Abstract
Repeated measurements can slow down (the quantum Zeno effect) or speed up (the quantum antiZeno effect) the temporal evolution of a quantum system. In this paper, a general treatment of the quantum Zeno and antiZeno effects is presented which is valid for an arbitrary systemenvironment model in the weak systemenvironment coupling regime. It is shown that the effective lifetime of a quantum state that is subjected to repeated projective measurements depends on the overlap of the spectral density of the environment and a generalized ‘filter function’. This filter function depends on the systemenvironment Hamiltonian, the state of the environment and the measurement being performed. Our general framework is then used to study explicitly the Zeno to antiZeno crossover behaviour for the spinboson model where a single twolevel system is coupled to a bosonic environment. It is possible to not only reproduce results for the usual population decay case as well as for the pure dephasing model, but to also study the regime where both decay and dephasing take place. These results are then extended to many twolevel systems coupled collectively to the bosonic environment to further illustrate the importance of the correct evaluation of the effective decay rate.
Introduction
It is wellknown that if a quantum system is subjected to rapidly repeated measurements, the temporal evolution of the quantum system slows down^{1}. This effect, known as the Quantum Zeno effect (QZE), has attracted widespread interest both theoretically and experimentally due to its relevance to the foundations of quantum mechanics as well as possible applications in quantum technologies^{2,3,4,5,6,7,8,9,10,11,12,13,14,15,16,17,18,19,20,21,22,23}. Surprisingly, however, it has also been found that if the measurements are not rapid enough, the opposite effect can occur, that is, the measurements can actually accelerate quantum transitions. This effect has been appropriately dubbed the quantum antiZeno effect (QAZE)^{24,25,26}. Since this discovery, both the QZE and QAZE have been studied in many different physical setups such as superconducting qubits^{10,23,27}, nanomechanical oscillators^{28}, Josephson junctions^{29}, disordered spin systems^{30} and localized atomic systems^{31}. Generally speaking, the focus has been to study the population decay of quantum systems, whereby the quantum system is prepared in an excited state and the system is thereafter repeatedly checked to see if the system is still in the excited state or not^{24,26,28,29,30,31,32,33,34,35,36,37}. It has then been shown that the decay rate depends on the overlap of the spectral density of the environment and a measurementinduced level width^{24}. This overlap changes as the measurement rate changes, generally leading to a crossover from the Zeno regime with large measurement rates to the antiZeno regime with relatively smaller measurement rates.
With increasingly sophisticated quantum technologies, it becomes important to investigate what happens beyond such population decay models. For instance, we can envisage repeatedly preparing not simply the excited state, but rather a superposition state of the ground and excited states. Such a superposition state will undergo not only population decay but also dephasing^{38}. To this end, the QZE and the QAZE have been studied for a pure dephasing model in ref. 39. It was found therein that there are considerable differences between this case and the population decay case. For example, for the pure dephasing model in the weak coupling regime, the lifetime of the quantum state depends on the overlap of the spectral density of the environment and a ‘filter function’ that is different from the usual sincsquared function obtained for the population decay model. Moreover, by examining the collective dephasing of many twolevel systems, it was found that multiple Zeno and antiZeno regimes can be found. At the same time, however, these results are limited in the sense that they are only applicable for exactly solvable pure dephasing models. Nevertheless, these differences motivate us to investigate the QZE and the QAZE for more arbitrary systemenvironment Hamiltonians and state preparations. To this end, in this work, we derive an expression for the effective lifetime of a quantum state, subjected to repeated projective measurements, that is valid for weak systemenvironment coupling strength. This effective lifetime depends on the overlap between the spectral density of the environment and a generalized ‘filter function’ that in turn depends on the state that is repeatedly prepared, the environment correlation function, the system Hamiltonian parameters, the measurement interval and the systemenvironment coupling. This expression is general in the sense that no assumption is made beforehand about the actual form of the systemenvironment Hamiltonian or the state that is being repeatedly prepared. The effective decay rate of the quantum state can thereby be controlled by suitably engineering the spectral density of the environment^{40}.
Once we have derived a general expression for the effective lifetime of a quantum state, our main task then is to actually evaluate the generalized filter function. To illustrate the application of our formalism, the task of evaluating this filter function is first performed for the usual population decay model to show that we reproduce the wellknown sincsquared filter function. Similarly, we produce results that are in agreement with the exactly solvable pure dephasing model in the weakcoupling regime. We then consider the QZE and QAZE for the general spinboson model where generally both population decay and dephasing take place. In particular, we show that the filter function is different for the general case as compared with the pure dephasing and decay cases and must be carefully evaluated. We then calculate the effective lifetime of the quantum state and thereby the Zeno to antiZeno crossover behaviour, to further illustrate the differences as compared to the pure dephasing and decay cases. We next consider a collection of twolevel systems collectively coupled to an environment that causes both dephasing and decay. In this case, we find that the effective decay rate is amplified depending on the number of particles coupled to the environment, thereby making the use of the correct filter function even more important.
