Introduction

Radiofrequency (rf) Paul traps [1,2,3] can store ions for a wide range of charge-to-mass ratios Q/m and thus represent a versatile and powerful tool with applications such as quantum information processing [4, 5] or cold chemistry [6, 7]. Many experiments involve trapping one or two atomic or molecular ion species. Over the course of the experiment, other (parasitic) isotopes or ion species may appear in the trap, e.g. due to chemical reactions of the ion of interest with background gas particles, and create a disturbance [8]. The parasitic ions can be embedded into the ion crystal after sympathetic cooling [9] or remain on large orbits [10].

In principle, it is possible to operate any quadrupole mass filter (including rf ion traps) in a parameter regime for which the trajectories of the desired species are stable and those of other species are unstable due to their specific charge-to-mass ratios. The dynamics are given by the solutions of the Mathieu equation and regions of stability can be described with the a and q parameters (see below) which are related to the electrostatic and radiofrequency voltages [1]. Due to technical limitations, it can be challenging to reach such regions of instability in an experiment. Other means of removing ions may then be advantageous, such as resonant excitation [11, 12].

By applying an oscillating voltage to one of the trap electrodes, the near-harmonic motion of the ions in the effective potential can be resonantly excited by displacing the ion from its equilibrium position [13]. This method, also known as “tickle”, will be referred to as displacement driving in the following. Since the secular frequency \(\omega _{\text {sec}}\) in the effective radial potential is proportional to Q/m, this method is also suitable to selectively remove ions from the trap [11] with a Q/m resolution depending on the driving duration [14].

Parametric resonances offer another possibility to efficiently drive a mechanical oscillator [15]. Ion traps are ideally suited to study parametric excitation due to the high degree of harmonicity of the typical potentials [16,17,18]. Applications range from ion removal with higher Q/m resolution [9, 19, 20] to excess micromotion compensation [21, 22]. Very recently, experiments in ion traps have exploited parametric excitation to create squeezed motional states for quantum control in both quantum sensing and experimental quantum simulations [23,24,25,26,27].

Here, we review and discuss the dynamics of a single ion in a Paul trap under the influence of parametric excitation and experimentally use this method for ion removal. We first perform numerical simulations to compare the ion removal efficiency achieved by either parametric excitation or resonant displacement driving. We find that parametric excitation can remove ions within milliseconds (or a few hundred oscillation cycles) with a Q/m resolution of better than \(10^{-3}\) and vanishing off-resonant excitation. In addition, we study the case in which an ion of mass \(m_2\) should be removed while it is sympathetically cooled by a co-trapped, laser cooled ion of different mass \(m_1\) which should remain in the trap. Finally, we discuss a first characterization of the experimental performance of the method and compare the results with our numerical calculations.

The method is flexible, as it only requires modulating the potential of the trap (in our case via the rf driving amplitude), representing a minor modification for typical ion trapping experiments. It can be used for any set of a and q parameters and does not require tuning the trap to a higher order (e.g. octupolar) instability [28, 29]. This method may be applicable to chemistry experiments which study reactions of ions and a (neutral) atomic ensemble [8, 30,31,32,33], but also to precision measurements where the spectroscopy ions are sympathetically cooled by an ion species amenable to laser cooling [34,35,36,37]. It could be extended to ions in Penning traps or storage rings.

Theoretical model

We consider a linear rf ion trap oriented along the z-axis. We discuss the experimental realization later and refer to Sect. 4 and Fig. 4. Two rf electrodes provide dynamical radial confinement while a set of segmented dc electrodes controls the electrostatic axial confinement along z as well as radial electric fields. The motion of the ion in the Paul trap in the radial xy-plane, here exemplarily shown for x, is described by the Mathieu equation [38]:

$$\begin{aligned} \frac{{\text {d}}^2x}{{\text {d}}t^2} + \frac{Ze}{m} \left [ U_{\text {dc}} \alpha _x + U_{\text {rf}} \alpha _x^{\prime } \cos (\varOmega t)\right] x = 0, \end{aligned}$$
(1)

