Abstract
Revivals of quantum correlations in composite open quantum systems are a useful dynamical feature against detrimental effects of the environment. Their occurrence is attributed to flows of quantum information back and forth from systems to quantum environments. However, revivals also show up in models where the environment is classical, thus unable to store quantum correlations, and forbids systemenvironment backaction. This phenomenon opens basic issues about its interpretation involving the role of classical environments, memory effects, collective effects and systemenvironment correlations. Moreover, an experimental realization of backactionfree quantum revivals has applicative relevance as it leads to recover quantum resources without resorting to more demanding structured environments and correction procedures. Here we introduce a simple twoqubit model suitable to address these issues. We then report an alloptical experiment which simulates the model and permits us to recover and control, against decoherence, quantum correlations without backaction. We finally give an interpretation of the phenomenon by establishing the roles of the involved parties.
Introduction
In a multipartite quantum system one can identify different kinds of quantum correlations (such as entanglement and genuine quantum correlations), each with characteristics useful as resources for quantum information processing^{1,2}. The exploitation of these quantum correlation resources is however jeopardized by the detrimental effects of the environment surrounding the quantum system. Quantum correlations between noninteracting qubits in independent environments have been shown to decay asymptotically^{2,3} or even to disappear at a finite time^{4,5} under the action of Markovian noise. NonMarkovian noise, like that arising from structured environments or from strong couplings, has instead been shown to lead, during the evolution, to revivals of quantum correlations^{4,6,7}, permitting their partial recovery and thus an extension of their exploitation.
Revivals of quantum correlations, initially present in a quantum system, have been explained in terms of repeated correlation exchanges between the qubits and their nonMarkovian quantum environments because of the backaction from the environments to the qubits^{4,6,8,9,10,11}. Recently, it has been shown that revivals of quantum correlations may also occur when the environment is classical^{2,12,13,14,15,16} and it does not back react on the quantum system. Moreover, in such a case, the environment cannot either store or share the quantum correlations initially present in the quantum system. It thus appears that for revivals to occur it is not essential to have a nonMarkovian quantum environment with backaction. This fact however leads to basic issues about the interpretation of backactionfree quantum revivals. In particular, it is essential to establish: (1) the role of the classical environment in reviving both entanglement and purely quantum correlations, for instance if it may act as a control system for what operation is applied to the qubits; (2) the role of collective effects of the environment on the qubits; (3) the role of the memory effects; (4) the role of possible system–environment correlations.
In order to address these issues and explain the mechanisms underlying the revivals without backaction, we consider a simple model that excludes the presence of collective effects of the environment on the qubits and also takes into account decoherence on the qubit evolution, so to be in a realistic scenario. We also require that the model present a system dynamics where the correlations are analytically measurable by known quantifiers, and moreover, it is realizable by a neat experimental setup that avoids any side effects that can affect the expected system dynamics and complicate the interpretation. Here we introduce a model of two noninteracting qubits, initially entangled, where only one qubit is subject to a random external classical field with inhomogeneous broadening in its amplitude. This model satisfies the above requirements. We then report the results of an alloptical experiment that simulates this model, with a random classical field mimicked by quantum degrees of freedom, and allows us to observe and control revivals of twoqubit quantum correlations without systemenvironment backaction. Moreover, we show a direct connection between the occurrence of the revivals and the intrinsic nonMarkovianity (not due to a quantum environment) of the system evolution. Finally, we give an interpretation of the phenomenon showing the role of the classical environment in reviving quantum correlations.
