Abstract
1. INTRODUCTION
Implementing a controllable and strong enough coupling to a quantum unit at a single-quanta level is a very desirable basic goal in quantum information processing (QIP) [1–8]. This type of strong coupling can first ensure complete and fast control of the qubits directly or indirectly at the single-quanta level [9,10], which also underlies applications of quantum simulation [11,12], manipulation [13,14], and metrology [15]. Second, such interactions can also be applied to explore many interesting and essential physics [16], such as single photon or phonon technology [17–19] and chiral quantum science [20–22].
Working as a point defect in diamond, the nitrogen-vacancy (NV) center integrated in a hybrid quantum system has recently emerged as one of the leading candidates for QIP. It is desirable thanks to its excellent spin properties [23–26], such as solid-state spins with atom-like properties and without an additional trap device [27,28], precise implantation and easy scalability [29,30], and longer coherence times even at ambient conditions [24,25,31], in addition to the convenient preparation, manipulation, and readout of its quantum state [32,33]. Significant theoretical and experimental investigations have been carried out using NV spins in hybrid systems to realize quantum simulation and quantum state manipulating [34–41]. In recent years, more and more attention has been devoted to the application of NV centers in the quantum acoustics area, which also leads to a growing interest in studying and exploiting coherent spin–phonon coupling [2,42,43]. However, it is still a huge challenge to significantly enhance the spin–phonon coupling at a single-quanta level by the means currently available [32].
In this work, we present a combined scheme to enhance the spin–phonon coupling in a hybrid setup, which consists of a single NV spin and three optical cavities dispersively coupled with three mechanical resonators (MRs) [44]. To further enhance the spin–phonon coupling in this spin–cavity–resonator tripartite system, there are two key points in our proposal. First, we can modify the spatial distribution of the electric field in the cavity through mechanical displacement, which is named as the mode field coupling (MFC) [45]. Importantly, the spin–phonon interaction can be controlled and enhanced by the optical field intensity with the rate , resulting in optically controlled spin–phonon coherent manipulation. Meanwhile, we apply the mechanical parametric amplification (MPA) to the MR by modulating its spring constant in time [32,46–56]. In the squeezed frame, we can further enhance the spin–phonon coupling with an exponential rate in this tripartite system [32,57]. By taking advantage of the joint assistance of MFC and MPA, we have achieved the goal to further strengthen the coherent spin–phonon coupling at a single-quanta level, compared to the previous investigations of this issue. In addition, we also have discussed several potential applications based on this tripartite interaction system. We believe that this scheme may provide a promising phonon-mediated platform to implement more active control of NV spins.
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2. MFC AND MPA
A. MFC
In a traditional cavity quantum electrodynamics (C-QED) system, the realistic dipole coupling to a single quantum emitter (QE) can be written as , with the emitter’s transition dipole moment and the electric field . We note that its coupling strength is determined through a given electric field at the certain position , and it is impossible to obtain a controllable or enhanced QE–photon coherent coupling in such a system. The MFC can help us to deal with this problem, and its core concept originates from the so-called optomechanical system [44], which indicates that the resonator’s displacement will also affect the cavity frequency with the dispersive coupling . Here, we state and are, respectively, the zero-point fluctuation and phonon annihilation operator. In addition, we take advantage of the basic idea of the ion trap system, and then we may establish a triple QE–photon–phonon coupled system (namely MFC) that uses the so-called sideband engineering. Importantly, this design will offer a mechanics-induced variation of the spatial distribution of the target cavity field. Going in this direction, we can obtain a mechanic mode-dependent QE-cavity coupling even at the given position and electric field. As a direct consequence, the relevant coupling strength of the QE to cavity mode can be expressed as , where the MFC coupling is defined as . With an assumed special condition , we can then get this triple interaction as . When we generally make a classical assumption of this cavity mode with , we can obtain an enhanced QE-phonon coupling , which results in the MFC-assisted enhancement of the QE-phonon interaction. With the continuous development of the optomechanical technology and applications [58], we have no doubt about the feasibility of this physical mechanism in the future.
We stress that this type of MFC coupling mechanism may be a general proposal, and we can demonstrate it in the traditional optomechanical system and also can introduce it to other optomechanics-like systems; the photon–magnon (lattice) system and the photon–phonon (lattice) system, for example.