where \(Ze=Q\) is the charge of the ion, e the elementary charge, m its mass, \(U_{\text {dc}}\) and \(U_{\text {rf}}\) are the voltages applied to the dc and rf electrodes and \(\varOmega\) is the angular frequency of the rf driving field. \(\alpha _x\) and \(\alpha _x^{\prime }\) are geometry factors with unit m\(^{-2}\) determined by the trap dimensions. The equations of motion along the y- and z-directions can be written analogously with \(|\alpha _y^{\prime }| \approx |\alpha _x^{\prime }|\) and \(\alpha _z^{\prime } \approx 0\) for a linear trap. The Mathieu equation can be rewritten in terms of the a and q parameters, which we will use in the following:

$$\begin{aligned} a_x = \frac{4Ze U_{\text {dc}} \alpha }{ m \varOmega ^2} , \quad q_x =\frac{2Ze U_{\text {rf}} \alpha ^\prime }{m\varOmega ^2} . \end{aligned}$$
(2)

In the limit \(a_x \ll 1\), \(q_x \ll 1\), the solution of the Mathieu equation can be approximated as a secular motion at frequency \(\omega _{x,\text {sec}}\) (along x) superimposed with a fast micromotion at \(\varOmega\) [38]. In this so-called pseudopotential approximation, \(\omega _{x,\text {sec}} \approx (\varOmega /2) \sqrt{a_x + q_x^2/2}\) [1].

Within the pseudopotential approximation, in which the micromotion is neglected, a modulation of \(U_{\text {rf}}\) at the frequency \(\omega _{\text {mod}}\) can again be modelled by the Mathieu equation. Similarly to the undriven ion trap, the parametrically driven harmonic oscillator exhibits regions of stability and instability, as has been previously shown and discussed in detail [18].

To study the dynamics of the problem and to study the experimental relevance of the method for various scenarios, we numerically solve the Mathieu equation, Eq. 1, after adding a parametric drive. The equation of motion is

$$\begin{aligned} \frac{{\text {d}}^2x}{{\text {d}}t^2} + \frac{1}{2} \varOmega ^2 x \left [ \frac{a_x}{2} + q_x \left( 1 + A_{p} \sin \left( {\omega _{\text {mod}} t}\right) \right) \cos \left( {\varOmega t}\right) \right] = 0 \; . \end{aligned}$$
(3)

We solve this equation in one dimension for our experimental parameters, \(\varOmega = 2\pi \times 1.4\,{\text {MHz}}\), \(a = 0.001\), \(q=0.25\), which are defined as in Eq. 2, and \(m=m_{\text {Ba}} = 138~\text {amu}\) (throughout this paper, \(m_{\text {Ba}}\) refers to the mass of \(^{138}{\text {Ba}}^{+}\)). We tune \(\omega _{\text {mod}} \approx 2 \omega _{x,{\text {sec}}}\) with an amplitude (modulation depth) up to \(A_{p} = 6 \times 10^{-3}\). On resonance, the parametrically driven oscillator becomes metastable and starts a coherent oscillation for an initial, nonzero displacement from the origin [15]. As initial conditions, we, therefore, choose the position \(x_{\text {ini}}=1 \,\mu \text {m}\) and momentum \(p_{\text {ini}} = 0\). Our parameters correspond to a secular frequency of \(\omega _{\text {sec}} \approx 2\pi \times 127 \, \text {kHz}\) and an initial potential energy of about \(k_{\text {B}} \times 5 \,\text {mK}\) (and zero kinetic energy).

Typical trajectories are shown in Fig. 1. Since the parametric modulation term \(q_x A_p \sin \left( {\omega _{\text {mod}}t} \right)\) in Eq. 3 is proportional to the oscillation amplitude x(t) at any time, the energy in the system increases exponentially [15, 16, 23], see Fig. 1c. The rate of energy gain is proportional to \(x_{\text {ini}}\), \(A_{p}\) and \(q_x\). We compare this result with resonant displacement driving in Fig. 1a, c, where the amplitude increases linearly and the energy increases quadratically. In the displacement driving case, the motion in x (y analogous) is described by

$$\begin{aligned} \frac{{\text {d}}^2x}{{\text {d}}t^2} + \frac{1}{2} \varOmega ^2 x \left [ \frac{a_x}{2} + q_x \cos \left( {\varOmega t} \right) \right] + \frac{Ze}{m} A_{d} \sin \left( \omega _{\text {mod}} t \right) = 0. \end{aligned}$$
(4)