Results
Theoretical model
We consider a system of two noninteracting initially entangled qubits, namely a and b, where the qubit a is isolated while the qubit b resonantly interacts with a random external classical field, whose phase is either ϕ_{+}=+π/2 or ϕ_{−}=−π/2 with equal probability 1/2 and whose amplitude has a Gaussian distribution. This model is illustrated in Fig. 1a. The interaction Hamiltonian between the qubit b and a classical field E with phase ϕ, in the rotating frame at the qubitfield frequency, is H=iħ(Ω/2)(σ_{+}e^{−iϕ}−σ_{−}e^{iϕ}) where the coupling constant (Rabi frequency) Ω is proportional to the field amplitude and σ_{±} are the raising and lowering operators in the basis {0〉,1〉}. The time evolution operator U(t)=e^{−iHt/ħ} has the matrix form^{15}
Due to the randomness of the field phase acting on the qubit b and being the qubit a isolated, the global dynamical map of the model of Fig. 1a is , where is the initial twoqubit state. A relevant property of this map is that it moves inside the class of Belldiagonal states (that is, mixtures of the four Bell states), for which analytic expressions of the most used quantifiers of correlations are known^{2,17,18}. Therefore, we shall choose special Belldiagonal states as initial states of the system. At this stage the evolution is cyclic and does not exhibit decoherence. In order to introduce decoherence in the system evolution, we consider the field suffering a noise source due to signal inhomogeneous broadening whose effect is to induce a Gaussian distribution in the field amplitude and thus in the Rabi oscillation frequency Ω of the qubit evolution, that is where Ω_{0} and σ are the central Rabi frequency and the Rabi frequency width, respectively. The effect of noise is therefore transferred to the intrinsic evolution of the quantum system. The final evolved state is obtained by tracing out the Rabi frequency degree of freedom from .
Experimental setup
The experimental setup simulating the model introduced above is displayed in Fig. 1b. The quantum system is given by two polarized photons, each one being a qubit with basis states H〉 (horizontal polarization) and V〉 (vertical polarization). The preparation part of the setup is able to generate polarizationentangled photon pairs in a given Belldiagonal state . The photon in mode a is directly sent to the state tomography part whereas the photon in mode b is directed to the environment part and successively to the state tomography part.
The environment is given both by the two photon paths separated by a beamsplitter, the reflected path p_{+} and the transmitted path p_{−}, and by the measurement process that traces over the time difference between the two paths themselves, creating a statistical mixture of them with equal probabilities (1/2). The effect of the two paths is to make the photon basis states H〉, V〉 undergo, apart from an unimportant global phase factor, the unitary transformations (see second section of Methods)
where =ωτ is the phase difference between H〉 and V〉 introduced by the SoleilBabinet compensator (SBC) and the quartz plates (QPs). ω is the photon frequency and τ ≡ LΔn/c is the time difference to cross the optical element (SBC or QP), with L being the thickness of the optical element, c the vacuum speed of light, Δn the difference between the indices of refraction of the horizontal and vertical polarizations. The action of each path in equation (2) corresponds to a rotation {U}_{{\text{p}}_{\pm}}() of the basis states {H〉,V〉} of b. The two paths p_{±} of equation (2) act on the photon b exactly as the two time evolution operators (t) of equation (1), respectively, with the correspondences 0〉 ↔ H〉, 1〉 ↔ V〉 and =ωτ ↔ Ωt (which implies Ω ↔ ω). The environment part of the setup simulates the random phase of the field acting on qubit b (random dephaser) by the action of the beamsplitter that separates the two photon paths, corresponding to the effect of the field with either phase, plus the measurement process that does not distinguish the two paths p_{±}. This mimics the random external field acting on qubit b, giving the overall output state . Up to now we have considered a photon with frequency ω. In fact, in our experiment the photon has an intrinsic Gaussian frequency distribution (ref. 19), where ω_{0} is the center frequency and σ the frequency width. This frequency degree of freedom introduces decoherence by a decoherence parameter κ=∫f(ω)cos[(ω)]dω=cos(ω_{0}τ)exp(−σ^{2}τ^{2}/16) (ref. 3). This decoherence source is of the same kind as that due to the Rabi frequency distribution in the model introduced above. The effective evolved state is then obtained by tracing out the photon frequency degree of freedom from .