B. MPA
Parametric amplification [including optical parametric amplification (OPA) and MPA] has been another hot topic related to the enhancement of coherent coupling since it was first proposed in an optomechanical system. In particular, a milestone achievement on this topic has also been reported and demonstrated in a hybrid ion trap system. This type of progress reinforces our confidence in the feasibility of the OPA or MPA, and we believe that in this work MPA will be a more feasible choice to further enhance the coherent coupling to a single QE. To realize MPA, the core point lies in the modulation of the time-dependent spring constant [32,50]; i.e., . Therefore, the Hamiltonian of the mechanical resonator is , and its quantized expression is . Then, we can transform this mechanical mode into the Bogoliubov mode ( with the squeezing parameter ) and diagonalize this Hamiltonian in a squeezed frame. Next, we can get an exponentially enhanced coupling strength with the expression .
In short, we believe that the MFC and MPA are both general physical ideas, and that this proposal can first show a joint cooperation of the MFC and MPA via a hybrid design to further enhance the EQ–phonon coupling. To induce this joint enhancement effect of the spin–phonon coupling to a feasible hybrid quantum system, we believe that optomechanics [44,58] or an optomechanics-like system will be a suitable choice; for example, the lattice of a photon–phonon coupling system or a hybrid optics–acoustics system [35,59–67]. Here, let’s consider the traditional optomechanical system and then discuss this joint scheme in detail.
3. POTENTIAL SCHEME FOR THE JOINT MFC AND MPA
We have designed this hybrid setup, as illustrated in Fig. 1(a), with three identical optical cavities with frequency arranged one by one, and these optical modes are named, respectively, modes , , and . The central cavity is symmetrically connected to the two bilateral cavities with identical optical fibers. Thus, through the exchange–photon process, the central cavity mode will interact with the two bilateral cavities with the same coupling rate . Each cavity also dispersively couples to an identical MR with the same coupling rate . For these three identical MRs, the fundamental frequencies are all , and these mechanical modes are correspondingly named , , and . Moreover, we add an additional second-order nonlinear pump on each resonator, which can be implemented easily through modulation of the mechanical spring constant in time. The central MR additionally couples to the other two bilateral MRs and with the same coupling rate . The coupling between the two mechanical modes can actually be realized by the Coulomb interaction between the charged mechanical media [69,70].
Figure 1.Schematic of our hybrid system. (a) Three identical optical cavities with frequency
In addition, as illustrated in Fig. 1(a), a single NV center is placed inside the central cavity. In the optical frequency domain, the optical mode will induce the NV spin’s quantum transition between the excited state and the ground state with a coupling rate . The energy level structure of a single NV center is shown in Fig. 1(b). The ground state and the excited state are denoted as and , and the optical transition frequency between them is . For a single NV center, this two-level system can be considered as a spin-1/2 particle with Pauli matrix definitions , , and .
Therefore, according to the Appendices A–C, we can get the total Hamiltonian to describe this hybrid system by
In Eq. (1), under the rotating frame with frequency , the first item is the Hamiltonian to describe these three MRs with the second-order nonlinear interaction, including their pairwise interactions between the central mode and the bilateral modes . The second item describes the NV spin and optical cavities, with the spin–cavity interaction and the pairwise interactions between the central mode and the bilateral modes . The last item means the Hamiltonian to describe the dispersive interactions between the cavities and the corresponding mechanical resonators.
According to Appendix D, we can simplify the total Hamiltonian for this system, and obtain an effective Hamiltonian with the tripartite interactions (spin–photon–phonon):
In view of this Hamiltonian in the squeezed frame, its effective triple coupling strength is strengthened with the rate via the MPA process. We also believe this type of enhanced three-body interaction is very important and interesting, especially for the application of QIP, quantum simulation, and quantum manipulation [71–76].
