# Direct Measurement of the Proton Magnetic Moment

###### Abstract

The proton magnetic moment in nuclear magnetons is measured to be , a 2.5 ppm (parts per million) uncertainty. The direct determination, using a single proton in a Penning trap, demonstrates the first method that should work as well with an antiproton () as with a proton (). This opens the way to measuring the magnetic moment (whose uncertainty has essentially not been reduced for 20 years) at least times more precisely.

###### pacs:

13.40.Em, 14.60.Cd, 12.20-mThe most precisely measured property of an elementary particle is the magnetic moment of an electron, , deduced to from the quantum jump spectroscopy of the lowest quantum states of a single trapped electron Hanneke et al. (2008). The moment was measured in Bohr magnetons, (with for electron charge and mass ). The measurement method works for positrons and electrons. Efforts are thus underway to measure the positron moment (now known 15 times less precisely R. S. Van Dyck, Jr. et al. (1987)) at the electron precision – to test lepton CPT invariance to an unprecedented precision.

Applying such one particle methods to measuring the magnetic moment of a or (with mass ) is challenging. Nuclear moments scale naturally as the smaller nuclear magneton with . Three measurements and two theoretical corrections Winkler et al. (1972); Mohr et al. (2008) together determine to 0.01 ppm (Fig. 1), but one of the measurements relies upon a hydrogen maser so this method cannot be used for . No measurement uses a method applicable to both and . For more than 20 years the magnetic moment has been deduced from exotic atom structure, to a precision that has remained at only 3000 ppm Kreissl et al. (1988); Pask et al. (2009) (Fig. 1).

This Letter demonstrates a one-particle method equally applicable to and , opening the way to a baryon CPT test made by directly comparing and p magnetic moments. The proton moment in nuclear magnetons is the ratio of its spin and cyclotron frequencies,

(1) |

Our measurements of these frequencies with a single trapped determine to 2.5 ppm, with a value consistent with the indirect determination Winkler et al. (1972); Mohr et al. (2008). The possibility to use a single trapped for precise measurements was established when for a trapped was measured to Gabrielse et al. (1999). It now seems possible to apply the measurement method demonstrated here to determine the magnetic moment times more precisely than do exotic atom measurements Kreissl et al. (1988); Pask et al. (2009). An additional precision increase of or more should be possible once a single or spin flip is resolved.

For the measurement of , a single is suspended at the center of the cylindrically symmetric “analysis trap” (Fig. 2a). Its stacked ring electrodes are made of OFE copper or iron, with a 3 mm inner diameter and an evaporated gold layer. The electrodes and surrounding vacuum container are cooled to 4.2 K by a thermal connection to liquid helium. Cryopumping of the closed system made the vacuum better than Torr in a similar system Gabrielse et al. (1990), so collisions are not important here. Appropriate potentials applied to electrodes with a carefully chosen relative geometry Gabrielse et al. (1989) make a very good electrostatic quadrupole near the trap center with open access to the trap interior from either end.

In a vertical magnetic field Tesla, a trapped proton’s circular cyclotron motion is perpendicular to B with a frequency MHz slightly shifted from by the electrostatic potential. The proton also oscillates parallel to B at about kHz. The proton’s third motion is a circular magnetron motion, also perpendicular to B, at the much lower frequency kHz. The spin precession frequency is MHz.

Driving forces flip the spin and make cyclotron transitions. Spin flips require a magnetic field perpendicular to B that oscillates at approximately . This field is generated by currents sent through halves of a compensation electrode (Fig. 2c). Cyclotron transitions require an electric field perpendicular to B that oscillates at approximately . This field is generated by potentials applied across halves of a compensation electrode (Fig. 2d).

Shifts in reveal changes in the cyclotron, spin and magnetron quantum numbers , and Brown and Gabrielse (1986),

(2) |

The shifts (50 mHz per cyclotron quanta and 130 mHz for a spin flip) arise when a magnetic bottle gradient,

(3) |

from a saturated iron ring (Fig. 2a) interacts with cyclotron, magnetron and spin moments . The effective shifts because the electrostatic axial oscillator Hamiltonian going as acquires an additional term going as . The bottle strength, T/m, is 190 times that used to detect electron spin flips Hanneke et al. (2008) to compensate for the small size of the nuclear moments.