In our experiment, a typical value for the amplitude is given by \(A_{d} = 1\, {\text {V/m}}\), corresponding to a voltage amplitude of \(10 \, {\text {mV}}\) (all amplitudes given as zero to peak) on a given dc electrode, in agreement with our segmented linear trap geometry with an ion–electrode distance of 9 mm, see Sect. 4.

Fig. 1
figure 1

Numerical calculation of the trajectory of an ion in a Paul trap under a the influence of an oscillating linear electric field at the resonance frequency (displacement driving, modulates the displacement of the pseudopotential ΦPseudo as shown in inset) and b an oscillating quadrupole electric field applied to the rf electrodes (parametric driving, modulates the pseudopotential curvature as shown in inset). The plots depict the envelope of the oscillation and show the linear versus exponential growth of the amplitudes. In c, the total (kinetic and potential) energy E of the ion is shown on a logarithmic scale in the case of displacement (dashed curved line) and parametric driving (solid line). The dashed horizontal line corresponds to a motional amplitude of \(1 \, {\text {mm}}\) (zero to peak), at which it is in general assumed that an ion is lost from the trap. For displacement driving, we choose an electric field amplitude of \(0.2\,{\text {V/m}}\) and for parametric driving, a modulation depth of \(6\times 10^{-3}\), both at a secular frequency of about \(\omega _{x,{\text {sec}}} = 2\pi \times 127\,{\text {kHz}}\)

The mass resolution is determined by the response of a single ion to the excitation as a function of the ratio m/(Ze), with \(Z = 1\) in our case. To compare the mass resolution in both the parametric and the displacement driving cases, we solve the equations of motion for the parameters given above. The modulation frequency \(\omega _{\text {mod}}\) (chosen to excite \(^{138}\text {Ba}^{+}\)) is constant while m is varied in discrete steps within the range \(m_{\text {Ba}} \pm 3\%\). We choose the duration \(t_{\text {exc}}\) and amplitude of the excitation for both parametric and displacement driving such that on resonance, the same oscillation amplitude of the ion is reached after \(t_{\text {exc}}\) (intersection of the two curves in Fig. 1c). As a figure of merit, we consider the relative energy gain ΔEEres, where ΔEres = E(texc) − E(t = 0) in the case of resonant excitation, i.e. for 138Ba+, and ΔE is the energy gain for m/mBa ≠ 1.

The results are shown in Fig. 2 and clearly emphasize the improved mass resolution with parametric excitation. While the full width at half maximum (FWHM) of the response to the parametric driving is only smaller by a factor of 1.6, the striking difference is the response when further detuned from the resonance. The response to displacement driving has a Lorentzian shape and falls off with a power law, while the response to parametric driving is Gaussian and falls off exponentially for \(m\ne {138}\, {\text {amu}}\) and allows for an improved mass resolution. This is equivalent to an improvement of the frequency resolution. For a relative mass difference \(|m - m_{\text {Ba}}| / m_{\text {Ba}} > \pm 0.2\%\), parametric driving already suppresses the excitation by 40 dB compared to displacement driving.

Fig. 2
figure 2

Mass dependence of the relative energy gain ΔEEres using parametric excitation compared to displacement driving. We simulate the dynamics of an ion for different \(m/m_{\text {Ba}}\) in both cases while keeping the excitation frequency constant. At \(t_{\text {exc}}\), we calculate the relative energy gain of the ion. The results for parametric excitation (blue solid line) and for displacement driving (green dashed line) are shown on a logarithmic scale. The driving amplitudes have been chosen as in Fig. 1, and to ensure comparability, \(t_{\text {exc}}=2.54 \,{\text {ms}}\) corresponds to the point in Fig. 1c where the energy curves for parametric and displacement driving intersect. Here, the parametric resonance is narrower than the displacement driving resonance by a factor of about 1.6 (full width at half maximum). More importantly, the tail of the parametric driving case falls off as a Gaussian, while that of the displacement driving resonance behaves as a Lorentzian function. Parametric driving thus acts as a knife for the ions close to resonance, allowing us to anticipate the separation of two ions with a mass ratio of 137/138 within milliseconds, as depicted by the dashed vertical line

