Abstract
In many applications entanglement must be distributed through noisy communication channels that unavoidably degrade it. Entanglement cannot be generated by local operations and classical communication (LOCC), implying that once it has been distributed it is not possible to recreate it by LOCC. Recovery of entanglement by purely local control is however not forbidden in the presence of nonMarkovian dynamics and here we demonstrate in two alloptical experiments that such entanglement restoration can even be achieved ondemand. First, we implement an openloop control scheme based on a purely local operation, without acquiring any information on the environment; then, we use a closedloop scheme in which the environment is measured, the outcome controling the local operations on the system. The restored entanglement is a manifestation of “hidden” quantum correlations resumed by the local control. Relying on local control, both schemes improve the efficiency of entanglement sharing in distributed quantum networks.
Introduction
Quantum mechanics promises breakthroughs in computing and information fields, some of which are already available^{1,2}. Similarly to networking in classical information and computation, the advent of quantum networks envisages further advancements in information science^{3,4,5}. Tasks such as measurements, computing and memorization may be performed by subsystems implemented on different platforms^{6}, networking also providing the large amount of resources required to fault tolerant computation schemes^{7,8}. Recent experimental upscaling of quantum processors made it clear that for hardwareintrinsic noise sources the lowdecoherence DiVincenzo criterion^{9} could be met by subsystems of limited size^{10} in distributed architectures. This is a new and uniquely “quantum” feature of networking.
The roadmap towards distributed networks critically relies on the possibility that pairs (or clusters) of nodes share entanglement^{11,12}. This is the fundamental resource allowing remote quantum teleportation^{13,14,15,16} of an unknown quantum state or secure keys distribution for cryptographic purposes^{17}. In particular for the scope of our work it is important to note that entanglement could enable universal quantum computation in networks of noninteracting nodes, provided single qubit local operations are possible^{18}. Sharing entanglement can reduce the communication complexity, that is the minimal information exchange required to solve a given problem distributed among separated parts^{19}. Very recently, it has been proposed that entanglement may improve accuracy and precision in applications related to global positioning and timing by networking geographically remote atomic clocks^{20}.
In order to use entanglement as a nonlocal resource^{11,12}, it must be generated somewhere and then distributed amongst different parties. However noise unavoidably affects distribution and storage of entanglement, determining its degradation. It is well known that different parties cannot create any further entanglement, if they are only allowed to operate locally, i.e. on their own subsystem, exchanging at most classical information^{21}.
Our scope is distributed networks of spatially separated quantum nodes, each subject to a local environment. They model the structure of physically relevant distributed architectures. Remarkably, when environments induce a system dynamics which can be physically unraveled into an ensemble of entangled pure state evolutions, it may happen that quantum correlations of initially entangled states are not destroyed. Indeed even if entanglement appears degraded when measured on the averaged state, it is not lost but rather hidden in the lack of classical knowledge about the elements of the ensemble^{22}. In this case, leveraging the existence of such classical information, the initially shared entanglement can be restored at an arbitrary time without resorting to nonlocal operations.
An operational scenario emerges in which local controls can be used for ondemand restoration of entanglement in distributed architectures. Here we demonstrate this concept by two alloptical experiments. We consider two entangled photons subject to local environments as an instance of distributed entanglement. In the first experiment a local environment produces lowfrequency noise^{23} and it is shown how by local open loop control^{24} the initial entanglement is recovered, even if in the absence of control it would be degraded to very low values. In the second experiment, decoherence is due to the coupling between a subsystem (photon) and a quantum environment, whose degrees of freedom are experimentally accessible. A measurement on this environment and a subsequent conditional local operation on the system implement a local closedloop control^{25}, succeeding in restoring the initial entanglement. The relevance of these setups to different physical systems is discussed at the end of this work.