A proton is initially loaded into a coaxial trap just above the analysis trap of Fig. 2. Its cyclotron motion induces currents in and comes to thermal equilibrium with a cold damping circuit attached to the trap. The is then transferred to the analysis trap by adjusting electrode potentials to make an axial potential well that moves adiabatically down into the analysis trap.

Two methods are used to measure the of Eq. 2 in the analysis trap, though the choice of which method to use in which context is more historical than necessary at the current precision. The first (used to detect cyclotron transitions with the weakest possible driving force) takes to be the shift of the frequency at which noise in a detection circuit is canceled by the signal from the proton axial motion that it drives Dehmelt and Walls (1968). The second (used to detect spin flips) takes to be the shift in the frequency of a self-excited oscillator (SEO) Guise et al. (2010). The SEO oscillation arises when amplified signal from the proton’s axial oscillation is fed back to drive the into a steady-state oscillation. The detected is first used to check if the cyclotron radius is below 0.3 , a shift Hz. If not, the is returned to the precision trap for cyclotron damping as needed to select a low cyclotron energy.

Spin and cyclotron measurements are based on sequences of deviations , with . The are a series of averages of the axial frequency over a chosen averaging time. A histogram of deviations (e.g. Fig. 3a) is characterized by an Allan variance,

(4) |

(often used to describe the stability of frequency sources). The Allan deviation is the square root of the variance.

The Allan variance is when no nearly resonant spin or cyclotron drive is applied (gray histogram in Fig. 3a). The source of this scatter is not yet well understood, as has been discussed Guise et al. (2010). When a nearly resonant drive at frequency induces spin flips or cyclotron transitions, the Allan variance increases slightly to (outline histogram in Fig. 3a). The small increase, , reveals spin or cyclotron resonance. The measured increases with cyclotron radius (Fig. 3b). It is minimized by selecting a with a cyclotron radius below 0.3 m, as described. The measured Allan deviation is then minimum for an averaging time s when the SEO is used (Fig. 3c) and for a longer when the noise shorting method is used.

The cyclotron and spin resonances are well known to be threshold resonances Brown (1985); Brown and Gabrielse (1986). A driving force has no effect below a resonance frequency ( or here). The transition rate between quantum states increases abruptly to its maximum at the resonant frequency. Above this threshold there is a distribution cyclotron or spin frequencies at which these motion can be driven. These correspond to the distribution of sampled by the thermal axial motion of the (in thermal equilibrium with the axial detection circuit) within the magnetic bottle gradient.

No natural linewidth broadens the sharp threshold edge because the spin and cyclotron motions are not damped in the analysis trap. The superconducting solenoid produces a stable B that does not significantly smear the edge. A small broadening arising because sideband cooling (of magnetron motion coupled to axial motion) selects different values from a distribution of magnetron radii (explored in detail in Guise et al. (2010)) is added as “magnetron broadening” uncertainty in Table 1.

Fig. 4 shows the cycle repeated to look for the spin frequency, . With the SEO stabilized for 2 s, the SEO frequency is averaged for 24 seconds to get . With the SEO off, a nearly-resonant spin flip drive at frequency is applied for 2 s. After the SEO is back on for 2 s its average frequency is measured. As a control, a spin drive detuned 50 kHz from resonance is next applied with the SEO off. It is detuned rather than off to check for secondary effects of the drive. After the average is measured, 2 s of sideband cooling and feedback cooling keep the magnetron radius from growing Guise et al. (2010).

The cycle in Fig. 4 is repeated for typically 36 hours for each drive frequency in Fig. 5a. The Allan deviation for the sequence of deviations represents the effect of fluctuations when a near-resonant spin drive is applied. The Allan deviation for the sequence of deviations represents fluctuations when no near-resonant drive is applied. The spin lineshape in Fig. 5a shows vs. drive frequency.

The expected sharp threshold that indicates the spin frequency is clearly visible. The uncertainty in the resonance frequency in Table 1 is the half-width of the edge. Smaller frequency steps that might have produced a more precise measurement were not investigated. The scale to the right in Fig. 5a is the average probability that the spin drive pulse makes a spin flip. A similar spin resonance is observed in a competing experiment Ulmer et al. (2011), but the fractional half-width of the whole resonance line is about 20 times wider and the fractional uncertainty specified is about 100 times larger.

