Skip to main content

Thank you for visiting You are using a browser version with limited support for CSS. To obtain the best experience, we recommend you use a more up to date browser (or turn off compatibility mode in Internet Explorer). In the meantime, to ensure continued support, we are displaying the site without styles and JavaScript.

Strong indirect coupling between graphene-based mechanical resonators via a phonon cavity

An Author Correction to this article was published on 19 March 2019

This article has been updated


Mechanical resonators are promising systems for storing and manipulating information. To transfer information between mechanical modes, either direct coupling or an interface between these modes is needed. In previous works, strong coupling between different modes in a single mechanical resonator and direct interaction between neighboring mechanical resonators have been demonstrated. However, coupling between distant mechanical resonators, which is a crucial request for long-distance classical and quantum information processing using mechanical devices, remains an experimental challenge. Here, we report the experimental observation of strong indirect coupling between separated mechanical resonators in a graphene-based electromechanical system. The coupling is mediated by a far-off-resonant phonon cavity through virtual excitations via a Raman-like process. By controlling the resonant frequency of the phonon cavity, the indirect coupling can be tuned in a wide range. Our results may lead to the development of gate-controlled all-mechanical devices and open up the possibility of long-distance quantum mechanical experiments.


The rapid development of nanofabrication technology enables the storage and manipulation of phonon states in micro- and nano-mechanical resonators1,2,3,4,5. Mechanical resonators with quality factors6 exceeding 5 million and frequencies7,8 in the sub-gigahertz range have been reported. These advances have paved the route to controllable mechanical devices with ultralong memory time9. To transfer information between different mechanical modes, tunable interactions between these modes are required10. While different modes in a single mechanical resonator can be coupled by parametric pump3,4,11,12,13,14,15,16 and neighboring mechanical resonators can be coupled via phonon processes through the substrate2 or direct contact interaction17, it is challenging to directly couple distant mechanical resonators.

Here, we observe strong effective coupling between mechanical resonators separated at a distance via a phonon cavity that is significantly detuned from these two resonator modes. The coupling is generated via a Raman-like process through virtual excitations in the phonon cavity and is tunable by varying the frequency of the phonon cavity. Typically, a Raman process can be realized in an atom with three energy levels in the Λ form18,19. The two lower energy levels are each coupled to the third energy level via an optical field with detunings. When these two detunings are tuned to be equal to each other, an effective coupling is formed between the lower two levels. To our knowledge, tunable indirect coupling in electro-mechanical systems has not been demonstrated before. The physical mechanism of this coupling is analogous to the coupling between distant qubits in circuit quantum electrodynamics20,21, where the interaction between qubits is induced by virtual photon exchange via a superconducting microwave resonator.


Sample characterization

The sample structure is shown in Fig. 1a, where a graphene ribbon22,23 with a width of ~1 μm and ~5 layers is suspended over three trenches (2 μm in width, 150 nm in depth) between four metal (Ti/Au) electrodes. This configuration defines three distinct electromechanical resonators: R1, R2 and R3. The metallic contacts S and D3 are each 2 μm wide and D1 and D2 are each 1.5 μm wide, which leads to a 7-μm separation between the centers of R1 and R3 (see Supplementary Methods and Supplementary Fig. 1). All measurements are performed in a dilution refrigerator at a base temperature of approximately 10 mK and at pressures below 10−7 torr. The suspended resonators are biased by a dc gate voltage (\(V_{{\rm g}i}^{{\mathrm{DC}}}\) for the ith resonator) and actuated by an ac voltage (\(V_{{\rm g}i}^{{\mathrm{AC}}}\) for the ith resonator with driving frequency fgi = ωd/2π) through electrodes (gi for the ith resonator) underneath the respective resonators. To characterize the spectroscopic properties of the resonators, a driving tone is applied to one or more of the bottom gates with frequency ωd, and another microwave tone with frequency ωd + δω is applied to the contact S. A mixing current (Imix = Ix + jIy) can then be obtained at D3 (D1 and D2 are floated during all measurements) by detecting the δω signal with a lock-in amplifier fixed at zero phase during all measurements (see Supplementary Methods and Supplementary Fig. 2).