We prepare initial Bell diagonal states of the form (see first section of Methods)
where λ_{+}+λ_{−}=1 and . λ_{+} is arbitrarily determined by the relative power between the two pump paths created by the Wollaston prism. As a consequence, the twophoton output state is the Belldiagonal state (see second section of Methods)
where . When L is small so that (exp(−σ^{2}τ^{2}/16) ≈1), the decoherence parameter becomes κ≈ cos(=ω_{0}τ) and we have a cyclic and thus coherent evolution: this is the case when only the SBC, that allows us to adjust small lengths, is used. When the QPs are used the decoherent evolution comes out.
Experimental dynamics of correlations
We investigate the dynamics of the various kinds of correlations present in the twoqubit system. We quantify the total correlations by the quantum mutual information^{2} and the entanglement by concurrence^{1} , where Γ is a function of . Quantum correlations are instead quantified by the quantum discord^{2} , where indicates the classical correlations (see third section of Methods).
The results for the coherent evolution, realized by the SBC device with the QPs removed, are plotted as a function of the relative phase =ω_{0}τ in Fig. 2a, starting from with λ_{+}=0.9. Total correlations oscillate with period π. Plateaus and sudden changes in the dynamics of classical and quantum correlations occur several times, showing their robustness against variations of the relative phase. Quantum correlations revive after vanishing at about π/2 and 3π/2 (in a 2π period). Entanglement exhibits dark periods around the same points and then revives.
In Fig. 2b, we further show the experimental results for the decoherent evolution, where both SBC and QPs are used. We plot the envelope dynamics of correlations as a function of the QP length L for the same initial state with λ_{+}=0.9, by measuring the maximum amplitudes of revival of the quantifiers. A sudden change in behaviour in the dynamics of the maximum values of classical and quantum correlations is found when L≈82λ_{0} (λ_{0}=800 nm is the center photon wavelength). The maximum of entanglement revivals decreases monotonously and completely vanishes at L≈258λ_{0}. The theoretical curves exhibiting these decaying revivals are displayed in the inset of Fig. 2b. The coherent evolution in Fig. 2a is part of the decoherent evolution in Fig. 2b, which is denoted by the red box in Fig. 2b. Although the decay behavior of the maximum values of correlations is similar to that in ref. 3, the internal noise mechanism is completely different. There are no revivals of correlations in the Markovian evolution of ref. 3, whereas here the correlations exhibit collapses and revivals during the evolution in absence of systemenvironment backaction.
Our experimental setup controls λ_{+} and thus the revival amplitude. Figure 3 shows the results for the coherent evolution at a relative phase =π/4 (also applicable at =3π/4 in the region of first revival). It is seen that all correlations are symmetric to the point λ_{+}=0.5, which represents a classical initial state (zero quantum correlations). Interestingly, there is a range of values of λ_{+} ( and ) where quantum correlations remain unchanged at their maximum value, implying that at =3π/4 they cannot take a value larger than that observed in Fig. 2a, for λ_{+}=0.9. This is connected to a peculiar behaviour of the sudden change points of Q. In contrast, the degree of entanglement revival at =3π/4 can be increased with respect to that of Fig. 2a, for example, by increasing λ_{+}.
Connection to nonMarkovianity
The observation of the revivals without backaction in our setup can be connected to the intrinsic nonMarkovianity of the system evolution. In our system, photon b experiences the noisy environment and photon a can be treated as an isolated ancilla. NonMarkovianity then immediately follows from the nonmonotonous behaviour of entanglement evolution obtained starting from the input Bell state (ref. 20), displayed in Fig. 4 for the coherent case. This aspect is emphasized if we consider the nonMarkovianity measure based on the trace distance D(t)^{8}. Any temporary increase of D(t) is a signature of nonMarkovianity that can be identified by the regions where the rate of change σ(t)=dD(t)/dt is positive. For our local map of random external fields, within the coherent case where =ω_{0}τ is the dimensionless time variable, we have^{21} σ()=−sgn(cos)sin where sgn(x) is the sign function (see last section of Methods). We find σ()>0 just when entanglement revivals occur, as displayed in Fig. 4. Interestingly, we also notice that the larger entangling rates of the system correspond to the larger signatures of memory effects (larger values of σ()).