Separation of ions with different masses

We now study the case of two co-trapped ions 1 and 2 which form a crystal and are strongly coupled. Ion 1 has mass \(m_1\) and is to remain in the trap while ion 2 with mass \(m_2\) is a parasitic ion which is to be removed from the trap. We numerically show that this can be achieved by cooling the ion 1 while parametrically driving ion 2. In this case, the crystal formed by the two ions has to melt in order to decouple the motion of the two ions.

We tested that performing the calculation with the full dynamics including \(\varOmega\) or within the pseudopotential approximation does not significantly change the dynamics of the ions in the simulation. In this section, we therefore use the pseudopotential approximation to speed up the calculation while extending it to three dimensions.

Along x, each of the two ions would individually oscillate at a secular frequency \(\omega _{x,{\text {sec}} 1}\) and \(\omega _{x,{\text {sec}} 2}\), where the frequencies depend on \(m_1\) and \(m_2\) (analogous for y, z). Due to the strong coupling of the ions, their motion can be described in the normal mode picture with 3N (\(N=2\)) oscillation frequencies. By exposing ions located near their equilibrium positions to homogeneous electric fields, only the common modes can be excited. However, as the oscillation amplitudes grow, the coupling between the ions becomes weaker until the normal mode description breaks down.

For a two-ion crystal with \(m_1 = m_2\), the motion in x can be decomposed into the center-of-mass mode \(\omega _{x,{\text {com}}} = \omega _{x,{\text {sec}}}\) and the so-called rocking mode

$$\begin{aligned} \omega _{x,{\text {rock}}} = \sqrt{\omega _{x,{\text {com}}}^2-\omega _{z,{\text {com}}}^2} , \end{aligned}$$
(5)

where \(\omega _{z,{\text {com}}} = \omega _{z,{\text {sec}}}\) is the center-of-mass frequency along the trap axis z. Generally, if \(m_1 \ne m_2\), the radial modes have a different structure and the center-of-mass frequency is not equal to either \(\omega _{x,{\text {sec}} 1}\) or \(\omega _{x,{\text {sec}} 2}\). Parametric driving at the frequency of the unperturbed ion 1 (\(\omega _{\text {mod}} = 2 \omega _{x,1}\)) is then not resonant with the common motion of the ions. The individual detuning from resonance, which is related to the excitation efficiency, depends on \(m_1/m_2\). In addition, the sympathetic cooling within the Coulomb crystal is also affected by the mass ratio (more efficient for mass ratios closer to 1), leading to a non-trivial behaviour of the excitation as long as the ions remain close to their coupled equilibrium positions. For our experimental parameters, the residual off-resonant excitation is sufficient to amplify the relative motion of the ions. Once the relative motion of the ions is sufficiently large, the ions are effectively decoupled and ion 1 is further excited parametrically as in the single ion case. The shift of the frequencies of the radial normal modes also depends on the axial confinement, as is apparent from Eq. 5. In our case, this shift is small (\(\approx 1\%\)) as \(\omega _{x,{\text {com}}} \gg \omega _{z,{\text {com}}}\), which is beneficial for effectively decoupling the ions in the parametric excitation scheme.

The simulation results for two ions with an additional damping term for ion 1 are shown in Fig. 3. The Coulomb crystal is initially radially displaced by \(1\,\mu {\text {m}}\). Here, we use a higher modulation amplitude for parametric driving than before to reduce the computation time followed by a qualitative analysis only. When comparing the trajectories of the two ions, we observe that the motion of the two ions is initially driven in common, that is, they still form a Coulomb crystal. Ion 1 (blue) is cooled and damps the motion of ion 2 (red). At a critical amplitude, ion 2 “breaks free” and the motion is decoupled from that of ion 1. The amplitude of ion 2 then increases exponentially as in the single ion case while ion 1 is again efficiently Doppler cooled.