Results
The general expression for the effective decay rate
We start by considering a general systemenvironment Hamiltonian written in the form H = H_{S} + H_{B} + V, where H_{S} is the system Hamiltonian, H_{B} is the Hamiltonian of the environment and V describes the systemenvironment interaction. At time t = 0, we prepare the initial system state . N repeated projective measurements, given by the projector , are now applied with equal time interval τ. It should be noted that before each measurement, we apply the operator in order to remove the system evolution due to H_{S} itself^{39,41}. In other words, following refs 39 and 41, we consider the socalled ‘dynamical fidelity’ to characterize the effective decay rate. If the survival probability of the quantum state is S after N time intervals, it is convenient to write S ≡ e^{−Γ(τ)Nτ}, thereby allowing us to interpret 1/Γ(τ) as the effective lifetime of the quantum state. Alternatively, Γ(τ) can be interpreted as the effective decay rate of the quantum state. We assume that the systemenvironment interaction is weak enough such that we can safely ignore the buildup of the systemenvironment correlations as the system and the environment evolve together^{39}. That is, we are neglecting any disturbance to the environment induced by measuring the system. In this case, S = [s(τ)]^{N} where s(τ) is the survival probability associated with one measurement. The effective decay rate is then . Now, assuming that the coupling V can be written as F ⊗ B where F is an operator acting in the Hilbert space of the system and B is an operator acting in Hilbert space of the environment, we have found that the effective decay rate can be written as an overlap integral of the spectral density of the environment J(ω) and a generalized ‘filter function’ Q(ω, τ). That is,
where the generalized filter function Q(ω, τ) is
Here , is a projector onto the subspace orthogonal to ρ_{S}(0) and . The environment correlation function is given by where , ρ_{B} is the initial state of the environment and Tr_{B} denotes taking trace over the environment. The function f(ω, t) can then be extracted from . Details regarding the derivation of Eq. (1) can be found in the Methods section.
Thus, we have found that if the systemenvironment coupling is weak, the effective decay rate of a quantum state Γ(τ) depends on the overlap of the spectral density of the environment J(ω) and an effective filter function Q(ω, τ). This filter function depends on the frequency of the measurement, the state that is repeatedly prepared, the way that the system is coupled to the environment and part of the environment correlation function. Note that the behaviour of Γ(τ) as a function of τ allows us to identify the Zeno and antiZeno regimes. One possible approach, followed for instance in refs 25 and 32, is to compare the ‘free’ effective decay rate in the absence of any measurements with the measurementmodified effective decay rate. An alternative approach, which we adopt in this paper, is to simply say that if Γ(τ) decreases when τ decreases, we are in the Zeno regime, while if Γ(τ) increases if τ decreases, then we are in the antiZeno regime^{24,33,36,39}. We also note that for the more generalized systemenvironment coupling V = ∑_{μ}F_{μ} ⊗ B_{μ}, Γ(τ) is again given by Eq. (1), but now the filter function is
where f_{μν}(ω, t) is extracted from .
Application to the population decay model
To illustrate the formalism that we have developed, let us start from the systemenvironment Hamiltonian (we set ħ = 1 throughout this work)
Here a twolevel system with level spacing ε interacts with an environment, which is modeled as a collection of harmonic oscillators and undergoes population decay. σ_{z} is the standard Pauli matrix, σ^{+} and σ^{−} are the raising and lowering operators respectively, ω_{k} are the frequencies of the environment oscillators, and b_{k} are the creation and annihilation operators for the oscillators and the g_{k} describe the interaction strength between the twolevel system and the environment modes. This systemenvironment Hamiltonian is widely used to study, for instance, spontaneous emission^{42}. Note that this Hamiltonian is the same as
except that the nonrotating wave approximation terms have been dropped. To calculate the filter function, we identify F_{1} = σ^{+}, , F_{2} = σ^{−} and . Let us first calculate the environment correlation functions. We find that , where 〈...〉_{B} denotes taking an average over the environment state. At zero temperature, all the oscillators are in their ground state and we get . This sum is converted to an integral over the environment frequencies via the substitution , thus allowing us to identify f_{12}(ω, t) = e^{−iωt}. On the other hand, it is straightforward to show that C_{11}(t) = C_{22}(t) = 0 and C_{21}(t) = 0 at zero temperature as well. The state initially prepared is the excited state which we denote by . It follows that , where . Using and , we find . Performing the integrals, we end up with , which is the usual filter function^{24,26}. Thus, our formalism reproduces the wellknown sincsquared function for the case where we study the Zeno to antiZeno transition in the context of population decay. In particular, if τ is small, then we obtain , thus putting us in the Zeno regime. However, for larger τ, decreasing τ can increase the overlap between J(ω) and Q(ω, τ), leading to the antiZeno effect.
