Abstract
In the experiments described in the previous chapter we detected coherent spin squeezed atomic quantum states. However the implementation of a full atom interferometer where the two modes are defined by two mean field wavefunctions in a double well potential is difficult. One of the problems is the limited range in which the system parameter \(\Uplambda\) can be tuned—especially the Rabi regime is not accessible for our setup.
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Notes
- 1.
We use the excitation of these modes when changing the barrier height \(V_0\) abruptly for a calibration of \(V_0\)[3].
- 2.
Technologically a coherent change of the frequency of one of the two electromagnetic fields is not possible in our experiment.
- 3.
We use the labeling \(|{a}\rangle\) and \(|{b}\rangle\) for both the single particle states and the mean field modes which is not rigorously correct. However since we neglect external dynamics and assume perfect wavefunction overlap this labeling is justified.
- 4.
Dipolar relaxation is a two body process meaning its rate \(L_2 \propto K_2N\) is proportional to the number of atoms in the trap. The loss coefficient for the \(|2,-1\rangle\) state was measured to \(K_2 = 8.8 \times 10^{-14}\,\text{cm}^3/\text{s}\) [26]
- 5.
At the time this measurement was done the active magnetic field compensation was not yet installed. Therefore we measure a larger width as theoretically expected. The inelastic width extracted from the measurement shown in Fig. 4.5 agrees well with the theoretical prediction.
- 6.
Experimentally we also found the best number squeezing at this magnetic field.
- 7.
A lower Rabi frequency than for the usual coupling is chosen here in order to work in a higher \(\Uplambda\) situation.
- 8.
We assume here without loss of generality \(\langle\hat J_y\rangle = 0\) such that the twist is symmetric to the \(J_y\) axis.
- 9.
We assume small fluctuations \(\Updelta J^2_{\perp, {\rm max}}\) as compared to the total atom number \(\Updelta J^2_{\perp, {\rm max}} < {N}^{2}/4\) such that the Bloch sphere can be locally approximated by a plane.
- 10.
The single-photon Rabi frequency for the coupling of the Zeeman sub-states is approximately \(2\pi \cdot 10 \) kHz.
- 11.
Experimentally the phase of the coupling pulses at time t can be found by a measurement of the population imbalance versus pulse phase of a final \(\pi/2\) pulse. The zero crossings identify the two phases where the rotation axis hits the center of the spin state.
- 12.
60 experimental repetitions define one dataset in all measurements done in context with the internal spin system.
- 13.
In order to obtain better statistics we average the measurements for \(\alpha = 16^\circ\) and \(\alpha = 17^\circ\).
- 14.
As explained in In Sect. 3.4.1 we always remove the photon shot noise in these experiments.
- 15.
Depending on the relative position of dipole trap and optical lattice the central well can contain up to \(450\) atoms.
- 16.
Experimentally the number of echo pulses should be kept minimal, since the coupling pulses introduce additional noise due to fluctuations of pulse phase and power.
- 17.
The spacing between the wells is only \(5.7\mu\!\)m such that magnetic field fluctuations and the electromagnetic radiation fields for the coupling are homogeneous over the whole system.
- 18.
Fluctuation measurements on a coherent spin state after a \(7\pi/2\) pulse in a Rabi cycle still show shot noise limited noise characteristics. This indicates negligible pulse power fluctuations in our experiment and suggests again that shot-to-shot magnetic field fluctuations are the main noise source.
- 19.
As a reminder, \(p=\langle n_a/N\rangle\) is the probability for an atom to be found in mode \(|{a}\rangle\).
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Groß, C. (2012). Non-linear Interferometry Beyond the Standard Quantum Limit. In: Spin Squeezing and Non-linear Atom Interferometry with Bose-Einstein Condensates. Springer Theses. Springer, Berlin, Heidelberg. https://doi.org/10.1007/978-3-642-25637-0_4
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