The tracedistance measure indicates the presence of nonMarkovianity when the distinguishability of the pair of states increases with time: this can be simply interpreted as a flow of information from the environment back to the system which enhances the possibility of distinguishing the two states. We however remark that this backflow of information does not necessarily imply backaction and correlation exchange. The presence of systemenvironment backaction means that the system affects its dynamics via the environment. When the environment dynamics is unaffected by the system this backaction on the system cannot occur. This is the case considered in our model and in the corresponding experimental setup.
Interpretation
The connection between the revivals and the intrinsic nonMarkovianity of the system evolution does not by itself provide an explanation of the observed phenomenon but only gives a necessary condition for it to occur. A possible interpretation of the phenomenon of quantum correlation recovery in absence of systemenvironment backaction can be provided when one describes the initial global systemenvironment state of our setup as a quantumclassical state^{15}, where the quantum part is the twophoton system and the classical part is the environment e acting locally on the photon b. The environment can only be in a separable mixture of its basis states that in our setup can be expressed as , where p_{±}〉_{e} are the basis states corresponding to the two random paths (field phases in the theoretical model) of equation (2). By this formalism, we are able to quantify the correlations present in the global quantumclassical system abe. We also show that the environment e and the photon b never become correlated during the evolution and that this aspect however does not jeopardize the role of the classical environment in reviving the quantum correlations initially present in the quantum system.
For the sake of simplicity let us consider the case when decoherence is negligible (analogous argumentations hold even if decoherence is present). The twoqubit output state is obtained by tracing the overall evolved state ρ_{se}() over the environment e, where and is the unitary operation acting on qubit b and its environment e. This way, the same dynamics observed above for ab correlations exhibiting the revivals is retrieved. During the time evolution, due to , the states of the classical environment are invariant, the qubit b does not affect the environment and the backaction by the environment on the qubit is absent. Moreover, a classical environment cannot store any quantum correlations on its own. One could then think that the presence of revivals is due to some correlation established between b and e. The subsystem be evolves under the local unitary operation U_{be} so that the correlations between be are invariant. If one traces ρ_{se}() over the isolated qubit a, it is straightforward to show that the qubit b and its environment e never become quantum correlated. For example, for an initial Belldiagonal state between a–b like that of equation (3), it results that the reduced state of b–e during the evolution is the uncorrelated state . Therefore, the qubit–environment correlations do not have any role in the occurrence of the phenomenon under investigation.
From the structure of U_{be} it is clear that the environment only has the role of a control system for what unitary operation is applied to the qubit b. By memory effects, the environment e keeps a classical record of what unitary operation has been applied to the qubit b and this happens even without backaction. It is the lack of this classical information that makes quantum correlations disappear at a given time and it is the recovery of this information that makes quantum correlations then revive. The information the environment holds about a system is therefore due to what action the environment performs on the system. To better clarify this aspect, let us consider the evolution in Fig. 4. When quantum correlations are zero, for example at =π/2, there is a complete lack of classical information about what unitary operation the environment is applying to the qubit (statistical mixing of the two different unitary operations {U}_{{\text{p}}_{\pm}}); successively, when the initial quantum correlations are recovered at =π, this information becomes known because the two unitaries both act as a σ_{x} ‘bitflip’ operation (they are just the same operation).
Discussion
In this article we have introduced a simple twoqubit model particularly suitable to investigate the issue of the occurrence of revivals of quantum correlations despite the absence of backaction. In this model only one qubit of the pair locally interacts with a classical environment, in the form of a random external field with inhomogeneous broadening. The model forbids any mechanism both of systemenvironment backaction and of quantum correlation storage. Moreover, this model presents an overall decoherent evolution where any collective effect of external fields on the twoqubit system is excluded. We have then reported the results of a novel alloptical experimental setup that simulates the introduced model and permits us to observe revivals of quantum correlations (entanglement, quantum discord), with a decreasing revival amplitude in time. The amplitude of revivals can be controlled by adjusting the parameter of the initially prepared state.