Application to the pure dephasing model
Let us now consider the system environment model specified by the Hamiltonian
A twolevel system with level spacing ε is interacting with an environment that is again modeled as a collection of harmonic oscillators. However, now there is no population decay. Instead, the system undergoes dephasing only, which is the reason why this model is known as the pure dephasing model^{39}. Once again, we start by calculating the environment correlation function. Assuming the environment to be in the standard equilibrium state, that is with Z_{B} the partition function, it is straightforward to show that . We consider the system state that we start off with to be , where, as before, and . We repeatedly measure to check if the state is still or not with time interval τ. Now , leading to . Performing the integrals and simplifying, we obtain .
On the other hand, the pure dephasing model can be solved exactly. Using the exact solution, it can be shown that^{39} , where . For weak coupling, however, 1 − e^{−γ(τ)} ≈ γ(τ), leading to , in agreement with the result obtained using the formalism that we have developed.
Application with both dephasing and decay present
We now consider the more general systemenvironment model given by the Hamiltonian
where Δ can be understood as the tunneling amplitude for the system and the rest of the parameters are defined as before. This is the wellknown spinboson model^{43,44,45}, which can be considered as an extension of the previous two cases in that we can now generally have both population decay and dephasing taking place. We revert to the usual dephasing model by setting Δ = 0, while setting ε = 0 leads to the population decay Hamiltonian (with the nonrotating wave approximation terms now included) after rotation about the yaxis. Experimentally, such a model can be realized, for instance, using superconducting qubits^{23,46,47} and the properties of the environment can be appropriately tuned as well^{48}.
We start from the general system initial state , where the states and are defined as before and θ and ϕ are parameters that characterize the state preparation. Measurements, with time interval τ, are now carried out to check if the system is still in this state or not. To evaluate Q(ω, τ), we first need to find the environment correlation function. We again consider the environment to be in a thermal equilibrium state. Consequently, as in the pure dephasing model, f(ω, t) = cos(ωt)coth(βω/2) − i sin(ωt). Next, we find . This is done using the standard commutation relation [σ_{k}, σ_{l}] = 2iε_{klm}σ_{m}. A straightforward application of the BakerHausdorff lemma^{49} shows that , with
and Ω^{2} = ε^{2} + Δ^{2}. Now, given , we can deduce that with . The rest of the calculation for the filter function proceeds in a straightforward manner, leading to
with and . Here r_{1}(t) = −a_{x}(t)cos ϕ cos θ − a_{y}(t)sin ϕ cos θ + a_{z}(t)sin θ and r_{2}(t) = a_{y}(t)cos ϕ − a_{x}(t)sin ϕ.
We next evaluate D_{1}(ω, τ) and D_{2}(ω, τ). Although the integrals can be done, the final analytical results for arbitrary θ and ϕ are, unfortunately, very long and not very illuminating. Instead, let us choose θ = π/2 and ϕ = 0. This choice of state has the advantage that we can then compare our results with the already wellknown cases of the population decay model and the pure dephasing model. In particular, the choice Δ = 0 then corresponds to the pure dephasing model (in the weak coupling limit). On the other hand, ε = 0 corresponds to (almost) the population decay model since we can rotate both the systemenvironment Hamiltonian and the state that we are measuring about the yaxis. The only difference is that we now have additional nonrotating wave approximation terms, but we expect these additional terms to not play a role in the weak systemenvironment coupling regime that we are in. It must be emphasized that we are now no longer restricted to these two models only. Rather, by varying the values of θ, ϕ, ε and Δ, we can explore regimes where both dephasing and relaxation play a role in the quantum Zeno and antiZeno effects.