The nonMarkovian nature of the dynamics^{26,27} is a key ingredient for the entanglement recovery in our experiments. Certain physical aspects are common to other phenomena involving nonMarkovianity, such as spontaneous entanglement revivals during the system dynamics^{28,29,30,31,32,33,34}, or entanglement preservation by dynamical decoupling^{35,36,37}. Here, at variance with these examples, we engineer the overal dynamics by a local control and we demonstrate that distributed entanglement can be fully restored ondemand by suitable local operations even though it would vanish in the absence of active control.
Results
We consider a prototype distributed quantum network implemented by an alloptical setup where the information carriers are two photons, A and B. The information is encoded in the photon polarization, being either horizontal H〉, or vertical V〉. The system AB is prepared in the twophoton entangled Bell state . Qubits A and B propagate in freespace (communication channel) experiencing local interactions with different environmental degrees of freedom.
Theoretical framework
Typically the information available at time t on the system AB is encoded in the reduced density matrix ρ(t), obtained after tracing over the environment. It can be decomposed, in an infinite number of ways, in terms of pure states ν(t)〉, each one occurring with a probability p_{ν}(t): . The entanglement of the average state ρ(t) is
where E is some measure, reducing for pure states to the entropy of entanglement^{11,12}. In this work we study the entanglement of formation^{11,12} E_{f}, but we discuss our results in terms of the concurrence C, an entanglement measure with a simpler and very intuitive form Ref. 38. Note that E_{f} monotonically depends on the concurrence and can be readily calculated from it as E_{f}(C), see Methods.
In the absence of interaction with the environment, the density matrix does not evolve ρ(t) = ρ(0) = Ψ^{−}〉〈Ψ^{−}, whereas due to the interaction of the qubits with the environment, ρ(t) evolves in a statistical mixture. The corresponding amount of entanglement is no longer equal to that of the initial state Ψ^{−}〉.
Here we demonstrate that, acting by suitable local controls, the entanglement initially present in the system AB can be restored. This is possible if ρ(t) corresponds to a specific physical decomposition and we are somehow able to tag each member of the ensemble and to know its state. In this case we can distill the average entanglement of
by using local operations and classical communication only. For any convex measure E of entanglement, we have that . The inequality has a natural meaning, namely the classical knowledge of the state of each member of the quantum ensemble allows for a larger entanglement with respect to situations where this information is not available.
The experiments
In the two experiments we present here, the twophoton state AB is generated by a spontaneous parametric downconversion (SPDC) source of photon pairs based on Ref. 39. In both experiments, the degraded entanglement E_{ρ}(t), Eq.(1), is restored by a local control, whose effect is to make available the entanglement , Eq.(2). For the sake of simplicity photon A is measured directly whereas photon B is sent through a noisy channel before being measured. We address situations where the evolution of the system AB is nonunitary, due to the interaction with a local environment O inducing a nonMarkovian dynamics of AB^{30,40}.
In a first experiment we simulate classical nonMarkovian noise through a sequence of liquid crystal retarders which add random phases to photon B during propagation (pure dephasing). As a result, the initial entanglement of the system AB decays monotonically as a function of the channel length. Despite we are aware of the physical decomposition in terms of pure states and probabilities , we are not able to tag each state in the ensemble. Therefore the entanglement of the average state is given by Eq. (1). The action of a bitflip on photon B applied at halfway propagation along the channel restores the initial entanglement (openloop control). Therefore such a local control is able to retrieve the classical information on each member of the quantum ensemble , thus allowing to make available the average entanglement , Eq. (2). The amount of entanglement recovered by this technique depends on the degree of correlations (nonMarkovianity) among the environmentadded random phases.
In a second experiment, we simulate a quantum environment by a third qubit, O, interacting with qubit B through a controlledNOT (CNOT) gate. The coherent exchange of information between AB and the environment O roots the emergence of memory effects and of a nonMarkovian evolution of the reduced system AB. Measurement of the environment in a given basis makes possible the physical selection of a given quantum ensemble , allowing at the same time to tag each state of this ensemble. The average entanglement of (which can be equal to the initial entanglement) is then obtained, by applying a local operation on qubit B, which depends on the (classical) information gained on the environmental state (closedloop control).