Fig. 1

Sample structure and device characterization. a Scanning electron microscope photograph of a typical sample. An ~1-μm-wide graphene ribbon was suspended over four contacts, labeled as S, D1, D2, and D3, respectively. These contacts divide the ribbon into three sections, each with a gate of ~150 nm beneath the ribbon. A driving microwave with frequency ωd + δω is applied to contact S and is detected at contact D3 after mixing with another driving tone with frequency ωd applied to one or more of the control gates. Scale bar is 1 μm. b The differentiation of the mixed current dIx/dωd as a function of driving frequency ωd and gate voltage \(V_{{\mathrm{g}}3}^{{\mathrm{DC}}}\) with \(V_{{\mathrm{g}}1}^{{\mathrm{DC}}} = V_{{\mathrm{g}}2}^{{\mathrm{DC}}} = 0\) V. Here, the frequencies of all resonators can be tuned from several tens of MHz to ~100 MHz by adjusting the dc gate voltages. c The mixing current as a function of the driving frequency ωd at voltage \(V_{{\mathrm{g}}3}^{{\mathrm{DC}}} = 10\,{\mathrm{V}}\). Using a fitting process (see Supplementary Fig. 8), we extract the linewidth of the mechanical mode. The data were obtained at a driving power of −5 dBm. d, e Spectra of coupled modes R1 and R2 (d, where \(V_{{\mathrm{g}}1}^{{\mathrm{DC}}} = 10.5\) V and \(V_{{\mathrm{g}}3}^{{\mathrm{DC}}} = 0\) V) and R2 and R3 (e, where \(V_{{\mathrm{g}}1}^{{\mathrm{DC}}} = 0\) V and \(V_{{\mathrm{g}}3}^{{\mathrm{DC}}} = 10.5\) V). Strong couplings between these modes are manifested as avoided level crossings in the plots. Coupling strengths Ω12/2π ~ 240 kHz and Ω23/2π ~ 200 kHz are extracted from the plots. f The spectrum of R2 coupled to both R1 and R3. In this case, the gate voltages \(V_{{\mathrm{g}}1}^{{\mathrm{DC}}} = 10.45\) V and \(V_{{\mathrm{g}}3}^{{\mathrm{DC}}} = 8.35\) V are fixed

Figure 1b shows the measured mixing current as a function of the dc gate voltage and the ac driving frequency on R3, where the oblique lines represent the resonant frequencies of the resonator modes. We denote the resonant frequency of the ith resonator as fmi = ωmi/2π. This plot shows that \({\rm d}f_{{\mathrm{m}}3}{\mathrm{/}}{\rm d}V_{{\mathrm{g}}3}^{{\mathrm{DC}}} \sim 7.7\,{\mathrm{MHz/V}}\) when \(|V_{{\mathrm{g}}3}^{{\mathrm{DC}}}| > 5\,{\mathrm{V}}\). The frequencies of the resonators can hence be tuned in a wide range (see Supplementary Note 1 and Supplementary Fig. 3 for results of R1 and R2), which allows us to adjust the mechanical modes to be on or off resonance with each other. The quality factors (Q) of the resonant modes are determined by fitting the measured spectral widths (see Supplementary Fig. 8) at low driving powers (typically −50 dBm). Figure 1c shows the spectral dependence of R3, which gives a linewidth of γ3/2π ~ 28 kHz at a resonant frequency of fm3 ~ 98.05 MHz. The resulting quality factor is Q ~ 3500. The quality factors of the other two resonators are similar, at ~3000.

Strong coupling between neighboring resonators

Neighboring resonators in this system couple strongly with each other, similar to previous studies on gallium arsenide2 and carbon nanotube17. Figure 1d, e shows the spectra of the coupled modes (R1, R2) and (R2, R3), respectively, by plotting the mixed current Ix as a function of gate voltages and driving frequencies. In Fig. 1e, the voltage \(V_{{\mathrm{g}}3}^{{\mathrm{DC}}}\) is fixed at 10.5 V, with a corresponding resonant frequency fm3 = 101.15 MHz, and \(V_{{\mathrm{g}}2}^{{\mathrm{DC}}}\) is scanned over a range with fm2 being near-resonant to fm3. A distinct avoided level crossing appears when fm2 approaches fm3, which is a central feature of two resonators with direct coupling. From the measured data, we extract the coupling rate between these two modes as Ω23/2π ~ 200 kHz, which is the energy splitting when fm2 = fm3. In Supplementary Note 2 and Supplementary Fig. 4, we fit the measured spectrum with a single two-mode model using this coupling rate. Similarly in Fig. 1d, by fixing \(V_{{\mathrm{g}}1}^{{\mathrm{DC}}}\) at 10.5 V and scanning the voltage \(V_{{\mathrm{g}}2}^{{\mathrm{DC}}}\), we obtain the coupling rate between R1 and R2 as Ω12/2π ~ 240 kHz. There are several possible origins for the coupling between two adjacent resonators in this system. One coupling medium is the substrate and the other medium is the graphene ribbon itself. Mechanical energy can be transferred in a solid-state material by phonon propagation, as demonstrated in several experiments2,17,24. Second, because adjacent resonators share lattice bonds, the phonon energy can transfer in the graphene ribbon. The dependence of the coupling strength on the width of the drain contacts is still unknown (see Supplementary Fig. 5 for another sample).