Matching a pulsed 221 MHz drive so that the needed current goes through required electrode (Fig. 2c) in a cryogenic vacuum enclosure is challenging. The strong drive applied (because the matching is not optimized) observably shifts as a function of spin drive power (Fig. 4b), presumably because the average trapping potential is slightly modified. The shift from the strongest drive in Fig. 4b is still too small to contribute to the uncertainty Table 1, however. Better matching should produce the same current with less applied drive and shift.

The basic idea of the cyclotron frequency measurement is much the same as for the spin frequency. The applied drive is weak enough that in 6 hours it causes no detectable growth in the average cyclotron radius and energy even for a resonant drive. The resonant drive is just strong enough to increase the measured Allan variance, . The cyclotron lineshape (Fig. 5b) shows clearly the expected sharp threshold at the trap cyclotron frequency, . The uncertainty in Table 1 is the half-width of the edge. Smaller frequency steps that might have produced a more precise measurement were not investigated.

For each of the drive frequencies represented in the cyclotron lineshape in Fig. 5b a cyclotron drive is applied continuously for about 6 hours. This initial approach was adopted to find the weakest useful cyclotron drive and was continued because it worked well. Deviations between consecutive 80 s averages are plotted as a histogram, and characterized by an Allan variance, . The subtracted off to get uses measurements below the threshold resonance.

We utilize no fits to expected resonance lineshapes for this measurement. However, we note that the spin lineshape fits well to the Brownian motion lineshape Brown (1985) expected for magnetic field fluctuations caused by thermal axial motion within a magnetic bottle gradient upon a spin 1/2 system. An axial temperature of 8 K is extracted from the fit, consistent with measurements using a magnetron method detailed in Guise et al. (2010). With no expected lineshape yet available for the cyclotron resonance, we note that the cyclotron line fits well to the expected spin lineshape but with an axial temperature of 4 K. A proper diffusion treatment of the way that a cyclotron drive moves population between cyclotron states is needed.

The magnetic moment in nuclear magnetons is a ratio of frequencies (Eq. 1). The free space cyclotron frequency, , is needed while trap eigenfrequencies , and are measured directly. The Brown-Gabrielse invariance theorem, Brown and Gabrielse (1982) determines from the eigenfrequencies of an (unavoidably) imperfect Penning trap.

The directly measured proton magnetic moment is

(5) |

Uncertainty sources are summarized in Table 1. Frequency uncertainties are the half-widths of the sharp edges in the lineshapes, as discussed. The magnetron linewidth uncertainty comes from the distribution of magnetron radii following sideband cooling, as discussed. All other known uncertainties are too small to show up in this table.

Resonance | Source | ppm |
---|---|---|

spin | resonance frequency | 1.7 |

spin | magnetron broadening | 0.7 |

cyclotron | resonance frequency | 1.6 |

cyclotron | magnetron broadening | 0.7 |

total | 2.5 |

The measurement of agrees within 0.2 standard deviations with a 0.01 ppm determination. The latter is less direct in that three experiments and two theoretical corrections are required, using

(6) |

The largest uncertainty (0.01 ppm) is for the measured ratio of bound moments, , measured with a hydrogen maser Winkler et al. (1972) that would be difficult to duplicate with antimatter. The two theoretical corrections between bound and free moments are known ten times more precisely Mohr and Taylor (2000) . Both the mentioned Hanneke et al. (2008) and Beier et al. (2002) are measured much more precisely still.

This measurement method is the first that can be applied to and . The magnetic moments of this particle-antiparticle pair could now be compared times more precisely than previously possible (Fig. 1) as a test of CPT invariance with a baryon system.

A yet illusive goal of this effort D’Urso et al. (2005) and another Ulmer et al. (2011) is to resolve a single spin flip of a trapped . The spin could be flipped in a trap with a very small magnetic gradient and thermal broadening, and transferred down to the analysis trap only to determine the spin state. The Allan deviation realized in Fig. 3c suggests that this goal is not far off. Then could then be determined by quantum jump spectroscopy, as for the electron magnetic moment Hanneke et al. (2008). Measuring for a trapped to better than has already been demonstrated Gabrielse et al. (1999) in a trap with a small magnetic gradient. A comparison of the and magnetic moments that is improved by a factor of a million or more seems possible. This would add a second precise CPT test with baryons to the comparison of the charge-to-mass ratios of and p Gabrielse et al. (1999).