Fig. 3
figure 3

Calculated trajectories of two ions with different masses in the rf trap. Here, the ions are considered to be \(^{137}{\text {Ba}}^{+}\) (red curve) and \(^{138}{\text {Ba}}^{+}\) (blue curve). The motion of the \(^{138}{\text {Ba}}^{+}\) ion is damped by laser cooling and sympathetically cools the \(^{137}{\text {Ba}}^{+}\) ion through the mutual Coulomb interaction. We set the common initial displacement in the x direction to \(1\,\upmu {\text {m}}\). At \(t=0\), a parametric excitation at twice the resonance frequency of a single \(^{137}{\text {Ba}}^{+}\) ion is turned on while the \(^{138}{\text {Ba}}^{+}\) ion is still directly laser cooled. The x (radial) and z (axial) positions of the ions are plotted as a function of time. Initially, the ions are aligned along the z-axis within a common ion crystal, with their Coulomb interaction in equilibrium with the axial electrostatic potential. The ions then begin oscillating in the x direction in common, until the motion of the \(^{138}{\text {Ba}}^{+}\) ion is sufficiently decoupled and only the amplitude of the \(^{137}{\text {Ba}}^{+}\) ion keeps growing. Here, this critical point is reached after about 2 ms and the \(^{138}\text {Ba}^{+}\) is cooled back to the trap center. The amplitude of the \(^{137}\text {Ba}^{+}\) reaches \(1\,\text {mm}\) at \(t \approx 2.8\,\text {ms}\), where it is assumed to leave the trap

Comparison with experimental results

Fig. 4
figure 4

Sketch of the experimental setup. \(^{138}\text {Ba}^{+}\) ions (blue circle) are trapped and laser cooled near the center of a segmented linear rf trap. The blade-style comprises two rf blades and two segmented dc blades with endcap (dc1, dc3, dc4 and dc6) and compensation segments (dc2 and dc5). An additional compensation electrode (dc7) located below the trap close to the yz-plane is not shown in the sketch. Other isotopes of barium (red circle) are also produced during photoionization and trapped. In addition, we can produce magneto-optically and all-optically trapped clouds of \(^{87}\)Rb, which sometimes leads to the production of Rb\(^{+}\) and Rb\(_2^{+}\) ions [8, 9]. These ions can be crystallized (strongly coupled to the laser cooled ions via Coulomb interaction) or in a plasma (weakly coupled). To remove all ions but \(^{138}\text {Ba}^{+}\), we modulate the rf drive of our Paul trap at twice the radial secular frequency of these ions through the helical resonator. We can also apply an oscillating displacement via the dc electrodes for determining the trapping frequencies (endcap segments for axial frequencies and compensation segments for radial frequencies)

Fig. 5
figure 5

Measurement of the timescale for removing a single ion via parametric excitation. After Doppler cooling, at \(t=0\), the cooling and repumping lasers are turned off and the rf trap drive is modulated to parametrically excite the ion at \(2\omega _{\text {sec}}\). After \(t_{\text {exc}}\), the parametric excitation is turned off and the cooling and repumping lasers are turned on again. Then the CCD camera signal is monitored to observe whether the ion is recooled into the trap. If, after 1 s, no fluorescence signal can be observed, we consider the removal attempt from the trap as successful. After loading a new ion if necessary, the experiment is repeated until each \(t_{\text {exc}}\) has been repeated about 30 times. Finally, the removal probability is shown in dependence on the excitation duration \(t_{\text {exc}}\). Due to the finite temperature of the ion, the initial conditions for position and momentum vary according to the Boltzmann distribution and lead to a smoothed transition from 0 to 100% removal probability. The shaded area is an estimate of the removal probability of the ion after \(t_{\text {exc}}\) based on a numerical calculation of its trajectory under the influence of parametric excitation and assuming an initial temperature of \(T \approx 360\, \upmu\)K corresponding to the Doppler limit. The ion is considered to be removed when it reaches a distance of 1 mm from the trap center