The measured coupling strength satisfies the strong coupling condition with \({\rm{\Omega }}_{23} \gg \gamma _2,\gamma _3\). Defining the cooperativity for this phonon–phonon coupling system as \(C = {\rm{\Omega}}_{23}^2/\gamma _2\gamma _3\), we find that C = 44. A similar strong coupling condition can be found between modes R1 and R2. By adjusting the gate voltages of these three resonators, R2 can be successively coupled to both R1 and R3 (see Fig. 1f).

For comparison, we study the coupling strength between modes R1 and R3. The frequency fm2 of resonator R2 is set to be detuned from fm1 and fm3 by 700 kHz in Fig. 2a. In the dashed circle, we observe a near-perfect level crossing when fm1 approaches fm3, which indicates a negligible coupling between these two modes, with \({\rm{\Omega }}_{13} \ll \gamma _1,\gamma _3\) (also see Supplementary Fig. 6).

Fig. 2

Hybridization between all three modes. a Measured spectrum of the three-mode system when the frequency of R2 is far off-resonance from that of mode R1 by a detuning Δ12/2π ~ 70 kHz (here, \(V_{{\mathrm{g}}1}^{{\mathrm{DC}}} = 10.5\) V and \(V_{{\mathrm{g}}2}^{{\mathrm{DC}}} = 7.64\) V). The dc voltage \(V_{{\mathrm{g}}3}^{{\mathrm{DC}}}\) is scanned over a wide range, crossing both fm1 and fm2. An avoided level crossing is observed when fm3 approaches fm2. A level crossing is observed when fm3 approaches fm1. b Measured spectrum of the three-mode system when the detuning is Δ12/2π ~ 180 kHz (here, \(V_{{\mathrm{g}}1}^{{\mathrm{DC}}} = 10.5\) V and \(V_{{\mathrm{g}}2}^{{\mathrm{DC}}} = 7.56\) V, and here the ranges of the axes are set to be the same as the black dashed box shown in a). Here, a strongly avoided level crossing appears when fm3 approaches fm1. The strengths of the direct couplings extracted from the measured spectrum are Ω12/2π = 240 kHz and Ω23/2π = 170 kHz. c, d Spectra calculated using the theoretical model for the three modes (Eq. (2)) and coupling constants Ω12 and Ω23. Δ12/2π = 700 kHz in c and Δ12/2π = 180 kHz in d

Raman-like coupling between well-separated resonators

The three resonator modes in our system are in the classical regime. The Hamiltonian of these three classical resonators can be written as:

$${\cal H}_{c} = \mathop {\sum }\limits_i^3 \frac{1}{2}(p_i^2 + \omega _{{\rm m}i}^2x_i^2) + {\mathrm{\Lambda }}_{12}x_1x_2 + {\mathrm{\Lambda }}_{23}x_2x_3,$$

where \({\mathrm{\Lambda }}_{ij} = {\rm{\Omega }}_{ij}\sqrt {\omega _{{\rm m}i}\omega _{{\rm m}j}}\) is a coupling parameter between i- and jth resonators, ppi is the effective momentum and xi is the effective coordinate of the oscillation for the ith resonator, respectively. Let \(x_i = \sqrt {\frac{1}{{2\omega _{{\rm m}i}}}} (\alpha _i^ \ast + \alpha _i)\) and \(p_i = {\mathrm{i}}\sqrt {\frac{{\omega _{{\rm m}i}}}{2}} (\alpha _i^ \ast - \alpha _i)\), with αi and \(\alpha _i^ \ast\) being complex numbers. The Hamiltonian in Eq. (1) can be written as

$${\cal H}_t = {\sum} {\omega _{{\rm m}i}\alpha _i^ \ast \alpha _i + \frac{{{\rm{\Omega }}_{12}}}{2}\left( {\alpha _1^ \ast \alpha _2 + \alpha _1\alpha _2^ \ast } \right) + \frac{{{\rm{\Omega }}_{23}}}{2}\left( {\alpha _2^ \ast \alpha _3 + \alpha _2\alpha _3^ \ast } \right)} .$$

Here, we have applied the rotating-wave approximation and neglected the \(\alpha _i\alpha _j\) and \(\alpha _i^ \ast \alpha _j^ \ast\) terms. This approximation is valid when \(\omega _{{\rm m}i} \gg {\rm{\Omega }}_{12},{\rm{\Omega }}_{23}\). This Hamiltonian describes the direct couplings between neighboring resonators (R1, R2) and (R2, R3). Through these couplings, the mechanical modes hybridize into three normal modes, and an effective coupling between modes R1 and R3 can be achieved. If the resonators work in the quantum regime, \(\alpha _i\) and \(\alpha _i^ \ast\) can be quantized into the annihilation and creation operators of a quantum harmonic oscillator, respectively.