We have also experimentally and theoretically shown, as a necessary condition for revivals of quantum correlations to occur, the link between the revivals themselves and the intrinsic nonMarkovian feature of the system evolution. We have provided a possible interpretation of the phenomenon in terms of quantumclassical system, showing the role had by the classical environment as a control system for what action it has on the quantum system and then in reviving quantum correlations. The introduced model and the corresponding experimental setup have thus permitted us to identify an interpretation of the phenomenon and to exclude side effects. Our findings clearly reveal that the revivals of quantum correlations are a dynamical feature of composite open systems independent of the nature (classical or quantum) of the environment.
Finally, our results introduce the possibility to recover and control, against decoherence, quantum correlation resources even in absence of backaction, without resorting to quantum structured environments^{22,23,24} or correction procedures^{4,25,26,27} and moreover open the way to further studies on the issue of quantum correlation revivals in classical environments^{15,28}.
Methods
State preparation process
As depicted in Fig. 1b, ultraviolet pulses are frequency doubled from a modelocked Ti:sapphire laser centered at 800 nm with 130 fs pulse width and 76 MHz repetition rate, and pass through a halfwave plate (HWP)1 and a Wollaston prism to be separated into two optical pump paths. The HWP1 rotates the polarization of the ultraviolet pulses which are separated by the Wollaston prism into two paths. The Wollaston prism transmits horizontal polarization H〉 and reflects vertical polarization V〉. Therefore, the relative amplitude between the two pump paths can be controlled by the HWP1. The HWP2 and HWP3 are used to control the polarization of the corresponding pump light. The two pump pulses are then combined by a polarizationindependent beamsplitter and pump two identically cut typeI betabariumborate crystals, with their optic axes aligned in mutually perpendicular planes^{29}, to generate entangled photon pairs. After compensating the birefringence effect between H〉 and V〉 in betabariumborate crystals with quartz plates (CP), maximally entangled photon pairs are generated in the state by the transmitted pump pulses and in the state by the reflected pump pulses. In our experiment, the time difference between the two pump paths is larger than the coherence length of the pump light so that the path information is traced out at the end of measurement^{3}. The prepared state is then the Belldiagonal state of equation (3).
Action of the environment part of the setup and output state
If the photon b is in the horizontal polarization H〉 and enters the environment part of the setup (see Fig. 1b), it undergoes all the transformations due to each optical component in the transmitted path (p_{−}) and reflected part (p_{+}) that give, respectively, and , where we have omitted the unimportant global phase factor e^{i}^{/2}. These are the two unitary transformations for H〉 given in equation (2), with =ωτ. Analogously, one obtains those for the polarization V〉. In particular, we find that the transmitted path transformation is , whereas the reflected path transformation is . These are the two unitary transformations for V〉 displayed in equation (2).
We now consider the evolution of the twophoton state with a single frequency ω. The state at the end of the transmitted part and of the reflected part is obtained by applying the transformations of equation (2) only on the second qubit b and it reads, respectively,
where . After tracing out the path information (the detection in our experiment traces over the time difference between the two paths), the input state Φ^{+}〉 then becomes the output mixed state.
Similarly, when the input state is Φ^{−}〉 the output state becomes
where . Therefore, starting from the effectively prepared state of equation (3), the twophoton output state is
The previous output state corresponds to the case of coherent evolution, where only the SBC is used (=ω_{0}τ). Considering the Gaussian distribution f(ω) of the frequency ω, the decoherence parameter κ=∫f(ω)cos(ω)dω arises by tracing out the photon frequency degrees of freedom. As and , the introduction of the decoherence parameter κ turns the previous state into the output state given in equation (4).