With θ = π/2 and ϕ = 0, the calculation for D_{1}(ω, τ) and D_{2}(ω, τ) becomes less laborious since r_{1}(t) and r_{2}(t) simplify greatly. Analytical expressions for D_{1}(ω, τ) and D_{2}(ω, τ) are given in the Supplemental Material. A few points are in order. First, if Δ = 0, then D_{2}(ω, τ) = 0, while D_{1}(ω, τ) = [1 − cos(ωτ)]/ω^{2}, which, as expected, leads back to the filter function for the pure dephasing model. Similarly, for zero temperature with ε = 0, D_{1}(ω, τ) and D_{2}(ω, τ) simplify such that we get back the filter function for the population decay model. For intermediate values of ε and Δ, however, the filter function is very different. This is illustrated in Fig. 1 where Q(ω, τ) has been plotted (in dimensionless units with ħ = 1) as a function of ω for two different values of τ. The dashed, red curve is the filter function for the population decay model with ε = 0 and Δ = 1 and is thus consequently peaked at ω = 1 in both Fig. 1(a,b). The dotdashed, magenta curve is the filter function for the pure dephasing model (with ε = 1 and Δ = 0), while the solid, blue curve shows the intermediate case with ε = 2 and Δ = 1. Clearly, if the value of τ is not too small, the filter function for the intermediate case resembles neither the population decay model nor the pure dephasing model. This means that for an arbitrary spectral density of the environment, the value of Γ(τ) is expected to be quite different with both Δ and ε nonzero as compared to the population decay and pure dephasing cases. On the other hand, as τ becomes smaller, we must have that Γ(τ) → 0 and thus the filter functions must start to resemble each other more for smaller τ. This is entirely consistent with what we see in Fig. 1(b).
With the different behaviour of the filter function, we expect that when there is both dephasing and decay, the effective decay rate will be quite different compared to either of the aforementioned cases and thus the Zeno and antiZeno behaviour is expected to be considerably modified. Let us now explicitly examine this claim for the case of subOhmic, Ohmic and superOhmic environments. To this end, we introduce the spectral density as . Here the parameter s characterizes the Ohmicity of the environment. Namely, s = 1 corresponds to an Ohmic environment, s > 1 gives a superOhmic environment, while s < 1 corresponds to a subOhmic environment. G is a dimensionless parameter characterizing the systemenvironment coupling strength and we have introduced an exponential cutoff function with a cutoff frequency ω_{c}. Let us first investigate an Ohmic environment. In Fig. 2(a), we illustrate the behaviour of the effective decay rate Γ(τ) as a function of the measurement interval τ, clearly showing the very different behaviour of Γ(τ) when both population decay and dephasing are present. For the population decay case (the dashed, red curve), with the chosen values of the systemenvironment parameters, Γ(τ) by and large decreases as τ decreases. Thus, we are in the Zeno regime. On the other hand, the pure dephasing case (dotdashed, magenta curve) displays a distinct Zeno regime and an antiZeno regime. For small values of τ, Γ(τ) decreases as τ is decreased, meaning that a shorter measurement interval helps to protect the quantum state, thus putting us in the Zeno regime. For larger values of τ, however, as the τ is decreased the opposite happens, namely, Γ(τ) increases as τ decreases, thus indicating the antiZeno regime. Now, when both dephasing and population decay take place (solid, blue curve), the behaviour of Γ(τ) is considerably different. Besides the quantitative differences in the values of Γ(τ), the effective decay rate displays qualitatively different behaviour in the sense that we now have clearly distinct multiple Zeno and antiZeno regions. This is evident from the fact that Γ(τ) displays multiple extrema, meaning that sometimes decreasing the measurement interval reduces the decay rate, while sometimes the opposite happens.
The effective decay rate, as we have emphasized, depends on the overlap of the spectral density and the generalized filter function. Thus, we expect that changing the environment and in particular the Ohmicity parameter, should alter the decay rate, at least quantitatively. In Fig. 2(b), we have calculated the decay rate with a similar set of parameters as was done with the Ohmic environment. The only difference is that we are now considering a subOhmic environment with s = 0.8. Once again, while the population decay case exhibits the QZE and the pure dephasing case exhibits both the QZE and the QAZE, the more general case displays multiple transitions between the QZE and the QAZE. We have also examined a superOhmic environment [see Fig. 2(c)] with s = 2. Now the population decay case also exhibits both the QZE and the QAZE. With both dephasing and population decay present, we again have multiple Zeno to antiZeno transitions, but these transitions are less clear cut as compared to what we observed in the previous cases. These results illustrate the importance of the type of environment in determing the QZEQAZE crossover behaviour.
Before moving on, let us also investigate the Zeno and antiZeno effects for a different state preparation. Namely, we choose θ = 0 and ϕ = 0. Once again we find D_{1}(ω, τ) and D_{2}(ω, τ) and use these to find the effective decay rate. Exact expressions for D_{1}(ω, τ) and D_{2}(ω, τ) can be found in a similar way as before (refer to the Supplemental Material). With these expressions in hand, we can investigate the behaviour of Γ(τ). In Fig. 2(d), we have shown the behaviour of Γ(τ) for the population decay Hamiltonian (dashed, red curve), the pure dephasing case (dotdashed, magenta curve) and the intermediate case (solid, blue curve) with an Ohmic environment. For pure dephasing, Γ(τ) remains zero. This makes sense since the state that we are repeatedly preparing, namely , does not evolve under the action of the pure dephasing Hamiltonian. On the other hand, the population decay Hamiltonian leads to both decay and dephasing, since, after rotation about the yaxis, the state that is repeatedly prepared is a superposition of the and states. Although both the population decay Hamiltonian and the intermediate case display multiple Zeno to antiZeno transitions, the actual value of the decay rate, in general, is considerably different for the two cases. These two cases also differ in the values of τ for which the transitions take place. By now, it should be clear that using the usual simple sincsquared filter function to analyze a system undergoing both dephasing and decay would be incorrect.