We study the hybridization of this three-mode system by fixing the gate voltages (mode frequencies) of modes R1 and R2, and sweeping the gate voltage of R3 over a wide range. The spectrum of this system depends strongly on the detuning between modes R1 and R2, which is defined as Δ12 = 2π(fm2fm1). In Fig. 2a, Δ12/2π ~ 70 kHz. Similar to Fig. 1f, modes R3 and R1 show a level crossing. Moreover, we observe a large avoided level crossing between modes R2 and R3 when the frequency fm3 approaches fm2, indicating strong coupling between these two modes. Hence, even with strong couplings between all neighboring resonators, the effective coupling between the distant modes R1 and R3 is still negligible when the frequency of mode R2 is significantly far off resonance from the other two modes. On the contrary, when the detuning Δ12/2π is lowered to ~180 kHz, a distinct avoided level crossing between modes R1 and R3 is observed, as shown inside the dashed circle in Fig. 2b.

With coupling strengths Ω12/2π = 240 kHz and Ω23/2π = 170 kHz extracted from the measured data, we plot the theoretical spectra of the normal modes in this three-mode system given by Eq. (2), for Δ12/2π = 700 and 180 kHz in Fig. 2c, d, respectively. Our result shows good agreement between theoretical and experimental results.

With direct couplings between neighboring resonators, an effective coupling between the two distant resonators R1 and R3 can be obtained via their couplings to mode R2. The effective coupling can be viewed as a Raman process, as illustrated in Fig. 3a. Here mode R2 functions as a phonon cavity that connects the mechanical resonators R1 and R3 via virtual phonon excitations. The physical mechanism of this effective coupling is similar to that of the coupling between distant superconducting qubits via a superconducting microwave cavity20. The detuning between the phonon cavity and the other two modes Δ12 can be used as a control parameter to adjust this effective coupling.

Fig. 3

Indirect coupling between separated resonators via a phonon cavity. a Raman-like coupling between modes R1 and R3 via virtual excitation of the phonon cavity R2. The coupling strength can be controlled by changing the detuning Δ12. b Effective coupling as a function of Δ12. The error bars are obtained from the s. e. m. of the measured data and are extracted from the statistical deviation of the estimated values at different detunings from Supplementary Fig. 7. The red line is given by Ω13 = Ω12Ω23/2Δ12, with Ω12/2π = 240 kHz and Ω23/2π = 170 kHz

To derive the effective coupling, we consider the case of Δ12 = Δ32 = Δ, where Δ32/2π = fm2fm3 and \(\left| {\rm{\Delta }} \right| \gg {\rm{\Omega }}_{12},\,{\rm{\Omega }}_{23}\). The avoided level crossing between modes R1 and R3 can be extracted at this point. Using a perturbation theory approach, we obtain the effective Hamiltonian between modes R1 and R3 as (see Methods for details)

$${\cal H}_{{\mathrm{eff}}} = (\Delta + \frac{{{\rm{\Omega }}_{12}^2}}{{4\Delta }})\alpha _1^ \ast \alpha _1 + (\Delta + \frac{{{\rm{\Omega }}_{23}^2}}{{4\Delta }})\alpha _3^ \ast \alpha _3 + \frac{{{\rm{\Omega }}_{13}}}{2}(\alpha _1^ \ast \alpha _3 + \alpha _3^ \ast \alpha _1).$$

Here, an effective coupling is generated between R1 and R3 with magnitude Ω13 = Ω12Ω23/2Δ, and the resonant frequencies of each mode are shifted by a small term. The effective coupling Ω13 in the Hamiltonian depends strongly on the detuning Δ. Thus, the effective coupling between R1 and R3 can be controlled over a wide range by varying the frequency (gate voltage) of resonator R2.

The effective coupling strength Ω13 between R1 and R3 as a function of Δ12 is shown in Fig. 3b. Each data point is obtained by changing the gate voltage of R2 and repeating the measurements in Fig. 2a, b (see Supplementary Fig. 7). Over a large range of detuning, the effective coupling is larger than the linewidths of the resonators γ1,2,3/2π, with Ω13 > 30 kHz. The red line shows the results using perturbation theory. The experimental data indicate good agreement with the theoretical results.