We next perform an experimental investigation of parametric driving as a tool for removing ions from a Paul trap. Our experimental setup [8, 39, 40] shown in Fig. 4 consists of a linear segmented Paul trap (with ion–electrode distance of 9 mm) under ultra-high vacuum (UHV). The rf source is a signal synthesizer operated at a frequency \(\varOmega = 2\pi \times 1.4\,\text {MHz}\). A helical resonator with a quality factor of 40 enhances \(U_{\text {rf}}\) up to 2000 V and is connected to two diagonally opposed rf blade electrodes via a standard vacuum high-frequency feedthrough. The dc blades consist of segmented electrodes which are grounded with respect to the rf electrodes and can be offset by small dc fields to compensate stray fields [41] and to provide axial confinement of typically \(\omega _{z,\text {sec}} = 2\pi \times 12\,\text {kHz}\). The rf electrodes feature slits symmetrically opposed to the gaps between the segments in the dc electrodes. \(^{138}\text {Ba}\) atoms (and other isotopes) are emitted from an oven, photoionized with a resonant 553-nm and an additional 405-nm laser [42], and subsequently Doppler cooled to below one millikelvin using lasers at 493 nm and 650 nm for cooling and repumping, respectively. The fluorescence emitted by \(^{138}\text {Ba}^+\) during Doppler cooling is imaged by a charge-coupled device (CCD) camera used for detection.

We first experimentally confirm the efficiency of the parametric excitation method, here with a single \(^{138}\text {Ba}^+\) ion as a showcase, see Fig. 5. To investigate the undamped dynamics as in Fig. 1, we first prepare a single Doppler-cooled \(^{138}\text {Ba}^{+}\) ion in the trap. We then turn off the cooling and repumping lasers and turn on parametric excitation for a variable duration \(t_{\text {exc}}\). Here, \(\omega _{x,\text {sec}} = 2\pi \times (120\pm 1) \, \text {kHz}\) and the corresponding modulation frequency is \(\omega _{\text {mod}} = 2\pi \times (240\pm 2) \, \text {kHz}\) with a modulation depth of \(8\times 10^{-3}\). We then turn on the cooling and repumping lasers and detect via fluorescence imaging whether the ion has remained in the trap. The probabilistic distribution of the initial position and the velocity after laser cooling translate to a distribution of the duration after which the ion is removed from the trap. This leads to the smooth transition from 0% removal probability to near-unity removal probability after about 5 ms. The experimental results are in reasonable agreement with the results of our simulation depicted by the red curve. Given that the growth of the motional amplitude is exponential, an accurate description of timescales is challenging.

In practice, we use a linear frequency chirp of about 1 kHz across the resonance (usually operated in the positive direction with increasing frequency) and sweep time of 1 ms, which is repeated periodically for the duration of the excitation \(t_{\text {exc}}\). This improves the repeatability in our experiment which we attribute to two effects. First, due to the high-frequency resolution, small drifts of the secular frequency on the order of 300 Hz require frequent tuning of the modulation frequency. Second, we suspect that anharmonicities of the trap lead to a change in \(\omega _{x,{\text {sec}}}\) at higher oscillation amplitudes. After reaching a critical amplitude, \(\omega _{\text {mod}}\) becomes detuned from \(\omega _{x,{\text {sec}}}\) and the modulation no longer efficiently excites the motion. The frequency chirp mitigates both possible issues.

Application to mass separation of mixed-species or mixed-isotope ion crystals and clouds

As discussed above, various processes can involve loading of contaminating ion species into the trap besides the laser-cooled ion species of interest. For two of such processes, we apply parametric excitation to remove the contaminating ion species.