Application to the large spinboson model
Let us now consider N_{s} twolevel systems interacting collectively with a common environment. The systemenvironment Hamiltonian is now
where ε and Δ are the level spacing and tunneling amplitude respectively for each twolevel system and J_{x} and J_{z} are the standard angular momentum operators. This Hamiltonian can be considered to be a generalization of the usual spinboson model to a large spin j = N_{s}/2^{39,50,51}. Physical realizations include a twocomponent BoseEinstein condensate^{52,53} that interacts with a thermal reservoir via collisions^{51}. Once again, we assume that the systemenvironment coupling is weak so that our formalism applies. The initial state is chosen to be such that and we repeatedly check, with time interval τ, whether the system state is still or not. We note that we can easily deal with some other choice of initial state as well. As before, our task is to calculate Q(ω, τ), the details of which are given in the Methods section. The important point to note here is that the decay rate is amplified depending on the number of twolevel systems coupled to the environment. Namely, we find that the filter function is now
with and . The filter function Q(ω, τ) for this case is then N_{s} times the filter function for a single spinhalf particle with θ = 0 and ϕ = 0. In other words, Γ(τ) for N_{s} particles is simply N_{s} times the decay rate for a single particle. For illustration purposes, we have plotted Γ(τ) as a function of the measurement interval τ in Fig. 3(a) for N_{s} = 20 and a subOhmic environment. It should be noted that the amplification of Γ(τ) now makes the use of the correct filter function even more critical. For instance, for the population decay Hamiltonian in Fig. 3(a) with Δ = 2 and ε = 0, the survival probability after five measurements with time interval τ = 1 is approximately 0.02, while the survival probability for the more general Hamiltonian with Δ = 2 and ε = 2 after five measurements with the same time interval τ = 1 is ten times smaller.
Suppose now that we prepare the state of each twolevel system in a coherent superposition such that the total state is where . This time we obtain
with and . We again find that Γ(τ) for N_{s} particles coupled collectively to the environment is given by N_{s} times the decay rate for a single particle. Quantitative results are presented in Fig. 3(b) for N_{s} = 20 with a superOhmic environment (s = 1.5). Again, due to the amplification of the effective decay rate, it becomes very important to use the correct filter function.
Discussion
We have derived an expression for the effective decay rate of a quantum state in the presence of repeated measurements which is valid when the systemenvironment coupling is weak. This expression implies that the effective decay rate of the quantum state depends on the overlap of the spectral density of the environment and a generalized filter function. We have shown that our formalism for calculating the effective decay rate reproduces the wellknown results for the population decay model and the pure dephasing model. Thereafter, we demonstrated that our formalism allows us to study the Zeno and antiZeno effects for the spinboson model in a rigorous fashion under the assumption that the systemenvironment coupling strength is weak. We have found qualitative and quantitative differences in the behaviour of the decay rate as a function of the measurement interval when both decay and dephasing are present as compared to the relatively simpler population decay and pure dephasing models. Finally, by considering many twolevel systems coupled collectively to a common environment, we have observed that the decay rate is amplified depending on the number of twolevel systems. Consequently, it is even more crucial to use the correct filter function to evaluate the effective decay rate. We should also emphasize that our framework can be used to study other systemenvironment models as well. Experimental implementations of the ideas presented in this paper are expected to be important for measurementbased quantum control, as well as stimulating further work on the Quantum Zeno and antiZeno effects.
Methods
Derivation of the effective decay rate
The systemenvironment Hamiltonian is H = H_{S} + H_{B} + V, where we recall that H_{S} is the system Hamiltonian, H_{B} is the Hamiltonian of the environment and V describes the systemenvironment interaction. At time t = 0, we prepare the initial system state . To calculate the effective decay rate, we find the survival probability s(τ), provided that we start from the pure system state . In order to do so, let us first find an expression for ρ_{S}(τ), the state of the system at time t = τ, just before the system is measured. Now, the total systemenvironment state at this time is ρ_{tot}(τ) = U(τ)ρ_{tot}(0)U^{†}(τ), where U(τ) represents the unitary timeevolution due to the total systemenvironment Hamiltonian H. We can then find the state of the system at time τ as ρ_{S}(τ) = Tr_{B}{U(τ)ρ_{tot}(0)U^{†}(τ)}, where Tr_{B} denotes taking partial trace over the environment. Generally speaking, however, it is usually impossible to find U(τ) exactly. Instead, we resort to perturbation theory, which can be used if we assume that the systemenvironment interaction is weak. We write U(τ) as U(τ) = U_{0}(τ)U_{I}(τ), where is the ‘free’ unitary timeevolution operator and U_{I}(τ) can be expanded as a perturbation series, that is, U_{I}(τ) = 1 + A_{1} + A_{2} + …, where A_{1} and A_{2} are the first and second order corrections respectively. The system density matrix at time τ is then
correct to second order in the systemenvironment coupling strength.