In summary, we have demonstrated indirect coupling between separated mechanical resonators in a three-mode electromechanical system constructed from a graphene ribbon. Our study suggests that coupling between well-separated mechanical modes can be created and manipulated via a phonon cavity. These observations hold promise for a wide range of applications in phonon state storage, transmission, and transformation. In the current experiment, the sample works in an environment subjected to noise and microwave heating with typical temperatures as high as 100 mK and phonon numbers reaching ~24. By cooling the mechanical resonators to lower temperatures25,26,27,28, quantum states could be manipulated via this indirect coupling29,30. Furthermore, in the quantum limit, by coupling the mechanical modes to solid-state qubits, such as quantum-dots and superconducting qubits17,31,32, this system can be utilized as a quantum data bus to transfer information between qubits33,34. Future work may lead to the development of graphene-based mechanical resonator arrays as phononic waveguides24 and quantum memories35 with high tunabilities.


Theory of three-mode coupling

We describe this three-mode system with the Hamiltonian (ħ = 1)

$${\cal H}_{\mathrm{t}} = {\sum} {\omega _{mi}\alpha _i^ \ast \alpha _i + \frac{{{\rm{\Omega }}_{12}}}{2}(\alpha _1^ \ast \alpha _2 + \alpha _1\alpha _2^ \ast ) + \frac{{{\rm{\Omega }}_{23}}}{2}(\alpha _2^ \ast \alpha _3 + \alpha _2\alpha _3^ \ast )} ,$$

where \({\rm{\Omega }}_{ij}\) is the coupling between mechanical resonators i and j. The couplings between the resonators induce hybridization of the three modes. The hybridized normal modes under this Hamiltonian can be obtained by solving the eigenvalues of the matrix

$$M = \left( {\begin{array}{*{20}{c}} {{\mathrm{\Delta }}_{12}} & {\frac{{{\rm{\Omega }}_{12}}}{2}} & 0 \\ {\frac{{{\rm{\Omega }}_{12}}}{2}} & 0 & {\frac{{{\rm{\Omega }}_{23}}}{2}} \\ 0 & {\frac{{{\rm{\Omega }}_{23}}}{2}} & {{\mathrm{\Delta }}_{23}} \end{array}} \right),$$

where Δij/2π = fmifmj is the frequency difference between Ri and Rj. The eigenvalues of this matrix correspond to the frequencies of the normal modes, i.e., the peaks in the spectroscopic measurement.

We consider the special case of Δ12 = Δ23 = Δ, with \(\left| {\mathrm{\Delta }} \right| \gg {\rm{\Omega }}_{12},\,{\rm{\Omega }}_{23}\), in the three-mode system. Here, the eigenvalues of the normal modes can be derived analytically. One eigenvalue is ωΔ = Δ, which corresponds to the eigenmode

$$\alpha _{\mathrm{\Delta }} = - \frac{{{\rm{\Omega }}_{23}}}{{\sqrt {{\rm{\Omega }}_{12}^2 + {\rm{\Omega }}_{23}^2} }}\alpha _1 + \frac{{{\rm{\Omega }}_{12}}}{{\sqrt {{\rm{\Omega }}_{12}^2 + {\rm{\Omega }}_{23}^2} }}\alpha _3.$$

This mode is a superposition of the end modes α1 and α3, and does not include the middle mode. The two other eigenvalues are

$${\mathrm{\omega }}_{{\mathrm{\Delta }} \pm } = \frac{1}{2}({\mathrm{\Delta }} \pm \omega _{{\mathrm{\Delta }}0})$$

with \(\omega _{\Delta 0} = \sqrt {\Delta ^2 + {\rm{\Omega }}_{12}^2 + {\rm{\Omega }}_{23}^2}\). The corresponding normal modes are

$$a_{{\mathrm{\Delta }} \pm } = \frac{{({\rm{\Omega }}_{12}a_1 \pm \left( {\omega _{\Delta 0} \mp \Delta } \right)a_2 + {\rm{\Omega }}_{23}a_3)}}{{\sqrt {2\omega _{{\mathrm{\Delta }}0}(\omega _{{\mathrm{\Delta }}0} \mp \Delta )} }}.$$

With \(\left| {\mathrm{\Delta }} \right| \gg {\rm{\Omega }}_{12},\,{\rm{\Omega }}_{23}\), for Δ > 0, \({\mathrm{\omega }}_{{\mathrm{\Delta }} + } \approx \Delta + ({\rm{\Omega }}_{12}^2 + {\rm{\Omega }}_{23}^2)/4\Delta\). The mode αΔ+ is nearly degenerate with αΔ, and

$$\alpha _{{\mathrm{\Delta }} + } \approx \frac{{{\rm{\Omega }}_{12}\alpha _1 + {\rm{\Omega }}_{23}\alpha _3}}{{\sqrt {{\rm{\Omega }}_{12}^2 + {\rm{\Omega }}_{23}^2} }}.$$