Both experiments and their results are described in detail in the following subsections.
Openloop control
In this experiment, the photon B interacts with a classical environment O described by a stochastic process x(t). The corresponding noisy channel acting on B is designed to induce pure dephasing, according to the Hamiltonian: , where σ_{z} = H〉〈H − V〉〈V and δ is the Dirac delta function. Here, the interaction between B and O takes place stroboscopically at times t_{k} (see Fig. 1 a). This Hamiltonian is experimentally realized by sending the photon through a sequence of four liquid crystal retarders (LC_{k}), each one introducing a phase χ_{k} ≡ x(t_{k}) between the photon polarization components: . The phase χ_{k} depends on the voltage V_{k} applied to LC_{k} and can be varied continuously from 0 to π (see Fig. 1 b). To simulate the stochastic process, we generate a set of N random phase sequences , in which the phases χ_{k} are Gaussian random variables with the same variance σ^{2} and correlations μ ≡ 〈χ_{k}χ_{k}_{+1}〉/σ^{2}, μ ∈ [0, 1] (see Methods). The system dynamics averaging with respect to these sequences is obtained by mixing together the tomographic measurement data obtained with each of the N random phase sequences.
We investigated three different situations: a) the uncontrolled dynamics, where we simply look at the entanglement degradation resulting from the noisy channel; b) the controlled dynamics where we show how accessing classical information on the environment allows to operate corrections which fully restore the entanglement and c) the echoed dynamics where entanglement is recovered by a simple local operation with no need to have access to the classical information.
Uncontrolled dynamics
The reduced dynamics of AB induced by noise is in this case unambiguously described by the quantum ensemble , where stands for the joint probability p(χ_{1}, χ_{2}, χ_{3}, χ_{4}) and
with the overall phase accumulated up to step k. As a result, each state of the ensemble is maximally entangled, so that also the average entanglement (2) is maximum for any k: . However, the entanglement (1) of the average state, E_{ρ}(k), exhibits quite a different behavior. The system concurrence for the uncontrolled dynamics decays with k: in the case μ = 1 (full correlations), theory gives . For μ < 1 the concurrence, though more involved (see Methods), shows a similarly decaying behavior. In the experiment we measured the entanglement E_{ρ}(k) obtained for three different values of μ with the generated sets of random phase sequences . For k < 4, the LC_{i} with i > k are set at a constant phase instead of χ_{i}. The experimental (black symbols) and theoretical results (black lines) are presented in Fig. 2. These results show that the system entanglement decreases as the accumulated phase φ_{k} grows.
Corrected dynamics
In this case, we know the induced noise (since we generate it) and we can compensate it. Indeed, all that is needed is to insert another LC (LC_{corr}) after the channel and to apply to it a voltage so as to produce a phase x_{corr} = −φ_{4}, see Fig. 1. In practice, having only four LCs available, we used LC_{4} as the correction step and set it at a phase x_{4} = −φ_{3}. For such corrected dynamics the initial state is fully recovered, together with its entanglement: C_{corr}(4) = 1, for any μ, see blue symbols (experiment) and blue lines (theory) in Fig. 2. This demonstrates that the channelinduced degradation of entanglement is only due to a lack of classical knowledge: once φ_{3} is known, entanglement is recovered by a local phaseshift operation.
Echoed dynamics (openloop control)
Accessing information on the environment is not possible in practice in real quantum networks, where noise sources correspond to a large number of uncontrollable environmental degrees of freedom. Nevertheless, an open loop scheme operated by local control may still allow to recover the entanglement. To demonstrate this we use a control technique introduced in NMR^{41}: just after the step k = 2, we apply a local bitflip operation (U_{echo} = σ_{x}) on photon B, which flips its polarization: σ_{x}H〉 = V〉 and σ_{x}V〉 = H〉, see Fig. 1 a. Experimentally we insert a halfwave plate at 45° between LC_{2} and LC_{3} when measuring the entanglement at k = 3, 4, see Fig. 1 b. Our purpose is to induce an entanglement echo in the system dynamics. The state (3) which describes the system in each run of the experiment for k ≥ 3 now reads:
The local pulse is equivalent to a change of sign of the phases acquired at steps k = 3, 4 and it may tend to cancel the effect of φ_{2} = χ_{1} + χ_{2} if the four χ_{i} phases are to a certain extent correlated. In general the echo pulse is expected to favor the recovery of the average state entanglement, especially for an environment with nonMarkovian correlations.