To proceed further, we assume that the initial systemenvironment state can be represented as ρ_{tot} = ρ_{S}(0) ⊗ ρ_{B}, that is, the initial systemenvironment state is a simple product state. This is a rather standard assumption in the open quantum systems literature, but it should be noted that the validity of this assumption is questionable when the systemenvironment coupling strength is strong and/or the number of particles collectively coupled with the environment is large^{54,55,56}. Moreover, we also assume that we can write V = F ⊗ B, where F(B) is an operator belonging to the system (environment) Hilbert space. The more general case where V = ∑_{μ}F_{μ} ⊗ B_{μ} can be dealt with via a straightforward extension. The operators A_{1} and A_{2} introduced above are then found to be and , with , where and . We now simplify Eq. (8) term by term. First, we find that , where is the system density matrix if the system and environment are not coupled together. Next,
But , which is zero for the systemenvironment models usually considered^{45}. Similarly, . The next term is
with the environment correlation function C(t_{1}, t_{2}) defined as . Similarly,
Finally, . Using the fact that , we can manipulate further to obtain
where h.c. denotes hermitian conjugate. Putting all the terms back together, the system density matrix can be written as
We can simplify this further by noting that the environment correlation function generally depends on the time difference t_{1} − t_{2} only. This motivates us to introduce t′ = t_{1} − t_{2}. The system density matrix at time τ then becomes
with the simplified notation for the environment correlation function.
Once we have the expression for the density matrix at time τ, we can compute the survival probability. This survival probability can be simply calculated as one minus the probability of getting some result other than the state that we have started off with. Consequently, it is useful to define the projection operator that projects onto the subspace orthogonal to the state . Moreover, we must also keep in mind that, just before performing the measurement, we perform a unitary operator (which is implemented on a very short timescale) in order to remove the evolution due to the system Hamiltonian itself. This unitary operator then removes the U_{S}(τ) and that can be found to the left and right of the right hand side of Eq. (9). Thus, we can write the survival probability as
where Tr denotes simply taking the trace over the system only and we have used the fact that . Using the fact that for any operator X, Tr(X + X^{†}) = 2Re[Tr(X)], where Re denotes taking the real part, we further simplify to
and we have replaced t_{1} with t for notational simplicity. Since , we get
Now, the environment correlation function will typically be of the form , where g_{k} is the coupling strength of the system with mode k of the environment and f(ω_{k}, t′) is simply a function containing the remaining information about C(t′). This sum is usually replaced by an integral over the frequencies of the environment via the substitution , thereby introducing the spectral density J(ω) of the environment. Also, what we are really interested in is the effective decay rate . For weak coupling strength, the deviation of s(τ) from unity is small. Therefore, the effective decay rate can be approximated as , where
By introducing the spectral density, we can write instead , where the generalized ‘filter function’ Q(ω, τ) is
thereby ending up with Eq. (1). The approach given above can easily be generalized to a coupling of the form , leading to Eq. (3).
Finding the effective decay rate for the large spinboson model
We first consider the case where we repeatedly prepare the state given by . We begin by calculating . Using the standard commutation relations, [J_{k}, J_{l}] = iε_{klm}J_{m} and the BakerHausdorff lemma, we find that
with a_{x}(t), a_{y}(t) and a_{z}(t) as defined in Eq. (4). Now, , leading to
By observing that and simplifying, we find the filter function given in Eq. (6).
Let us now calculate the filter function for the case when we repeatedly prepare the state given by . To investigate the Zeno and antiZeno effects now, it is best to transform to a rotated frame, that is, we rotate both the systemenvironment Hamiltonian and the state that we are repeatedly preparing. In other words, we use the fact that
where the transformed Hamiltonian is
with ε_{r} = Δ and Δ_{r} = −ε. We then find that , with , and , where . The rest of the calculation proceeds in a very similar way to what we did with the state and leads to
with and . Now, it is easy to show that b_{x}(t) = a_{z}(t) and b_{y}(t) = −a_{y}(t). Thus, we obtain the filter function given in Eq. (7).