Correlation quantifiers
Total correlations are calculated by the quantum mutual information , where ρ_{a} and ρ_{b} are the reduced density matrices of ρ_{ab} whereas is the von Neumann entropy^{2}. Classical correlations are defined as the maximal information gained about ρ_{ab} by a measurement on one of the qubits, that is^{2}
where is the set of projective measurements performed on qubit b, and is the postmeasurement state of a after obtaining the outcome j on b. Quantum correlations (quantum discord) are then given by^{2} . Twoqubit entanglement is quantified by concurrence^{1} C(ρ_{ab})=max{0,Γ}, where , and χ_{j} are the eigenvalues in decreasing order of the matrix with σ_{y} denoting the second Pauli matrix and corresponding to the complex conjugate of ρ_{ab} in the canonical basis {HH〉,HV〉,VH〉,VV〉}. The theoretical dynamics of the correlation quantifiers is found by using their known analytical expressions for Belldiagonal states^{2,17}. The experimental results are acquired from the reconstructed output density matrices (by state tomography). Total correlations and concurrence are directly calculated for the output states. For obtaining classical and quantum correlations the maximization of equation (9) is required, performed by scanning the projective operators represented by {cosαH〉+e^{iθ}sinαV〉, e^{−iθ}sinαH〉−cosαV〉} on photon b. The scan precision of α and θ is set to π/100.
Quantifier of nonMarkovianity
We consider a maximally entangled input state , with the photon b subject to the environment and photon a isolated. The output state, in the coherent evolution case (=ω_{0}τ is the dimensionless time variable), becomes . The entanglement of the final state is quantified by the concurrence C=2 max[1/2(1+cos), 1/2(1−cos)]−1, that is C()=cos.
We quantify the memory effects present in the evolution of a system using the criterion of nonMarkovianity based on the distinguishability of two evolving quantum states, as measured by the trace distance D(ρ_{1}(t),ρ_{2}(t))=(1/2)ρ_{1}(t)−ρ_{2}(t), where , ρ_{i}(t)=Λ_{t}ρ_{i}(0) (i=1,2) and Λ_{t} is a dynamical map of the open system^{8}. The rate of change of the trace distance is
Given two initial states of the system, any temporary increase of the trace distance (σ(t)>0) is a signature of memory effects (nonMarkovianity of the dynamical map of the system). In order to obtain the degree of nonMarkovianity one then takes the maximum of σ(t) over the possible initial states ρ_{1,2}(0) and calculates^{8} .
Let us now consider the dynamical map of random external fields acting on a qubit in the coherent case (small lengths of the QPs, SBC compensator) , where U_{ϕ} is defined in equation (1) and Ωt ≡ ω_{0}τ=. For two arbitrary initial states, ρ_{k}(0) (k=1,2) in the basis {0〉 ≡ H〉,1〉 ≡ V〉}
the trace distance evolves as . It follows that the maximum of the rate of change is found for the initial states having α_{1}=α_{2}=1/2 and β_{1}=−β_{2}=i/2, that is the pure states . In this case the trace distance is D(ρ_{1}(),ρ_{2}())=cos=C() and the corresponding rate of change is σ()=−sgn(cos)sin^{21}.
Additional information
How to cite this article: Xu, J.S. et al. Experimental recovery of quantum correlations in absence of systemenvironment backaction. Nat. Commun. 4:2851 doi: 10.1038/ncomms3851 (2013).
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Acknowledgements
This work was supported by the National Basic Research Program of China (Grant No. 2011CB921200), National Natural Science Foundation of China (Grant Nos 11004185, 11274297, 61322506, 60921091, 11274289, 11325419, 61327901), the Fundamental Research Funds for the Central Universities (Grant No. WK 2030020019, WK2470000011), Program for New Century Excellent Talents in University (NCET120508), Science foundation for the excellent PHD thesis (Grant No. 201218) and the CAS.
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J.S.X. designed the experiment. J.S.X. and K.S. performed the experiment with the assistance of X.Y.X. R.L.F., G.C. and E.A. provided the theoretical analysis. C.F.L. and G.C.G. supervised the project. R.L.F., G.C. and J.S.X. wrote the manuscript. All authors read the manuscript and discussed the experimental results.
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Xu, JS., Sun, K., Li, CF. et al. Experimental recovery of quantum correlations in absence of systemenvironment backaction. Nat Commun 4, 2851 (2013). https://doi.org/10.1038/ncomms3851
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DOI: https://doi.org/10.1038/ncomms3851
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