4. ENHANCING THE SPIN–PHONON COUPLING
We consider that the cavity is pumped with a large coherent field with an average photon number . Therefore, we can write the cavity field as . Neglecting the quantum fluctuations (valid for ), we can acquire the effective Rabi type Hamiltonian
Next, in the interaction picture (IP), we transfer Eq. (3) into an equivalent expression with the relations and (the red sideband detuning), by discarding the high frequency oscillation terms:
Whether it is a J–C model or an anti J–C model, we can get an enhanced coupling strength with the effective coupling strength
To enhance the coherent coupling between the NV spin and supermode , the cooperation of the MFC and MFA is superior to the MFC. This is due to the fact that is limited to the driving power , which can not be increased arbitrarily in a real experiment. For a single NV center, we can achieve a traditional weak spin–phonon coupling at single quantum level with the strength . To quantify the enhancement of the spin–phonon coupling, we exploit the cooperativity . Here, and correspond, respectively, to the effective mechanical dissipation rates and the decay rate of the spin. Note that in presence of the mechanical amplification, the noise coming from the mechanical bath is also amplified. To circumvent this detrimental effect, a possible strategy is to use the dissipative squeezing approach to keep the mechanical mode in its ground state in the squeezed frame [49,51,77,78]. This steady-state technique has already been implemented experimentally [79]. In this case, we can obtain the engineered effective dissipation rate in the squeezed frame. Therefore, we can also define the effective cooperativity .
In Fig. 2, we plot the spin–phonon coupling enhancement and the cooperativity enhancement , versus the squeezing parameter and photon number of the classical driven field on the mode . Increasing the squeezing parameter and the photon number , one can achieve a distinct enhancement in the spin–phonon coupling, thus directly giving rise to the cooperativity enhancement.
Figure 2.(a) Spin–phonon coupling enhancement
Furthermore, in Fig. 3, we also plot the dynamical population of the phonon number operator and the spin operator according to the J–C model [in Eq. (4)] and the anti J-C model [in Eq. (5)], with the different parameters, such as and . The numerical results above show the distinct quantum dynamics of this spin–phonon system for different cases, in which the spring constant is modulated or not, and is increased from to . Therefore, with the joint assistance of the mechanical squeezing (with parameter ) and the classical driving of the mode (with intensity ), the system can be pumped and driven from the weak-coupling regime to the strong-coupling regime, or even to the ultrastrong-coupling regime.
Figure 3.Dynamical population of the phonon number
5. ENHANCEMENT OF PHOTON–SPIN–PHONON INTERACTION
On the other hand, if is too weak, the quantum fluctuation will dominate the supermode . As a result, we can get the effective tripartite interaction Hamiltonian from Eq. (2) with two different kinds of expression in IP. For the first condition, such as the blue sideband, when the resonance condition satisfies , we can also discard the high frequency oscillation terms, and get the blue sideband effective three-quantum-system Hamiltonian,
For the second case, such as the red sideband, when the resonance condition satisfies , discarding the high frequency oscillation terms, we can get
In this tripartite interaction quantum system, the effective coupling strength is
In Fig. 4, we make the simulations on this tripartite interaction system according to Eq. (7) and Eq. (8), and then plot the dynamical population of the phonon number operator , the photon number operator , and the spin operator with the different squeezing parameter . The numerical results above evidently show that we can strengthen this tripartite interaction by increasing the squeezing parameter .
Figure 4.(a), (b) Dynamical population of the spin operator
6. APPLICATION OF THIS PROPOSAL
A. Entangling Collective NV Spins Dynamically
In this section, the first potential application for this proposal is that we can entangle separated NV spins. We assume a certain number of NV spins are set separately in this central optical cavity. According to Eq. (3), we can obtain the effective Hamiltonian as
Here, we assume , and the effective coupling to the th NV spin is . We stress that this inhomogeneous coupling strength is mainly caused by the differences in the location of NV spins in the cavity, which maps to the factors and . In this scheme, one can reduce this system disorder through implanting NV spins precisely with the advanced processing techniques. By discarding this weak adverse effect, we can rewrite the effective Hamiltonian in the interaction picture (IP) as
Here, the coupling is identical ; therefore, we can use the collective spin operator in the equation above with the definition . We note that this type interaction corresponds to the so-called Mølmer–Sørensen (MS) gate [80,81], which is used to generate the multiparticle entanglement. Its system dynamics is governed by the unitary evolution operator . Taking advantage of the Magnus formula [82], we get when for the integer number . This means that the mechanical mode is decoupled from the NV spins at this moment.
Note that because this operator has no contribution from the mechanical modes, in this instance the system gets insensitive to the states of the mechanical modes. Starting from the initial state of the mechanical mode and NV spins , we can obtain the target entangled state of the collective NV spins with the form , which is the well-known Greenberger–Horne–Zeilinger (GHZ) type state with the number of the spins. Next we plot the numerical simulation result shown in Fig. 5. As illustrated in Fig. 5, taking a realistic condition such as the NV decay rate and the mechanical dissipation into consideration, we can quickly entangle NV spins with a high fidelity of more than 0.98 in this scheme.