Additional Information
How to cite this article: Chaudhry, A. Z. A general framework for the Quantum Zeno and antiZeno effects. Sci. Rep. 6, 29497; doi: 10.1038/srep29497 (2016).
References
Misra, B. & Sudarshan, E. C. G. The Zeno’s paradox in quantum theory. J. Math. Phys. (NY) 18, 756–763 (1977).
Facchi, P., Gorini, V., Marmo, G., Pascazio, S. & Sudarshan, E. Quantum Zeno dynamics. Phys. Lett. A 275, 12–19 (2000).
Facchi, P. & Pascazio, S. Quantum Zeno subspaces. Phys. Rev. Lett. 89, 080401 (2002).
Facchi, P. & Pascazio, S. Quantum Zeno dynamics: mathematical and physical aspects. J. Phys. A: Math. Theor . 41, 493001 (2008).
Wang, X.B., You, J. Q. & Nori, F. Quantum entanglement via twoqubit quantum Zeno dynamics. Phys. Rev. A 77, 062339 (2008).
Maniscalco, S., Francica, F., Zaffino, R. L., Lo Gullo, N. & Plastina, F. Protecting entanglement via the quantum Zeno effect. Phys. Rev. Lett. 100, 090503 (2008).
Facchi, P. & Ligabò, M. Quantum Zeno effect and dynamics. J. Phys. A: Math. Theor . 51, 022103 (2010).
Militello, B., Scala, M. & Messina, A. Quantum Zeno subspaces induced by temperature. Phys. Rev. A 84, 022106 (2011).
Xu, D. Z., Ai, Q. & Sun, C. P. Dispersivecouplingbased quantum Zeno effect in a cavityQED system. Phys. Rev. A 83, 022107 (2011).
Zhang, Z.T. & Xue, Z.Y. Demonstration of quantum Zeno effect in a superconducting phase qubit. JETP Letters 93, 349–353 (2011).
Raimond, J. M. et al. Quantum Zeno dynamics of a field in a cavity. Phys. Rev. A 86, 032120 (2012).
Smerzi, A. Zeno dynamics, indistinguishability of state and entanglement. Phys. Rev. Lett. 109, 150410 (2012).
Wang, S.C., Li, Y., Wang, X.B. & Kwek, L. C. Operator quantum Zeno effect: Protecting quantum information with noisy twoqubit interactions. Phys. Rev. Lett. 110, 100505 (2013).
McCusker, K. T., Huang, Y.P., Kowligy, A. S. & Kumar, P. Experimental demonstration of interactionfree alloptical switching via the quantum Zeno effect. Phys. Rev. Lett. 110, 240403 (2013).
Stannigel, K. et al. Constrained dynamics via the Zeno effect in quantum simulation: Implementing nonabelian lattice gauge theories with cold atoms. Phys. Rev. Lett. 112, 120406 (2014).
Zhu, B. et al. Suppressing the loss of ultracold molecules via the continuous quantum Zeno effect. Phys. Rev. Lett. 112, 070404 (2014).
Schäfer, F. et al. Experimental realization of quantum Zeno dynamics. Nat. Commun. 5, 3194–3199 (2014).
Signoles, A. et al. Confined quantum Zeno dynamics of a watched atomic arrow. Nat. Phys . 10, 715–719 (2014).
Debierre, V., Goessens, I., Brainis, E. & Durt, T. Fermi’s golden rule beyond the Zeno regime. Phys. Rev. A 92, 023825 (2015).
Kiilerich, A. H. & Mølmer, K. Quantum Zeno effect in parameter estimation. Phys. Rev. A 92, 032124 (2015).
Qiu, J. et al. Quantum Zeno and Zenolike effects in nitrogen vacancy centers. Sci. Rep . 5, 17615 (2015).
Zhang, Y.R. & Fan, H. Zeno dynamics in quantum open systems. Sci. Rep . 5, 11509 (2015).
Slichter, D. H. et al. Quantum Zeno effect in the strong measurement regime of circuit quantum electrodynamics. New J. Phys. 18, 053031 (2016).
Kofman, A. G. & Kurizki, G. Acceleration of quantum decay processes by frequent observations. Nature (London) 405, 546–550 (2000).
Facchi, P., Nakazato, H. & Pascazio, S. From the Quantum Zeno to the Inverse Quantum Zeno Effect. Phys. Rev. Lett. 86, 2699 (2001).
Koshino, K. & Shimizu, A. Quantum Zeno effect by general measurements. Phys. Rep . 412, 191–275 (2005).
Cao, X., Ai, Q., Sun, C.P. & Nori, F. The transition from quantum Zeno to antiZeno effects for a qubit in a cavity by varying the cavity frequency. Phys. Lett. A 376, 349–357 (2012).