In conclusion, a direct measurement of the proton magnetic moment to 2.5 ppm is made with a single suspended in a Penning trap. The measurement is consistent with a more precise determination that uses several experimental and theoretical inputs. The measurement method is the first that can be applied to a or . It should now be possible to compare the magnetic moments of and a thousand times more precisely than has been possible so far, with another thousand-fold improvement factor to be realized when spin flips of a single are individually resolved.

We are grateful for contributions made earlier by N. Guise and recently by M. Marshall, and for their comments on the manuscript. This work was supported by the AMO programs of the NSF and the AFOSR.

## References

- Hanneke et al. (2008) D. Hanneke, S. Fogwell, and G. Gabrielse, Phys. Rev. Lett. 100, 120801 (2008).
- R. S. Van Dyck, Jr. et al. (1987) R. S. Van Dyck, Jr., P. B. Schwinberg, and H. G. Dehmelt, Phys. Rev. Lett. 59, 26 (1987).
- Winkler et al. (1972) P. Winkler, D. Kleppner, T. Myint, and F. Walther, Phys. Rev. A 5, 83 (1972).
- Mohr et al. (2008) P. J. Mohr, B. N. Taylor, and D. B. Newall, Rev. Mod. Phys. 80, 633 (2008).
- Kreissl et al. (1988) A. Kreissl, A. Hancock, H. Koch, T. Köehler, H. Poth, U. Raich, D. Rohmann, A. Wolf, L. Tauscher, A. Nilsson, M. Suffert, M. Chardalas, S. Dedoussis, H. Daniel, T. von Egidy, F. Hartmann, W. Kanert, H. Plendl, G. Schmidt, and J. Reidy, Z. Phys. C: Part. Fields 37, 557 (1988).
- Pask et al. (2009) T. Pask, D. Barna, A. Dax, R. Hayano, M. Hori, D. Horváth, S. Friedrich, B. Juhász, O. Massiczek, N. Ono, A. Sótér, and E. Widmann, Phys. Lett. B 678, 55 (2009).
- Gabrielse et al. (1999) G. Gabrielse, A. Khabbaz, D. S. Hall, C. Heimann, H. Kalinowsky, and W. Jhe, Phys. Rev. Lett. 82, 3198 (1999).
- Gabrielse et al. (1990) G. Gabrielse, X. Fei, L. A. Orozco, R. L. Tjoelker, J. Haas, H. Kalinowsky, T. A. Trainor, and W. Kells, Phys. Rev. Lett. 65, 1317 (1990).
- Gabrielse et al. (1989) G. Gabrielse, L. Haarsma, and S. L. Rolston, Intl. J. of Mass Spec. and Ion Proc. 88, 319 (1989), ibid. 93:, 121 (1989).
- Brown and Gabrielse (1986) L. S. Brown and G. Gabrielse, Rev. Mod. Phys. 58, 233 (1986).
- Dehmelt and Walls (1968) H. Dehmelt and F. Walls, Phys. Rev. Lett. 21, 127 (1968).
- Guise et al. (2010) N. Guise, J. DiSciacca, and G. Gabrielse, Phys. Rev. Lett. 104, 143001 (2010).
- Brown (1985) L. S. Brown, Ann. Phys. (N.Y.) 159, 62 (1985).
- Ulmer et al. (2011) S. Ulmer, C. C. Rodegheri, K. Blaum, H. Kracke, A. Mooser, W. Quint, and J. Walz, Phys. Rev. Lett. 106, 253001 (2011).
- Brown and Gabrielse (1982) L. S. Brown and G. Gabrielse, Phys. Rev. A 25, 2423 (1982).
- Mohr and Taylor (2000) P. J. Mohr and B. N. Taylor, Rev. Mod. Phys. 72, 351 (2000).
- Beier et al. (2002) T. Beier, H. Häffner, N. Hermanspahn, S. G. Karshenboim, H.-J. Kluge, W. Quint, S. Stahl, J. Verdú, and G. Werth, Phys. Rev. Lett. 88, 011603 (2002).
- D’Urso et al. (2005) B. D’Urso, R. Van Handel, B. Odom, D. Hanneke, and G. Gabrielse, Phys. Rev. Lett. 94, 113002 (2005).