Figure 5.Dynamical fidelity of the target entangled GHZ state for four NV spins, in which, the initial state is
B. Local Cooling One Supermode of Triple Resonators with an NV Ensemble
On the other hand, we stress that another potential application on this scheme is to cool down the mechanical supermode to its ground state efficiently with the NV center ensemble (NVE). Here, we assume a number of NV centers are set inside the central optical cavity, which form an NVE. Taking the Eqs. (4) and (10) into consideration, we can obtain the effective Hamiltonian in IP for this hybrid system:
Similarly, we can also ignore this weak system disorder adverse effect according to the advanced processing techniques. Then, we can rewrite this effective Hamiltonian as
Figure 6.Dynamical population of this mechanical supermode
Figure 7.Dynamical evolution of the mechanical population of the left local mode
7. EXPERIMENTAL PARAMETERS
To examine the feasibility of our scheme in a realistic experiment, we now discuss the relevant experimental parameters. We consider a high-quality optical cavity with frequency and , and can assume its coupling strength to a single NV center can reach [83–89]. For the MR with a frequency and , the optic-mechanic coupling to the cavity mode will be [44]. For a single NV center, the lifetime of its excited state is about 10 ns, so the spontaneous decay rate of its excited state is about [90–92]. Considering the dynamical process for entangling the NV spins in this work, we can obtain the GHZ state at the time of . Compared to this time interval, we think its coherence time is enough to implement this scheme.
8. CONCLUSION
In summary, we propose a protocol to further enhance the spin–phonon coupling at the single-quanta level with two methods jointly working together: the MFC and MPA. Importantly, in our scheme, we can enhance the coherent spin–phonon interaction not only by the optical field intensity with rate , but also by the amplified zero-field fluctuation of the mechanical mode with rate . In other words, taking advantage of the joint assistance of both amplifications means we can realize the goal to further strengthen the coherent spin–phonon coupling at a single-quanta level in this hybrid system. In addition, we also have to briefly discuss the potential applications of this tripartite interaction system. We believe that this investigation may provide a more promising direction to implement active control of the spin–phonon coupling at a single quanta-level.
Acknowledgment
Acknowledgment. Yuan Zhou thanks Peng-Bo Li for valuable discussions. Part of the simulations are coded in Python using the QuTiP library [93,94].
APPENDIX A: THE HAMILTONIAN OF MECHANICAL MODES WITH SECOND-ORDER NONLINEAR INTERACTION
The Hamiltonian for the th mechanical system with a modulated spring constant can be expressed as
Here, we assume that these are three identical MRs, with an intrinsic frequency , the time-dependent spring constant , and the nonlinear coefficient . Using the frame rotating with frequency and dropping the terms () that explicitly oscillate in time, then we can acquire the Hamiltonian with a second-order nonlinear interaction for the th mechanical resonator
Furthermore, in this scheme, the central mechanical mode also interacts with two other bilateral mechanical modes and . Assuming the identical coupling strength is , we can obtain their Hamiltonian as
In this scheme, the coefficient of this nonlinear interaction item is tunable using the high precision electromagnetic technology, and the coupling strength between the mechanical modes can also be modulated via some electrical means, such as the capacitor method.
APPENDIX B: THE HAMILTONIAN OF SPIN–CAVITY AND CAVITY–CAVITY INTERACTIONS
As illustrated in Fig.
APPENDIX C: THE INTERACTIONS BETWEEN THE MECHANICAL MODES AND CAVITY MODES
In this scheme, the three cavity modes will also interact with the three mechanical modes . By setting the same coupling strength as for simplicity and under the frame rotation with frequency , we can express this type interaction with the Hamiltonian form,
APPENDIX D: THE EFFECTIVE HAMILTONIAN DERIVATION FOR THIS WHOLE SYSTEM
Considering the Hamiltonian in Eq. (
Here, the relevant coefficients are defined, respectively, as
The mechanical part of this Hamiltonian can also be diagonalized by the canonical transformation
Applying a unitary transformation with the definition to the Hamiltonian , we can obtain
Then, we can also diagonalize the cavity-mode part in the Hamiltonian by introducing another canonical transformation
When the spectral separation between the supermodes is much larger than the mechanical frequency (), we can neglect the effect of the terms of supermodes and get the effective Hamiltonian by using the approximate relation so
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