Chen, P.W., Tsai, D.B. & Bennett, P. Quantum Zeno and antiZeno effect of a nanomechanical resonator measured by a point contact. Phys. Rev. B 81, 115307 (2010).
Barone, A., Kurizki, G. & Kofman, A. G. Dynamical control of macroscopic quantum tunneling. Phys. Rev. Lett. 92, 200403 (2004).
Fujii, K. & Yamamoto, K. AntiZeno effect for quantum transport in disordered systems. Phys. Rev. A 82, 042109 (2010).
Fischer, M. C., GutiérrezMedina, B. & Raizen, M. G. Observation of the quantum Zeno and antiZeno effects in an unstable system. Phys. Rev. Lett. 87, 040402 (2001).
Maniscalco, S., Piilo, J. & Suominen, K.A. Zeno and antiZeno effects for quantum brownian motion. Phys. Rev. Lett. 97, 130402 (2006).
Segal, D. & Reichman, D. R. Zeno and antiZeno effects in spinbath models. Phys. Rev. A 76, 012109 (2007).
Zheng, H., Zhu, S. Y. & Zubairy, M. S. Quantum Zeno and antiZeno effects: Without the rotatingwave approximation. Phys. Rev. Lett. 101, 200404 (2008).
Ai, Q., Li, Y., Zheng, H. & Sun, C. P. Quantum antiZeno effect without rotating wave approximation. Phys. Rev. A 81, 042116 (2010).
Thilagam, A. ZenoantiZeno crossover dynamics in a spinboson system. J. Phys. A: Math. Theor . 43, 155301 (2010).
Thilagam, A. Nonmarkovianity during the quantum Zeno effect. J. Chem. Phys. 138, 175102 (2013).
Schlosshauer, M. Decoherence and the quantumtoclassical transition (Springer, Berlin, 2007).
Chaudhry, A. Z. & Gong, J. Zeno and antiZeno effects on dephasing. Phys. Rev. A 90, 012101 (2014).
Nokkala, J., Galve, F., Zambrini, R., Maniscalco, S. & Piilo, J. Complex quantum networks as structured environments: engineering and probing. Sci. Rep . 6, 26861 (2016).
Matsuzaki, Y., Saito, S., Kakuyanagi, K. & Semba, K. Quantum Zeno effect with a superconducting qubit. Phys. Rev. B 82, 180518 (2010).
Scully, M. O. & Zubairy, M. S. Quantum optics (Cambridge University Press, Cambridge, 1997).
Leggett, A. J. et al. Dynamics of the dissipative twostate system. Rev. Mod. Phys. 59, 1–85 (1987).
Weiss, U. Quantum dissipative systems (World Scientific, Singapore, 2008).
Breuer, H.P. & Petruccione, F. The Theory of Open Quantum Systems (Oxford University Press, Oxford, 2007).
Clarke, J. & Wilhelm, F. Superconducting quantum bits. Nature (London) 453, 1031–1042 (2008).
You, J. & Nori, F. Atomic physics and quantum optics using superconducting circuits. Nature (London) 474, 589–597 (2011).
Le Hur, K. Kondo resonance of a microwave photon. Phys. Rev. B 85, 140506 (2012).
Puri, R. R. Mathematical methods of quantum optics (Springer, Berlin, 2001).
Vorrath, T. & Brandes, T. Dynamics of a large spin with strong dissipation. Phys. Rev. Lett. 95, 070402 (2005).
BarGill, N., Rao, D. D. B. & Kurizki, G. Creating nonclassical states of boseeinstein condensates by dephasing collisions. Phys. Rev. Lett. 107, 010404 (2011).
Gross, C., Zibold, T., Nicklas, E., Estève, J. & Oberthaler, M. K. Nonlinear atom interferometer surpasses classical precision limit. Nature 464, 1165–1169 (2010).
Riedel, M. F. et al. Atomchipbased generation of entanglement for quantum metrology. Nature 464, 1170–1173 (2010).
Chaudhry, A. Z. & Gong, J. Amplification and suppression of systembathcorrelation effects in an open manybody system. Phys. Rev. A 87, 012129 (2013).
Chaudhry, A. Z. & Gong, J. Role of initial systemenvironment correlations: A master equation approach. Phys. Rev. A 88, 052107 (2013).
Chaudhry, A. Z. & Gong, J. The effect of state preparation in a manybody system. Can. J. Chem. 92, 119–127 (2014).
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Chaudhry, A. A general framework for the Quantum Zeno and antiZeno effects. Sci Rep 6, 29497 (2016). https://doi.org/10.1038/srep29497
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DOI: https://doi.org/10.1038/srep29497
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