The plots in Fig. 2 show that, indeed, the entanglement for the echoed dynamics starts to increase at k ≥ 3, see red symbols (experiment) and red lines (theory). It is also clear that entanglement recovery strongly depends on correlations. For μ = 1 (Fig. 2 a), the characteristic time scale of the environment dynamics is much larger than that of the system dynamics. In this case full entanglement recovery is possible: χ_{3} + χ_{4} = −φ_{2} and we have that (red line), see Methods. Partial recovery is possible when 0 < μ < 1 (Fig. 2 b for μ = 0.7 and Fig. 2 c for μ = 0.2). In that case, χ_{3} + χ_{4} cancels φ_{2} only partially and we have to deal with a bit more involved expression for the concurrence (red lines), see Methods. Let us stress that, whereas in the corrected dynamics we used the knowledge of the sequence to cancel the accumulated random phase, in the echoed dynamics the (partial) cancellation of the phase needs no knowledge of the environment.
Our experimental data reported in Fig. 2 show a very good entanglement recovery, both for the corrected and the echoed dynamics. Deviations from the ideal expectations are mainly due to the imperfect preparation of the input state: in Fig. 2 we also plot (dashed lines) the expected entanglement for a mixed input state with a (measured) fidelity to the ideal input state Ψ^{−}〉, see Eqs. (10) and (11) in Methods. Black and red dashed lines refer respectively to the uncontrolled and echoed entanglement, which are derived from Eqs. (18) and (19) in Methods. For the corrected dynamics (blue squares), the recovered entanglement at step k = 4 does not quite reach the initial entanglement at k = 0, this is due to the finite precision we have on setting the phases for each LC. In the same way, for the echoed dynamics, the slight discrepancy between the measured (red triangles) and the theoretical (red dashed line) values for k ≥ 3 is due to small differences between the phase responses of each LC.
We remark that, although the system dynamics we consider is nonMarkovian^{26,27}, no spontaneous entanglement revival occurs in the uncontrolled dynamics. NonMarkovianity remains undetected by any measure based on the nonmonotonicity of entanglement^{40}. The local control triggers a reverse flow of classical information from the environment to the system^{42}. This also makes nonMarkovianity be phenomenologically evident and detectable by measures which are based on the nonmonotonicity of some suitable quantity^{27}.
Closedloop control
In this second experiment, qubits A and B are still encoded in the polarization of photons A and B, the environment being now a third qubit O, encoded in the longitudinal momentum degree of freedom (the path) of photon B. The state of O can be either “up”, u〉 = 0〉, or “down”, d〉 = 1〉, see Fig. 3. The system plus environment ABO is initially prepared in the state
The interaction of B with the environment O is engineered as follows: O is first rotated by the gate , where and ; subsequently, B undergoes the CNOT gate , which may flip the polarization of B according to the state of O, see Fig. 3 a. The gate is experimentally implemented by a balanced beamsplitter and an attenuation filter in both its output ports, with a ratio p′ = p/(1 − p) between their respective intensity transmission coefficients; the CNOT gate G_{BO} is implemented by an halfwave plate at 45° in the “down” path of photon B, see Fig. 3 b.
Uncontrolled dynamics
The state of ABO after the BO interaction is:
where is another Bell state. After tracing out the environment, the system is described by , with concurrence C_{unco}(p) = 1 − 2p. No further operation is applied on B before we measure the entanglement of AB. The corresponding entanglement of formation E_{f} depends on p, exhibiting a monotonous decay in the range [0, 1/2], see the black curve (theory) and points (experiment) in Fig. 4 a.