The mode αΔ− has frequency \({\mathrm{\omega }}_{{\mathrm{\Delta }} - } \approx - ({\rm{\Omega }}_{12}^2 + {\rm{\Omega }}_{23}^2)/4\Delta\), with αΔ− ≈ α2. The normal modes now become separated into two nearly degenerate modes {αΔ,αΔ+}, which are superpositions of modes α1 and α3, and a third mode αΔ− that is significantly off resonance from the other two modes. The nearly degenerate modes can be viewed as a hybridization of α1 and α3 with an effective splitting \(({\rm{\Omega }}_{12}^2 + {\rm{\Omega }}_{23}^2){\mathrm{/}}2{\mathrm{\Delta }}\). A similar result can be derived for Δ < 0, where \({\mathrm{\omega }}_{{\mathrm{\Delta }} - } \approx {\mathrm{\Delta }} + ({\rm{\Omega }}_{12}^2 + {\rm{\Omega }}_{23}^2){\mathrm{/}}4{\mathrm{\Delta }}\), with αΔ− given by the expression in Eq. (8), and \({\mathrm{\omega }}_{{\mathrm{\Delta }} + } \approx - ({\rm{\Omega }}_{12}^2 + {\rm{\Omega }}_{23}^2){\mathrm{/}}4{\mathrm{\Delta }}\) with αΔ+ ≈ α2.

The effective coupling rate can be derived with a perturbative approach on the matrix M. When |Δ| \( \gg\) Ω12, Ω23, the dynamics of α1 and α3 is governed by matrix

$${M_{\mathrm{eff}}} = \left( {\begin{array}{*{20}{c}} {\Delta + \frac{{{\rm{\Omega }}_{12}^2}}{{4\Delta }}} & {\frac{{{\rm{\Omega }}_{12}{\rm{\Omega }}_{23}}}{{4{\mathrm{\Delta }}}}} \\ {\frac{{{\rm{\Omega }}_{12}{\rm{\Omega }}_{23}}}{{4{\mathrm{\Delta }}}}} & {\Delta + \frac{{{\rm{\Omega }}_{23}^2}}{{4\Delta }}} \end{array}} \right).$$

This matrix tells us that because of their interaction with the middle mode α2, the frequency of mode α1 (α3) is shifted by \(\frac{{{\rm{\Omega }}_{12}^2}}{{4\Delta }}\) (\(\frac{{{\rm{\Omega }}_{23}^2}}{{4{\mathrm{\Delta }}}}\)), which is much smaller than |Δ|. Meanwhile, an effective coupling is generated between these two modes with magnitude \({\rm{\Omega }}_{13} = \frac{{{\rm{\Omega }}_{12}{\rm{\Omega }}_{23}}}{{2{\mathrm{\Delta }}}}\). The effective Hamiltonian for α1 and α3 can be written as

$${\cal H}_{{\mathrm{eff}}} = (\Delta + \frac{{{\rm{\Omega }}_{12}^2}}{{4\Delta }})\alpha _1^ \ast \alpha _1 + (\Delta + \frac{{{\rm{\Omega }}_{23}^2}}{{4\Delta }})\alpha _3^ \ast \alpha _3 + \frac{{{\rm{\Omega }}_{13}}}{2}(\alpha _1^ \ast \alpha _3 + \alpha _3^ \ast \alpha _1).$$

The effective coupling can be controlled over a wide range by varying the frequency of the second mode α2.

Data availability

The remaining data contained within the paper and Supplementary files are available from the author upon request.

Change history

  • 19 March 2019

    The original version of this Article contained a number of errors. As a result of this, changes have been made to both the PDF and the HTML versions of the Article. A full list of these changes is available online


  1. 1.

    Metcalfe, M. Applications of cavity optomechanics. Appl. Phys. Rev. 1, 031105 (2014).

    ADS  Article  Google Scholar 

  2. 2.

    Hajime, O. et al. Coherent phonon manipulation in coupled mechanical resonators. Nat. Phys. 9, 480–484 (2013).

    Article  Google Scholar 

  3. 3.

    Faust, T., Rieger, J., Seitner, M. J., Kotthaus, J. P. & Weig, E. M. Coherent control of a classical nanomechanical two-level system. Nat. Phys. 9, 485–488 (2013).

    CAS  Article  Google Scholar 

  4. 4.

    Zhu, D. et al. Coherent phonon Rabi oscillations with a high-frequency carbon nanotube phonon cavity. Nano Lett. 17, 915–921 (2017).

    ADS  CAS  Article  Google Scholar 

  5. 5.

    Aspelmeyer, M., Meystre, P. & Schwab, K. Quantum optomechanics. Phys. Today 65, 29–35 (2012).

    CAS  Article  Google Scholar 

  6. 6.

    Moser, J., Eichler, A., Guttinger, J., Dykman, M. I. & Bachtold, A. Nanotube mechanical resonators with quality factors of up to 5 million. Nat. Nanotechnol. 9, 1007–1011 (2014).

