectively, and λ = 1 for both.

is when the maximum of geometric distance is reached ().

As the energy of an open system is not conserved, the average of the dissipator decreases with time and ; as a result, we have since . depends on the short duration from 0 to at most, so we can simply replace the time average by the maximum and eliminate the subscript ,

Substituting Eq. (3) into Eq. (2), the final bound for yields

which is valid for general quantum systems, regardless of whether they are closed or open and how strong the coupling is. It is found that the QSL Eq. (4) in the strong-coupling regime has a fitting decreasing slope as shown in Fig. 2. However, this bound is not asymptotic when . To derive a sharper QSL, we notice that Eq. (3) can take an approximation,

where the parameter β introduced as a metric of the time average rests upon specific models, and the rough bound of Eq. (3) can also be treated as β = 1. For this case, we consider that in the strong-coupling regime when ,

The first-order approximation yields , since . The exact solution of yields . Here is the chronological super-operator which orders the t′ arguments to increase from right to left34. Hence,

where . Generally speaking, for a continuous evolution, strong coupling between the system and environment certainly involves a non-Markovian bidirectional flow of energy and/or coherence, which can always be characterized as oscillator(s). Therefore, a general form like Eq. (6) can provide a reasonable approximation of oscillation for other models.

It is found that the parameter β depends typically on the relation between and in the strong-coupling limit. With different (when ), the time average in the left term of Eq. (5) will take a different time period, and β thus changes in the range from 0 to 1. In this case of the damped Jaynes-Cummings model, we have as , suggesting that the time average in Eq. (5) should take nearly a π/2 period. Taking Eq. (6) into Eq. (5) immediately indicates β = 2/π then. From Fig. 2, it is clear that this bound is sharp, but is not valid when it comes into the weak-coupling regime since the approximation is invalid there.

Renormalized Hamiltonian

To verify our result and manifest the influence of the renormalized Hamiltonian term in Eq. (2), we introduce another two-level system containing a two-band environment as the second example. This model can simulate the interaction between a spin and a single-particle quantum dot3536, of which the total Hamiltonian is H = H0 + V where with σ the Pauli operator. The lower energy band contains N1 levels and the upper N2 levels, with the same band width δε and the inter-bands distance ΔE in resonance with the spin. V represents the interaction that , with λ the coupling coefficient and c(n1, n2) complex Gaussian random variables. At the beginning, we numerically solve the model concerning the minimal evolution time problem and identify the same singularity at λ ≈ 0.0072 and steep decrease when λ > 0.0072 like those shown in Fig. 2. To demonstrate the influence of renormalized Hamiltonian, first we set with a driving time τ = 8.0, from which one derives Θ ≈ 0.7707 and (see Fig. 3(a,b)). As , 1 now35. It is recalculated from Eq. (5) that . Further calculation shows that the previous QSL16 is too large, while Eqs. (3) and (5) indicate and . Both of them stay valid while the latter is sharp. Second, we set ΔE = 10ħ, and τ = 8.0, from which one derives ΘR ≈ 0.7832 and (see Fig. 3(c,d)). Since ρ0 is not diagonal, and should be considered. Further calculation shows that the previous QSL16 is too large, while and . The mere difference between and implies that the renormalized Hamiltonian H is dominant in Eq. (4). As added, becomes smaller, which apparently follows the time-energy uncertainty relation.

Figure 3

Numerical solution of the relative-purity fidelity (red lines) and the dissipator (blue lines) of the quantum dot model35.

λ = 0.02 which represents the strong-coupling regime, with N1 = N2 = 500 and δε = 0.5ħ. The initial states are (a), (b): and (c), (d): , respectively.

Discussion

Only Hamiltonian was considered in some of previous investigations6789101112, while for an open system, the coupling strength of its dissipator also has an influence on QSL1516. However, it is demonstrated in our study that in non-Markovian case such influence could be more significant than it was thought. Therefore, to achieve a high speed of evolution5, it is more probable that we only focus on improving the coupling interaction instead of increasing the energy. This implies that the power consumption can stay a low level for cavity-QED process while high efficiency can still be achieved. Previously it was always thought that a strong coupling with environment should be prevented due to its enhanced decoherence effect on qubits. However, as a trade-off, the operation time for transforming and/or erasing qubits for example can also be remarkably reduced in the strong-coupling regime. It is thus possible to make quantum computation more feasible and achievable by adjusting the coupling strength in a well-chosen pattern.

In summary, we derive a sharp bound as the quantum speed limit of open systems available for mixed initial states. Considering the non-Markovian feature, we find that the minimal evolution time of the two two-level examples considered here has singularity nearly at the cross-point of regimes and a steep decrease in the strong-coupling regime. This result may lead to high-efficiency quantum information research and engineering. As the time-energy uncertainty relation dictates, renormalized Hamiltonian will also contribute to the final quantum speed limit bound as manifested in the quantum dot model in detail. We expect our result to be used for quantum time analysis and optimal control, as well as in pertinent topics on general physics.

Methods

Norms of operators

A general Schatten p-norm of an operator A is , where singular values are the eigenvalues of , and , and as the operator norm, trace norm and Hilbert-Schmidt norm of A, respectively37.

Approximation for the dissipator of the damped Jaynes-Cummings model in the strong-coupling regime

With

given13, the exact solution of yields

We have in the strong-coupling regime. As a result,

which yields the result of Eq. (6). In this case, we also have as γ0 increases, which implies that the time average in Eq. (5) takes nearly a π/2 period. Taking Eq. (6) into Eq. (5) then indicates β = 2/π.

Additional Information

How to cite this article: Meng, X. et al. Minimal evolution time and quantum speed limit of non-Markovian open systems. Sci. Rep. 5, 16357; doi: 10.1038/srep16357 (2015).