Controlled dynamics
We show how it is possible to recover entanglement by a “closedloop” like control scheme. It consists of two steps: 1) after the gate G_{BO}, O is projectively measured in the basis and 2) depending on the outcome k, a unitary operation is performed on B, and , see Fig. 3 a. Experimentally, the selection of the O measurement basis is obtained by a MachZehnder interferometer with a variable phase φ = 2θ which realizes the rotation , see Fig. 3 b. The unitary is obtained by doing nothing further on the output path θ_{u}〉 and inserting a halfwave plate at 45° in the path θ_{d}〉. The entanglement in AB is measured by mixing the polarization tomography data obtained on both output paths. Note that we actually used a folded version of the setup presented in Fig. 3 b, see Methods and Fig. 3 c.
The fact that we can distinguish the modes k = u, d emerging from the second interferometer, allows to associate on a physical basis the ensemble (see Methods) to the state of the system. Moreover, we tag the actual state of the ensemble during each run of the experiment. This classical information enables us to apply some suitable local control which depends on the actual state. The goal is to obtain a new quantum ensemble (see Methods), whose corresponding density matrix, , exhibits the average entanglement of .
We investigate two special cases. First we take θ = 0 (the measurement basis of O is thus its natural basis), yielding the quantum ensemble . For it we have for any value of p. This entanglement is restored by the local control which flips the photon B polarization each time the system is the state Φ^{−}〉. This produces the output state , whose concurrence C_{cont}(p) = 1. We plot the corresponding entanglement obtained after the control loop as a function of p in Fig. 4 a, see violet line (theory) and triangles (experiment): the restoration of the initial entanglement is achieved for any value of p when the measurement basis angle is θ = 0. As a second example, we consider the case in which the entanglement for the uncontrolled dynamics vanishes, which happens for p = 0.5. We show that the amount of entanglement recovery depends on the measurement performed on O, that is to say on the angle θ of the rotated measurement basis. This measurement selects the system AB quantum ensemble (see Methods). For it we find , since the concurrence of both states is cos(2θ). The O measurement by itself does not produce any effect on the AB entanglement, which is vanishing for any θ in that case, see black line (theory) and points (experiment) in Fig. 4 b. Instead application afterwards of the local control on the qubit B may lead to recovery of the average entanglement of the ensemble, . Indeed, the resulting output state for AB is
whose concurrence is C_{cont}(θ) = cos(2θ), see the pink line (theory) and triangles (experiment) in Fig. 4 b. Here we see that the natural basis of O is the optimal measurement basis to recover the entanglement, whereas for no entanglement is regained.
The experimental data (symbols) plotted in Fig. 4 show some deviation from the ideal expectations (continuous line). To explain them, we take into account the imperfect state preparation by our SPDC source: we also plot on Fig. 4 the expected entanglement for a mixed input state whose fidelity with the ideal input state is (dotted line) or 0.95 (dashed line), see Methods. Note that in Fig. 4 a, the entanglement measured for p = 1 is slightly lower than for p = 0 (violet triangles) mainly because of the noise added by the CNOT on Φ^{−}〉.
Discussion
In this article we have presented two experiments showing that recovery of entanglement after the interaction of the members of an entangled state with a local nonMarkovian environment can be achieved ondemand through local operations only. In the first experiment, the local environment is classical and induces low frequency noise, so that entanglement may be recovered by a local echo pulse. In the second experiment, the environment is a small quantum system (here a qubit) accessible to measurement, whose output controls a subsequent local operation on the system: as a result, entanglement recovery is obtained.
We note that in the second experiment there exists a measurement basis that selects system states with the largest amount of average entanglement. This maximum entanglement, recovered by the subsequent local operation, is known as entanglement of assistance^{43,44}, a concept of which we provide here an experimental illustration. Instead the first experiment is a prototype of situations where the environment is not accessible in practice, typically because a large number of uncontrolled degrees of freedom are involved. Nevertheless, the recovery of entaglement by local operations is possible, since entanglement is not actually destroyed, but rather hidden due to a lack of classical information about which element in an ensemble of entangled states we are dealing with^{22}.