The photoionization process is not perfectly isotope selective in our experiment due to an angle of about \(110^{\circ }\) between the photoionization laser axis and the direction of the hot atomic beam from the oven. This leads to loading of barium isotopes with 136 and 137 nucleons into the trap with a probability of about 10%. Reactions of electronically excited \(^{138}\text {Ba}^{+}\) with background \(\text {H}_2\) molecules can also lead to the formation of \(\text {BaH}^{+}\) hydride ions [43,44,45]. After sympathetic cooling by \(^{138}\text {Ba}^{+}\), the ensemble consisting of \(^{138}\text {Ba}^{+}\) and another ion species forms a crystal. Only the \(^{138}\text {Ba}^{+}\) ion emits fluorescence from the near-resonant cooling laser and appears as a bright spot on the CCD camera image. The presence of another (dark) ion shifts the \(^{138}\text {Ba}^{+}\) ion from its equilibrium position at the center of the trap.

If the fluorescence image indicates that such a mixed crystal is present in the trap, we apply parametric driving on the trap electrodes. We tune the modulation frequency to the resonance of \(^{136}\text {Ba}^{+}\) (\(^{137}\text {Ba}^{+}\)) while laser cooling \(^{138}\text {Ba}^{+}\). We observe that the dark ions can be removed from the trap by applying the parametric driving resonant with the secular frequency of \(^{136}\text {Ba}^{+}\) (\(^{137}\text {Ba}^{+}\)). This procedure now takes a few seconds to successfully remove the parasitic ions. We were not able to remove the parasitic ions using displacement driving while the laser-cooled \(^{138}\text {Ba}^{+}\) remains in the center of the trap.

Compared to the numerical simulations presented in Fig. 3, where it was possible to remove ion 2 within milliseconds while ion 1 remained in the trap, we experimentally observe longer timescales. In our simulations, we found that the behaviour depends on the damping rate, \(\omega _{x,{\text {sec}}}/\omega _{z,{\text {sec}}}\) and \(A_p\). Reaching the critical point at which the parasitic ion is sufficiently decoupled from the laser-cooled ion strongly depends on the initial conditions [15, 16] and can be challenging. In our experiment, this may be assisted by instantaneous heating effects. Given the observed timescales and our background pressure on the order of \(5\times 10^{-10} \, {\text {mbar}}\), it is possible that background gas collisions initiate the process. The effective continuous sampling of the Boltzmann distribution of the ion while it is being laser cooled may also assist the process.

We have also used this method to remove \(\text {Rb}^{+}\) and \(\text {Rb}_2^{+}\) ions from our trap [8]. In this case, the ions are typically not embedded into the crystal structure at the center of the trap. Ions on high orbits with large kinetic energy can be removed reliably within tens of milliseconds while only minimally disturbing the \(^{138}\text {Ba}^{+}\) in the center of the trap.

Summary and outlook

We have discussed parametric excitation as a method for mass-selectively removing ions from an rf ion trap. We find that parametric excitation at twice the ion’s resonance frequency is a highly efficient and fast method for this purpose. For the high oscillation amplitudes (10–50% of the ion–electrode distance) required to remove ions from the trap, the mass resolution is significantly enhanced compared to displacement driving at the resonance frequency. Efficiently removing ions with parametric excitation requires precise tuning of the excitation frequency. Small drifts of the trapping frequency can thus limit the performance of the method. While the secular frequencies can be stabilized via rf and dc voltages [46], we used a sweep of the excitation frequency in a 1 kHz window near the resonance. Further improvement could be achieved by initially transferring a controlled amount of energy to the ions by applying a resonant displacement driving pulse at \(\omega _{x,{\text {sec}}}\) [13, 16] or giving the ions a kick with a voltage pulse.

The amplitude modulation index is limited due to the bandpass filter constituted by the helical resonator. Other schemes to enhance the rf-amplitude which leads to less damping of the modulation sidebands may be advantageous, especially at low trap drive frequencies where higher voltages can be achieved in the pre-amplification. Using even higher harmonics \(n\,\omega _{\text {sec}}\) (with even integer n) could further improve the frequency resolution [18]. Parametric excitation may be useful when initializing a large ion trap with a single ion, e.g. in the context of shallow optical trapping potentials [39]. Due to the recent interest in experiments relying on a multitude of ion species in a single trap, including ions for sympathetic cooling and, e.g. molecular ions, we believe that removal of ions by parametric excitation may be a useful tool for many ion trapping groups.