    ADS  CAS  Article  Google Scholar 

  7. 7.

    Sazonova, V. et al. A tunable carbon nanotube electromechanical oscillator. Nature 43, 284–287 (2004).

    ADS  Article  Google Scholar 

  8. 8.

    Chen, C. Y. et al. Graphene mechanical oscillators with tunable frequency. Nat. Nanotechnol. 8, 923–927 (2013).

    ADS  CAS  Article  Google Scholar 

  9. 9.

    Mahboob, I. & Yamaguchi, H. Bit storage and bit flip operations in an electromechanical oscillator. Nat. Nanotechnol. 3, 275–279 (2008).

    CAS  Article  Google Scholar 

  10. 10.

    Cirac, J. I., Zoller, P., Kimble, H. J. & Mabuchi, H. Quantum state transfer and entanglement distribution among distant nodes in a quantum network. Phys. Rev. Lett. 78, 3221–3224 (1997).

    ADS  CAS  Article  Google Scholar 

  11. 11.

    Eichler, A., del Álamo Ruiz, M., Plaza, J. A. & Bachtold, A. Strong coupling between mechanical modes in a nanotube resonator. Phys. Rev. Lett. 109, 025503 (2012).

    ADS  CAS  Article  Google Scholar 

  12. 12.

    Liu, C. H., Kim, I. S. & Lauhon, L. J. Optical control of mechanical mode-coupling within a MoS2 resonator in the strong-coupling regime. Nano Lett. 15, 6727–6731 (2015).

    ADS  CAS  Article  Google Scholar 

  13. 13.

    Li, S. X. et al. Parametric strong mode-coupling in carbon nanotube mechanical resonators. Nanoscale 8, 14809–14813 (2016).

    ADS  CAS  Article  Google Scholar 

  14. 14.

    Mathew, J. P., Patel, R. N., Borah, A., Vijay, R. & Deshmukh, M. M. Dynamical strong coupling and parametric amplification of mechanical modes of graphene drums. Nat. Nanotechnol. 11, 747–751 (2016).

    ADS  CAS  Article  Google Scholar 

  15. 15.

    De Alba, R. et al. Tunable phonon-cavity coupling in graphene membranes. Nat. Nanotechnol. 11, 741–746 (2016).

    ADS  Article  Google Scholar 

  16. 16.

    Castellanos-Gomez, A., Meerwaldt, H. B., Venstra, W. J., van der Zant, H. S. J. & Steele, G. A. Strong and tunable mode coupling in carbon nanotube resonators. Phys. Rev. B 86, 041402 (2012).

    ADS  Article  Google Scholar 

  17. 17.

    Deng, G. W. et al. Strongly coupled nanotube electromechanical resonators. Nano Lett. 16, 5456–5462 (2016).

    ADS  CAS  Article  Google Scholar 

  18. 18.

    Raman, C. V. & Krishnan, K. S. A new type of secondary radiation. Nature 121, 501–502 (1928).

    ADS  CAS  Article  Google Scholar 

  19. 19.

    Gaubatz, U., Rudecki, P., Schiemann, S. & Bergmann, K. Population transfer between molecular vibrational levels by stimulated raman-scattering with partially overlapping laserfields - a new concept and experimental results. J. Chem. Phys. 92, 5363–5376 (1990).

    ADS  CAS  Article  Google Scholar 

  20. 20.

    Majer, J. et al. Coupling superconducting qubits via a cavity bus. Nature 449, 443–447 (2007).

    ADS  CAS  Article  Google Scholar 

  21. 21.

    Deng, G. W. et al. Coupling two distant double quantum dots with a microwave resonator. Nano Lett. 15, 6620–6625 (2015).

    ADS  CAS  Article  Google Scholar 

  22. 22.

    Bunch, J. S. et al. Electromechanical resonators from graphene sheets. Science 315, 490–493 (2007).

    ADS  CAS  Article  Google Scholar 

  23. 23.

    Chen, C. Y. et al. Performance of monolayer graphene nanomechanical resonators with electrical readout. Nat. Nanotechnol. 4, 861–867 (2009).

    ADS  CAS  Article  Google Scholar 

  24. 24.

    Hatanaka, D., Mahboob, I., Onomitsu, K. & Yamaguchi, H. Phonon waveguides for electromechanical circuits. Nat. Nanotechnol. 9, 520–524 (2014).

    ADS  CAS  Article  Google Scholar 

  25. 25.

    Teufel, J. D. et al. Sideband cooling of micromechanical motion to the quantum ground state. Nature 475, 359–363 (2011).

    ADS  CAS  Article  Google Scholar 

  26. 26.

    Chan, J. et al. Laser cooling of a nanomechanical oscillator into its quantum ground state. Nature 478, 89–92 (2011).