Interestingly, the scheme of our first experiment is the simplest instance of recently proposed architectures, which should limit the detrimental upscaling hardwareintrinsic decoherence, namely networks of smaller mutually entangled subsystems. Striking examples are trapped ions where modes in a single trap become dense as the trap becomes larger, acting as stray degrees of freedom, besides exquisitely solidstate systems as electrostatically defined quantum dots, siliconbased implanted impurities and optically active dopants^{10}. Very effective ondemand recovery by local operations is possible when noise has strong lowfrequency components. We stress that this is a very relevant physical case, 1/f noise being a major drawback for solid state quantum computation^{10,23} and it is likely to be an important source of decoherence in practical computation and communication networks. Direct applications of the scheme of our second experiment can be also envisaged in cavity quantum electrodynamics (QED)^{45,46} or in circuit QED systems^{47}, where twolevel quantum systems are strongly coupled to discrete photon modes in highquality cavities. Finally we remark that this work, besides experimentally demonstrating novel physics related to nonMarkovianity of open quantum systems, namely entanglement recovery by local operations, envisages new applications of quantum control techniques^{48,49,50,51,52} to distributed architectures.
Methods
Entanglement of formation
As entanglement measure E_{ρ} we use the entanglement of formation E_{f}^{11,12}, which can be directly obtained from the concurrence C(ρ)^{38} by the following formula:
where h(x) = −x log_{2} x − (1 − x) log_{2}(1 − x) and C(ρ) = max{0, λ_{1} − λ_{2} − λ_{3} − λ_{4}}. Here λ_{i} (λ_{i} ≥ λ_{i}_{+1}) are the square roots of the eigenvalues of the nonHermitian matrix , being the conjugate of ρ.
Openloop control
Random phases
The random variables χ_{k} are Gaussian with a standard deviation σ = 0.6 rad and an average , 〈·〉 being the ensemble average. Since we disposed of halfwave LCs, which could only generate phases in [0, π], this setting provided that 99% of the random phases were inside the experimentally achievable interval. Each sequence of random variables were generated (using Scilab random number generation function “grand”) by keeping χ_{i} equal to χ_{i}_{−1} with probability μ and χ_{i} independent from χ_{i}_{−1} with probability 1 − μ.
The degree of memory in may be quantified by μ, which corresponds to the correlation coefficient^{53} between χ_{k} and χ_{k}_{+1} inside each sequence:
Imperfect initial state
To take into account the effect of the imperfect state generated by our SPDC source, we consider the following partially mixed state as input sate:
where input state is the maximally mixed input state and the mixing parameter η is related to the fidelity by
Theoretical calculation of the entanglement
We calculate the output state of the twophoton system when the initial state is ρ_{in} = Ψ^{−}〉〈Ψ^{−}.
For the uncontrolled dynamics, the twophoton state averaged on is:
where is given by Eq. (3). We will use the following abbreviations: ρ_{ij}(t_{n}) ≡ 〈iρ(t_{n})j〉 where i, j ∈ {a, b, c, d} and a〉 ≡ 00〉, b〉 ≡ 01〉, c〉 ≡ 10〉, d〉 ≡ 11〉. The noise only affects the coherences . These coherences are calculated by averaging the phase factor :
whose explicit expressions are:
For the echoed dynamics, we have to replace in Eq. (12), for k = 3, 4, with from the state (4). We call the new average state. The only nontrivial element we have to calculate is
whose explicit expressions are:
By means of the equations (14), (16) and by taking into account that the considered noisy channel is unital (the channel does not change the input state ), it is straightforward to calculate the corresponding output state for the initial state (10), simply by using the linearity of quantum operations.