    ADS  CAS  Article  Google Scholar 

  27. 27.

    Kepesidis, K. V., Bennett, S. D., Portolan, S., Lukin, M. D. & Rabl, P. Phonon cooling and lasing with nitrogen-vacancy centers in diamond. Phys. Rev. B 88, 064105 (2013).

    ADS  Article  Google Scholar 

  28. 28.

    Stadler, P., Belzig, W. & Rastelli, G. Ground-state cooling of a carbon nanomechanical resonator by spin-polarized current. Phys. Rev. Lett. 113, 047201 (2014).

    ADS  CAS  Article  Google Scholar 

  29. 29.

    Jähne, K. et al. Cavity-assisted squeezing of a mechanical oscillator. Phys. Rev. A 79, 063819 (2009).

    ADS  Article  Google Scholar 

  30. 30.

    Palomaki, T. A., Teufel, J. D., Simmonds, R. W. & Lehnert, K. W. Entangling mechanical motion with microwave fields. Science 342, 710–713 (2013).

    ADS  CAS  Article  Google Scholar 

  31. 31.

    Steele, G. A. et al. Strong coupling between single-electron tunneling and nanomechanical motion. Science 325, 1103–1107 (2009).

    ADS  CAS  Article  Google Scholar 

  32. 32.

    Lassagne, B., Tarakanov, Y., Kinaret, J., Garcia-Sanchez, D. & Bachtold, A. Coupling mechanics to charge transport in carbon nanotube mechanical resonators. Science 325, 1107–1110 (2009).

    ADS  CAS  Article  Google Scholar 

  33. 33.

    Tian, L. & Zoller, P. Coupled ion-nanomechanical systems. Phys. Rev. Lett. 93, 266403 (2004).

    ADS  CAS  Article  Google Scholar 

  34. 34.

    Schneider, B. H., Etaki, S., van der Zant, H. S. J. & Steele, G. A. Coupling carbon nanotube mechanics to a superconducting circuit. Sci. Rep. 2, 599 (2012).

    CAS  Article  Google Scholar 

  35. 35.

    Zhang, X. F. et al. Magnon dark modes and gradient memory. Nat. Commun. 6, 8914 (2015).

    CAS  Article  Google Scholar 

Download references


This work was supported by the National Key R&D Program of China (Grant No. 2016YFA0301700), the NSFC (Grants Nos. 11625419, 61704164, 61674132, 11674300, 11575172, and 91421303), the SPRP of CAS (Grant No. XDB01030000), and the Fundamental Research Fund for the Central Universities. L.T. is supported by the National Science Foundation under Award No. DMR-0956064 and PHY-1720501 and the UC Multicampus-National Lab Collaborative Research and Training under Award No. LFR-17-477237. This work was partially carried out at the USTC Center for Micro and Nanoscale Research and Fabrication.

Author information




G.L. and Z.-Z.Z. fabricated the device. G.-W.D. and Z.-Z.Z. performed the measurements. L.T., G.-W.D, and Z.-Z.Z analyzed the data and developed the theoretical analysis. H.-O.L, G.C., M.X., and G.-C.G. supported the fabrication and measurement. G.-P.G. and G.-W.D. planned the project. All authors participated in writing the manuscript.

Corresponding authors

Correspondence to Guang-Wei Deng or Lin Tian or Guo-Ping Guo.

Ethics declarations

Competing interests

The authors declare no competing financial interests.

Additional information

Publisher's note: Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.

Electronic supplementary material

Rights and permissions

Open Access This article is licensed under a Creative Commons Attribution 4.0 International License, which permits use, sharing, adaptation, distribution and reproduction in any medium or format, as long as you give appropriate credit to the original author(s) and the source, provide a link to the Creative Commons license, and indicate if changes were made. The images or other third party material in this article are included in the article’s Creative Commons license, unless indicated otherwise in a credit line to the material. If material is not included in the article’s Creative Commons license and your intended use is not permitted by statutory regulation or exceeds the permitted use, you will need to obtain permission directly from the copyright holder. To view a copy of this license, visit

Reprints and Permissions

About this article

Verify currency and authenticity via CrossMark

Cite this article

Luo, G., Zhang, ZZ., Deng, GW. et al. Strong indirect coupling between graphene-based mechanical resonators via a phonon cavity. Nat Commun 9, 383 (2018).

Download citation

Further reading


By submitting a comment you agree to abide by our Terms and Community Guidelines. If you find something abusive or that does not comply with our terms or guidelines please flag it as inappropriate.


Quick links

Nature Briefing

Sign up for the Nature Briefing newsletter — what matters in science, free to your inbox daily.

Get the most important science stories of the day, free in your inbox. Sign up for Nature Briefing