The system AB concurrence can be calculated by the formula
since the AB density matrix assumes always a Xform^{54}. In the case of uncontrolled dynamics, the concurrence reads
with k ∈ {1, 2, 3, 4}, whereas in the case of echoed dynamics, the concurrence is given by
with k ∈ {3, 4}. Obviously, for η = 1 we obtain the formula relative to the perfect state preparation ρ_{in} = Ψ^{−}〉〈Ψ^{−}. From (18) and (19), we can derive the entanglement of formation by means of Eq. (8).
Closedloop control
Actual experimental setup
The actual setup that was implemented for this second experiment is shown in Fig. 3 c. For the sake of phasestability and convenience, we opted for a folded version of the setup shown in Fig. 3 b: the two MachZehnder interferometers were replaced by two Sagnac interferometers using a single beamsplitter. Likewise, we chose to measure the exit modes “θ_{u}” and “θ_{d}” on the same exit port “θ_{u/d}”: for a given angle θ, “θ_{u}” was measured for ϕ = 2θ and “θ_{d}” was measured for ϕ = π − 2θ.
Ensembles of pure states
In the ensemble of pure states , , , and . With regard to the quantum ensemble , we have and . For the ensemble , and .
Imperfect state preparation
To take into account the imperfection of the state preparation (originating from the SPDC source and the CNOT wave plate mainly), we modeled the initial state as in Eq. 10. The fidelity of the initial AB state was comprised in the interval {0.90, 0.95}, it was estimated by measuring separately the fidelity of the Ψ^{−}〉 and Φ^{−}〉 states in the “up” and “down” paths respectively.
Theoretical calculation of the entanglement
For the uncontrolled dynamics, when the input state is the mixed state given by (10), the output state ρ_{out}(p) has a concurrence:
For the controlled dynamics and the same input state, the output state has the concurrence:
Error bars
The errors bars on Fig. 4 are calculated from the Poissonian statistical errors associated to the coincidence counts.
The vertical error bars stem from the propagation of the Poissonian statistical errors of the 36 coincidence counts used for the quantum tomography that allows to measure E_{f}.
The horizontal error bars, for the measurements done varying p′ (Fig. 4 a), stem from the Poissonian statistical errors of the coincidence counts used to set p′:
where C_{HHd} and C_{VVd} (C_{HVu} and C_{VHu}) are measured coincidence counts corresponding to the state Φ^{−}〉 on the path d〉 (to the state Ψ^{−}〉 on the path u〉). The error δp′ on p′ is thus given by:
where δC_{j} is the the Poissonian statistical error on C_{j}.
The horizontal error bars, for the measurements done varying θ (Fig. 4 b), stem from the Poissonian statistical errors of the coincidence counts used to set θ:
where C_{HV}_{1} and C_{VH}_{1} (C_{HV}_{0} and C_{VH}_{0}) are the coincidence count values measured on the output mode θ_{d} (θ_{u}). The error δθ on θ is given by:
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Acknowledgements
G.B. acknowledges support from MIURPRIN 2011. P.M., F.S. and A.O. acknowledge support from the European project QWAD, Quantum Waveguide Application and Devices, http://www.qwadproject.eu/. R.L.F. acknowledges support by the Brazilian funding agency CAPES [Pesquisador Visitante EspecialGrant No. 108/2012]. A.D'A. and R.L.F. acknowledge support from Centro Siciliano di Fisica Nucleare e Struttura delle Materia (Catania).
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A.D'A., R.L.F., G.B., E.P. and G.Fa. conceived the original theoretical idea. A.O., A.D'A., G.Fe., F.S. and P.M. planned the experimental implementation. A.O., G.Fe. and P.M. carried away the experiment. A.O., A.D'A. and P.M. analysed the data. All authors contributed to the preparation of the manuscript.
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Orieux, A., D'Arrigo, A., Ferranti, G. et al. Experimental ondemand recovery of entanglement by local operations within nonMarkovian dynamics. Sci Rep 5, 8575 (2015). https://doi.org/10.1038/srep08575
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DOI: https://doi.org/10.1038/srep08575
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